Issue 
A&A
Volume 624, April 2019



Article Number  A117  
Number of page(s)  19  
Section  Astronomical instrumentation  
DOI  https://doi.org/10.1051/00046361/201834822  
Published online  22 April 2019 
The PLATO Solarlike Lightcurve Simulator
A tool to generate realistic stellar lightcurves with instrumental effects representative of the PLATO mission
^{1}
LESIA, Observatoire de Paris, Université PSL, CNRS, Sorbonne Université, Univ. Paris Diderot, Sorbonne Paris Cité, 5 Place Jules Janssen, 92195 Meudon, France
email: reza.samadi@obspm.fr
^{2}
Escola Politécnica – Departamento de Engenharia de Telecomunicações e Controle, Universidade de São Paulo, Av. Prof. Luciano Gualberto, 05508010 São Paulo, Brazil
^{3}
Institute of Optical Sensors Systems, German Aerospace Center (DLR), Rutherfordstrasse 2, 12489 Berlin, Germany
^{4}
Univ. Rennes, CNRS, IPR (Institut de Physique de Rennes) – UMR 6251, 35000 Rennes, France
^{5}
IRAP, Université de Toulouse, CNRS, CNES, UPS, Toulouse, France
^{6}
Institute of Planetary Research, German Aerospace Center, Rutherfordstrasse 2, 12489 Berlin, Germany
Received:
11
December
2018
Accepted:
25
February
2019
Context. ESA’s PLATO space mission, to be launched by the end of 2026, aims to detect and characterise Earthlike planets in their habitable zone using asteroseismology and the analysis of the transit events. The preparation of science objectives will require the implementation of hareandhound exercises relying on the massive generation of representative simulated lightcurves.
Aims. We developed a lightcurve simulator named the PLATO Solarlike Lightcurve Simulator (PSLS) in order to generate lightcurves representative of typical PLATO targets, that is showing simultaneously solarlike oscillations, stellar granulation, and magnetic activity. At the same time, PSLS also aims at mimicking in a realistic way the random noise and the systematic errors representative of the PLATO multitelescope concept.
Methods. To quantify the instrumental systematic errors, we performed a series of simulations at pixel level that include various relevant sources of perturbations expected for PLATO. From the simulated pixels, we extract the photometry as planned onboard and also simulate the quasiregular updates of the aperture masks during the observations. The simulated lightcurves are then corrected for instrumental effects using the instrument point spread functions reconstructed on the basis of a microscanning technique that will be operated during the inflight calibration phases of the mission. These corrected and simulated lightcurves are then fitted by a parametric model, which we incorporated in PSLS. Simulation of the oscillations and granulation signals rely on current stateoftheart stellar seismology.
Results. We show that the instrumental systematic errors dominate the signal only at frequencies below ∼20 μHz. The systematic errors level is found to mainly depend on stellar magnitude and on the detector charge transfer inefficiency. To illustrate how realistic our simulator is, we compared its predictions with observations made by Kepler on three typical targets and found a good qualitative agreement with the observations.
Conclusions. PSLS reproduces the main properties of expected PLATO lightcurves. Its speed of execution and its inclusion of relevant stellar signals as well as sources of noises representative of the PLATO cameras make it an indispensable tool for the scientific preparation of the PLATO mission.
Key words: asteroseismology / stars: oscillations / techniques: image processing / techniques: photometric / methods: numerical
© R. Samadi et al. 2019
Open Access article, published by EDP Sciences, under the terms of the Creative Commons Attribution License (http://creativecommons.org/licenses/by/4.0), which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.
1. Introduction
ESA’s PLATO^{1} space mission is expected to be launched by the end of 2026 with the goal of detecting and characterising Earthlike planets in the habitable zone of dwarf and subgiant stars of spectral types F to K (Rauer et al. 2014). The age and mass of planethosting stars will be determined by applying stellar seismic techniques to their solarlike oscillations (see e.g. Gizon et al. 2013; Van Eylen et al. 2014, 2018; Huber et al. 2019). The determination of these stellar parameters is a complex procedure since it relies on both the precise seismic analysis of the individual mode frequencies and the use of sophisticated stellar modelling techniques (see e.g. Lebreton et al. 2014a,b). To develop and test such complex procedures, realistic simulated lightcurves are needed. These simulated lightcurves are, for instance, typically used to conduct hareandhounds exercises^{2} involving various teams in charge of the seismic analysis and stellar modelling (see e.g. Reese et al. 2016, and references therein). They are also used to conduct massive Monte Carlo simulations that enable one to assess the performances of seismic analysis pipelines (e.g. de Assis Peralta et al. 2018, and reference therein). The simulated lightcurves must be sufficiently realistic to accurately account for the properties of the modes but also for the other sources of stellar noise such as the granulation noise and the instrumental random noise that – to a large extent – limit the precision of the age and mass determination. Similar hareandhounds exercises are also planned to be carried out to test the efficiency of planet detection and the accuracy of the derived transit parameters. Since planetary transits are expected to last several hours, their analysis is quite sensitive to the noises occurring at low frequencies (typically below a few ten of μHz). Finally, simulated lightcurves are also used to prepare the analysis of the PLATO lightcurves for a variety of other scientific objectives that are also relevant at low frequencies. We can, for instance, mention the characterisation of stellar granulation, the detection and characterisation of rotational modulations, among others. Accordingly, it is necessary to simulate in a realistic way the different sources of noise that dominate the signal at low frequencies. Among them, we have predominantly the stellar activity signal, but systematic instrumental errors may also intervene.
The CoRoT (Baglin et al. 2006b,a) and Kepler (Borucki et al. 2010) space missions, allowed us to carry out seismic studies of several thousands of pulsating redgiant stars (De Ridder et al. 2009; Kallinger et al. 2010; Stello et al. 2013) thus enabling important progress in our understanding of stellar interiors (see e.g. the reviews by Mosser & Miglio 2016; Hekker & ChristensenDalsgaard 2017). These observations opened up the path to what we now call ensemble asteroseismology (see e.g. Huber et al. 2011; Belkacem et al. 2013; Miglio et al. 2015) with various applications in the field of Galactic archaeology (Miglio et al. 2017). PLATO can potentially observe a large number of faint red giants. The number of targets that can be observed in addition to the targets of the core program is nevertheless limited to about 40 000 per pointing. An optimal choice of those targets can rely on the seismic performance tool of Mosser et al. (2019). On the other hand, the design and the development of seismic analysis pipelines that are able to process in an automatic way a large number of red giants require the generation of simulated lightcurves representative of such stars.
To our knowledge the lightcurve simulator developed by De Ridder et al. (2006) in the framework of the Eddington space project is the first code made available to the community that simulates solarlike oscillations together with the stellar granulation noise and the instrumental sources of noise. This simulator relies on a description of the modes and stellar granulation noise that predates CoRoT and Kepler space missions. However, our knowledge of solarlike oscillations and stellar granulation has greatly improved since that time. Very recently, Ball et al. (2018) proposed a lightcurve simulator dedicated to the TESS mission and that includes an uptodate description of solarlike oscillators and the granulation background. However, in this simulator, white noise is the only nonstellar source of noise; this means that systematic errors are not included. However, the latter, which are very specific to a given instrument and its space environment, are in general frequency dependent and can only be realistically quantified with simulations made at detector pixel level. Furthermore, the level of the white noise (random noise) also strongly depends on the implemented photometry method and the performance of the instrument. Finally, these simulators do not include planetary transits and are not suited for red giant stars. Indeed, red giants show the presence of numerous mixedmodes, and calculating mixedmode frequencies with pulsation codes requires a very high number of mesh points in the stellar models thus making the massive generation of corresponding simulated lightcurves numerically challenging.
The PLATO mission has some characteristics that make it very different from other spacebased mission based on highprecision photometry such as CoRoT, Kepler or TESS. Indeed, one of the main specificities of the mission is that it relies on a multitelescope concept. Among the 26 cameras that compose the instrument, two of them are named “fast” cameras and work at a 2.5 s cadence while the remaining 24 are named “normal” cameras and work at a 25 s cadence. The normal cameras are divided into four groups of six cameras, with large fields of view (∼1100 square degrees) that partially overlap. Each camera is composed of four Charge Couple Devices (CCD hereafter) which are read out at the cadence of 25 s with a timeshift of 6.25 s between each of them. Accordingly, the observations made for a given target by various groups of camera will be timeshifted thereby allowing us to perform superNyquist seismic analysis (Chaplin et al. 2014). Because of the large field of view and the longterm change of the pointing direction of each individual camera, star positions will slowly drift on the camera focal plane by up to 1.3 pixels during the 3month uninterrupted observation sequences. As a consequence, stars will slowly leave the aperture photometry (i.e. masks), leading obviously to a longterm decrease of their measured intensities. Furthermore, during the life of the mission, the instrument will be continuously exposed to radiation (mostly proton impacts). This will generate more and more traps in the CCD thus increasing the Charge Transfer Inefficiency (CTI hereafter, see e.g. Massey et al. 2014, and references therein) over time. Coupled with the longterm drift of the stellar positions, the CTI will induce an additional longterm variability of the photometric measurements.
To mitigate the flux variations induced by the instrument and the observational conditions, the aperture masks used onboard will be updated on a quasiregular basis. This will nevertheless leave residual flux variations of about several % over three months, which remain high w.r.t. the science requirements. The residual flux variations will fortunately be corrected a posteriori onground on the basis of the knowledge of the instrumental point spread function (PSF). Nevertheless, such a correction will leave systematic errors in the power spectrum that will rapidly increase with decreasing frequency. All of these instrumental systematic errors together with the stellar activity noise component can in principle impact the detection and characterisation of the planetary transits, limit the seismic analysis of very evolved red giant stars, and affect any science analysis of the signal at rather low frequencies.
The Plato Stellar Lightcurve Simulator^{3} (PSLS) aims at simulating stochasticallyexcited oscillations together with planetary transits, stellar signal (granulation, activity) and instrumental sources of noise that are representative of the PLATO cameras. The simulator allows us to simulate two different types of oscillation spectra: (i) oscillation spectra computed on the basis of the socalled Universal Pattern by Mosser et al. (2011) optionally including mixedmodes following the asymptotic gravity mode spacing (Mosser et al. 2012b) and (ii) oscillation spectra computed using a given set of theoretical frequencies precomputed with the ADIPLS pulsation code (ChristensenDalsgaard 2008).
The instrumental noise level is quantified by carrying out realistic simulations of the instrument at CCD pixel level using the Plato Image Simulator (PIS) for threemonth observation sequences. These simulations are performed for different stellar magnitudes, and for both the beginning of life (BOL^{4}) and end of life (EOL^{5}) observation conditions. The photometry is extracted from these simulated images in the same manner as planned onboard, that is using binary masks that minimise the noisetosignal ratio (NSR) of each target. The corresponding simulated lightcurves are then corrected using PSFs reconstructed on the basis of a microscanning technique, which will be operated inflight before each threemonth observation sequence and which we also simulate in the present work. This set of simulated lightcurves, corrected for the instrumental errors, then enables us to quantify the expected level of residual systematic errors. These simulations are then used to derive – as a function of the stellar magnitude – a parametric model of the residual errors in the time domain. This model is in turn implemented into PSLS.
Finally, the other components of the stellar signal (granulation signal, and planetary transits) are included in PSLS following prescriptions found in the literature.
2. General principle
The stochastic nature of the different phenomena (i.e. white noise, stellar granulation and stochasticallyexcited oscillations) are simulated following Anderson et al. (1990, see also Baudin et al. 2007). As detailed below, the properties of the simulated stellar signal are first modelled in the Fourier domain, we next add a random noise to simulate the stochastic nature of the signal, and finally we perform an inverse Fourier transform to come back into the time domain and derive the corresponding timeseries (i.e. lightcurve). We note that other authors (e.g. Chaplin et al. 1997; De Ridder et al. 2006) have proposed instead to work directly in the time domain. Although, rigorously equivalent, it is more convenient to describe the stellar signal in the Fourier domain since this is the common way signals (such as pulsation, granulation, and activity) are analysed in solarlike pulsators.
Let ℱ(ν) be the Fourier Transform (FT hereafter) of the simulated lightcurve 𝒮(t), and $\overline{\mathcal{P}}(\nu )$ the expectation of the Power Spectral Density (PSD) associated with the stellar signal (i.e. the PSD one would have after averaging over an infinite number of realisations). If the frequency bins of the PSD are uncorrelated, we can then show that
$$\begin{array}{c}\hfill \mathcal{F}(\nu )=\sqrt{\overline{\mathcal{P}}}\phantom{\rule{0.166667em}{0ex}}(u+i\phantom{\rule{0.166667em}{0ex}}v),\end{array}$$(1)
where u, and v are two uncorrelated Normal distributions of zero mean and unit variance, and i is the imaginary unit (i^{2} = −1). We finally compute the inverse Fourier Transform of $\widehat{F}(\nu )$ to derive the simulated lightcurve 𝒮(t) for a given realisation. We note that the PSD 𝒫(ν) associated with a given realisation verifies
$$\begin{array}{c}\hfill \mathcal{P}(\nu )={\mathcal{F}(\nu )}^{2}=\overline{\mathcal{P}}\phantom{\rule{0.166667em}{0ex}}({u}^{2}+{v}^{2}).\end{array}$$(2)
Our PSD is “singlesided”, which means that the integral of the PSD from ν = 0 (excluded) to the Nyquist frequency is equal to the variance of the timeseries.
Here, the expectation $\overline{\mathcal{P}}(\nu )$ is the sum of an activity component 𝒜(ν), the granulation background G(ν), and the oscillation spectrum O(ν), that is
$$\begin{array}{c}\hfill \overline{\mathcal{P}}(\nu )=\mathcal{A}(\nu )+G(\nu )+O(\nu ).\end{array}$$(3)
In accordance with our initial hypothesis, all these components are uncorrelated. However, some interferences can in principle exist between the various stellar signal components, such as the activity, the granulation and the oscillations. For instance there are some observational evidences about correlations between granulation (i.e. convection) and modes. Indeed, solar mode profiles slightly depart from symmetric Lorentzian profiles (Duvall et al. 1993). Likewise, pieces of evidence for similar asymmetries were recently found in stars observed by Kepler (Benomar et al. 2018). Helioseicmic data clearly show that this asymmetry is reversed between velocity and intensity measurements (e.g. Duvall et al. 1993; Nigam et al. 1998; Barban et al. 2004). This reversal is believed to be the signature of a correlation between convection and oscillations (Roxburgh & Vorontsov 1997; Nigam et al. 1998). However, the departures from symmetric Lorentzian profiles are small w.r.t. the mode linewidths. Hence, we consider this as an indication of a small level of correlation between convection (i.e. granulation) and oscillations. Finally, concerning possible interferences between activity and convection, to our knowledge there are no pieces of evidence. For these reasons, in this work, we decided to neglect the correlations between the stellar signal components.
Once the FT associated with the stellar signal is simulated on the basis of Eq. (1), we perform an inverse Fourier transform to come back into the time domain. This then provides the stellar signal as a function of time. However, in order to take into account the fact that each group of cameras are timeshifted by Δt = 6.25 s, we multiply Eq. (1) by the phase term e^{i2πΔt} prior to calculating its inverse Fourier Transform.
The instrumental signal component (i.e. the systematic errors plus the instrumental random sources of noise) is simulated in the time domain as explained in Sect. 4. Finally, once the instrumental signal is simulated, it is multiplied by the stellar signal and the planetary transit (which as the instrumental component is simulated in the time domain) to get finally the simulated lightcurve averaged over a given number of cameras. We describe in the following sections the way each simulated component is modelled.
3. Solarlike oscillations
In this section, we describe the modelling of the oscillation spectrum 𝒪(ν). It is the sum over the different normal modes
$$\begin{array}{c}\hfill \mathcal{O}(\nu )={\displaystyle \sum _{i}{\mathcal{L}}_{i}(\nu ),}\end{array}$$(4)
where each individual resolved mode of frequency ν_{i} is described by a Lorentzian profile
$$\begin{array}{c}\hfill {\mathcal{L}}_{i}(\nu )=\frac{{H}_{i}}{1+{(2(\nu {\nu}_{i})/{\mathrm{\Gamma}}_{i})}^{2}},\end{array}$$(5)
where H_{i} is the mode height, and Γ_{i} its linewidth. A mode is considered to be resolved when Γ_{i} > 2δf where δf is the frequency resolution (or equivalently the inverse of the observation duration). In contrast, for an unresolved mode the profile is given by (see, e.g. Berthomieu et al. 2001),
$$\begin{array}{c}\hfill {\mathcal{L}}_{i}(\nu )=\frac{\pi \phantom{\rule{0.166667em}{0ex}}{\mathrm{\Gamma}}_{i}\phantom{\rule{0.166667em}{0ex}}{H}_{i}}{2\delta \nu}\phantom{\rule{0.166667em}{0ex}}{\mathrm{sinc}}^{2}\left[\pi (\nu {\nu}_{i})\right],\end{array}$$(6)
where δν is the resolution of the spectrum.
To go further, one needs to determine the mode frequencies, heights, and linewidths. To do so, we consider two different methods for the frequencies. For mainsequence and subgiant stars, the method consists in computing a set of theoretical mode frequencies using the ADIPLS adiabatic pulsation code while for red giant stars we consider the method developed by Mosser et al. (2011), which relies on what is commonly known as the Universal Pattern. This distinction is motivated by the difficulty to compute red giant frequencies. Indeed, for evolved stars, a proper modelling of the normal frequencies requires an important number of grid points in the innermost layers. While still feasible, this makes the computation more demanding. We therefore adopt a more flexible and affordable method based on asymptotic considerations to ensure the possibility of using the simulator on a massive scale.
3.1. Mainsequence and subgiant stars
The oscillation spectrum is constructed using a set of theoretical eigenfrequencies computed using the ADIPLS code (ChristensenDalsgaard 2008). The program allows one to include uniform rotational splittings as specified by an input surface rotation period T_{rot} = 2π/Ω_{surf} where Ω_{surf} is the surface rotation rate. The set of frequencies included in the model are
$$\begin{array}{c}\hfill {\nu}_{n,\ell ,m}^{(0)}={\nu}_{n,\ell}+\frac{m}{{T}_{\mathrm{rot}}}\phantom{\rule{0.166667em}{0ex}}(\phantom{\rule{0.166667em}{0ex}}1{c}_{n,\ell}),\end{array}$$(7)
where n is the radial order, ℓ the angular (or harmonic) degree, m the azimuthal order, and c_{n, ℓ} the Ledoux constant (see, e.g. Unno et al. 1989) provided by ADIPLS. We consider all the modes from n = 1 up to the cutoff frequency, with angular degrees ranging from ℓ = 0 to 3 inclusive. Nearsurface effects are eventually added using the empirical correction proposed by Sonoi et al. (2015):
$$\begin{array}{c}\hfill {\nu}_{n,\ell ,m}={\nu}_{n,\ell ,m}^{(0)}+a\phantom{\rule{0.166667em}{0ex}}{\nu}_{\mathrm{max}}\phantom{\rule{0.166667em}{0ex}}(1\frac{1}{1+{({\nu}_{n,\ell ,m}^{(0)}/{\nu}_{\mathrm{max}})}^{b}}),\end{array}$$(8)
where a and b are two parameters, which are expressed in terms of T_{eff} and log g thanks to the scaling laws provided in Eqs. (10) and (11) of Sonoi et al. (2015), respectively.
The mode height of each given mode is computed according to
$$\begin{array}{c}\hfill {H}_{n,\ell ,m}=G({\nu}_{n,\ell ,m}\u037e\delta {\nu}_{\mathrm{env}})\phantom{\rule{0.277778em}{0ex}}{V}_{\ell}^{2}\phantom{\rule{0.166667em}{0ex}}{r}_{n,\ell ,m}^{2}(i)\phantom{\rule{0.166667em}{0ex}}{H}_{\mathrm{max}},\end{array}$$(9)
where V_{ℓ} is the mode visibility (V_{0} = 1, V_{1} = 1.5, V_{2} = 0.5, V_{3} = 0.05), H_{max} the mode height at the peak frequency, and r_{n, ℓ, m} the (relative) visibility of a mode of azimuthal order m within a multiplet for a given inclination angle i. The ratio r_{n, ℓ, m} is computed according to Dziembowski (1971, see also Gizon & Solanki 2003) and represents – at fixed values of n and ℓ – the ratio of the mode height for a given inclination angle i to the mode height at i = 0°. Finally, G is the Gaussian envelope defined as
$$\begin{array}{c}\hfill G({\nu}_{n,\ell ,m}\u037e\delta {\nu}_{\mathrm{env}})=exp\left[\frac{{({\nu}_{n,\ell ,m}{\nu}_{\mathrm{max}})}^{2}}{\delta {\nu}_{\mathrm{env}}^{2}/4ln2}\right],\end{array}$$(10)
where δν_{env} is the full width at half maximum, which is supposed to scale as (Mosser et al. 2012a):
$$\begin{array}{c}\hfill \delta {\nu}_{\mathrm{env}}=0.66\phantom{\rule{0.166667em}{0ex}}{\nu}_{\mathrm{max}}^{0.88}.\end{array}$$(11)
This scaling relation was established for red giants. The applications presented in Sect. 6 show that it provides rather good results for less evolved stars.
To compute Eq. (9), we now need to specify H_{max}. For a singleside PSD, the mode height is related to the mode linewidth as (see, e.g. Baudin et al. 2005)^{6}
$$\begin{array}{c}\hfill {H}_{\mathrm{max}}=\frac{2\phantom{\rule{0.166667em}{0ex}}{A}_{\mathrm{max}}^{2}}{\pi \phantom{\rule{0.166667em}{0ex}}{\mathrm{\Gamma}}_{\mathrm{max}}},\end{array}$$(12)
where A_{max} is the rms of the mode amplitude at the peak frequency. The latter is related to the bolometric amplitude A_{max, bol} using the correction proposed for Kepler’s spectral band by Ballot et al. (2011)
$$\begin{array}{c}\hfill {A}_{\mathrm{max}}={A}_{\mathrm{max},\mathrm{bol}}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{{T}_{\mathrm{eff}}}{5934\phantom{\rule{0.166667em}{0ex}}\mathrm{K}}\right)}^{0.8}.\end{array}$$(13)
We note that the CoRoT spectral band results in very similar corrections (see Michel et al. 2009). Finally, A_{max, bol} is derived from the scaling relations derived by Corsaro et al. (2013) and defined as
$$\begin{array}{cc}\hfill ln({A}_{\mathrm{max},\mathrm{bol}})=& ln({A}_{\mathrm{max},\mathrm{bol},\odot})+\phantom{\rule{0.166667em}{0ex}}(2s3t)ln({\nu}_{\mathrm{max}}/{\nu}_{\mathrm{max},\odot})\hfill \\ \hfill & +(4t4s)ln(\mathrm{\Delta}\nu /\mathrm{\Delta}{\nu}_{\odot})\hfill \\ \hfill & +(5s1.5tr+0.2)ln({T}_{\mathrm{eff}}/{T}_{\mathrm{eff},\odot})+ln(\beta ),\hfill \end{array}$$(14)
where A_{max, bol, ⊙} = 2.53 ppm (rms) is the maximum of the bolometric solar mode amplitude (Michel et al. 2009), and s, t, r and β are coefficients that depend on the star’s evolutionary status (see Tables 3 and 4 in Corsaro et al. 2013).
Finally, one needs to specify the mode linewidths. To this end, we note that the product of the mode linewidth and the mode inertia has a parabolic shape (Belkacem et al. 2011, see Fig. 2). Therefore,
$$\begin{array}{c}\hfill {\mathrm{\Gamma}}_{n,\ell ,m}={\mathrm{\Gamma}}_{\mathrm{max}}\phantom{\rule{0.166667em}{0ex}}\left(\frac{{I}_{\mathrm{max}}}{{I}_{n,\ell}}\right)\phantom{\rule{0.166667em}{0ex}}\gamma ({\nu}_{n,\ell ,m}),\end{array}$$(15)
where I_{n, ℓ} is the mode inertia, I_{max} is the mode inertia of the radial modes interpolated at ν = ν_{max}, Γ_{max} is the mode linewidth at ν = ν_{max} derived from two different scaling relations (see below), and the function γ(ν) models the frequency dependence of the product Γ_{n, ℓ, m}I_{n, ℓ} around ν_{max}. The latter is modelled empirically as follows
$$\begin{array}{c}\hfill \gamma (\nu )=1+A\phantom{\rule{0.166667em}{0ex}}(1G({\nu}_{n,\ell ,m}\u037e2\delta {\nu}_{\mathrm{env}})),\end{array}$$(16)
where G is the Gaussian function defined by Eq. (10), A is a constant, and δν_{env} is given by the scaling relation of Eq. (11). With A = 2 for ν ≥ ν_{max} and A = 6 for ν < ν_{max}, Eq. (16) reproduces rather well the variation with frequency of the solar mode linewidths. Given the objectives targeted by the simulator, we assume that this empirical description is sufficiently representative for other stars. An alternative approach would have been to use the relation describing the frequency dependence derived from Kepler observations by Appourchaux et al. (2014, see its corrigendum in Appourchaux et al. (2016)). However, this relation was established for a limited number of targets and hence in limited ranges in effective temperatures, surface gravities and surface metal abundances. Therefore, to avoid extrapolations we prefer to adopt Eq. (15). In addition, the relation inferred by Appourchaux et al. (2014) was established on limited frequency intervals. Since the mode linewidths scale as the inverse of the mode inertia (Eq. (15)), this scaling relation allows us instead to derive the frequency dependence of Γ_{n, ℓ, m} for the whole acoustic spectrum of a given star.
Finally, the mode linewidth at the peak frequency, Γ_{max}, is determined on the basis of the scaling relation derived by Appourchaux et al. (2012) from mainsequence Kepler targets, that is
$$\begin{array}{c}\hfill {\mathrm{\Gamma}}_{\mathrm{max}}={\mathrm{\Gamma}}_{\mathrm{max},0}+\beta \phantom{\rule{0.166667em}{0ex}}{\left(\frac{{T}_{\mathrm{eff}}}{{T}_{\mathrm{eff},\odot}}\right)}^{s},\end{array}$$(17)
where Γ_{max, 0} = 0.20 μHz, β = 0.97, and s = 13.0.
3.2. Redgiant stars
Each mode frequency ν_{n, ℓ} is computed according to the Universal Pattern proposed by Mosser et al. (2011)
$$\begin{array}{cc}\hfill {\nu}_{n,\ell ,m}=& \phantom{\rule{3.33333pt}{0ex}}n+\frac{\ell}{2}+\epsilon (\mathrm{\Delta}\nu ){d}_{0\ell}(\mathrm{\Delta}\nu )+\frac{{\alpha}_{\ell}}{2}{(n\frac{{\nu}_{\mathrm{max}}}{\mathrm{\Delta}\nu})}^{2}\mathrm{\Delta}\nu \hfill \\ \hfill & +m\phantom{\rule{0.166667em}{0ex}}\delta {\nu}_{\mathrm{rot}}\phantom{\rule{0.166667em}{0ex}}+{\delta}_{n,\ell},\hfill \end{array}$$(18)
where ε is an offset, d_{0ℓ}, the small separation, α_{ℓ} the curvature, Δν the large separation, δν_{rot} the rotational mode splitting (included only for dipolar modes, as will be explained later on), and finally δ_{n, ℓ} a term that accounts for a possible coupling with the gravity modes, which results in the deviation of the mode frequency from its uncoupled solution (“pure” acoustic mode) and gives the mode its mixedmode nature. For a dipole mode, δ_{n, ℓ} is computed according to the asymptotic gravitymode spacing (Mosser et al. 2012b)
$$\begin{array}{c}\hfill {\delta}_{n,\ell}=\frac{\mathrm{\Delta}\nu}{\pi}arctan[qtan\pi (\frac{1}{\mathrm{\Delta}{\mathrm{\Pi}}_{1}{\nu}_{n,\ell}}{\u03f5}_{g})],\end{array}$$(19)
where q is the coupling coefficient, ΔΠ_{1} the asymptotic period spacing of the (pure) dipole g modes, and ϵ_{g} an offset fixed to the value 0.25, which is representative for most red giants (Mosser et al. 2017). For radial modes, one obviously has δ_{n, 0} = 0, while for all modes with angular degree ℓ ≥ 2 we neglect the deviation and assume δ_{n, ℓ} = 0.
The mode height of each given mode (n, ℓ, m) is given by
$$\begin{array}{c}\hfill {H}_{n,\ell}=G({\nu}_{n,\ell})\phantom{\rule{0.166667em}{0ex}}{V}_{\ell}^{2}\phantom{\rule{0.166667em}{0ex}}{H}_{\mathrm{max}},\end{array}$$(20)
where G(ν_{n, ℓ}) is given by Eq. (15), V_{ℓ}, is the mode visibility determined from Mosser et al. (2012a) and H_{max} is the maximum of the mode heights derived from the scaling relation established by de Assis Peralta et al. (2018), that is
$$\begin{array}{c}\hfill {H}_{\mathrm{max}}=2.01\times {10}^{7}\phantom{\rule{0.166667em}{0ex}}{\nu}_{\mathrm{max}}^{1.9}.\end{array}$$(21)
Concerning the mode linewidths Γ_{n, ℓ}, they are assumed to be constant with frequency. This assumption is motivated by the fact that modes are observed in a relatively small frequency range compared to mainsequence and subgiant stars. This constant value is determined from the theoretical scaling relation of Vrard et al. (2018), which depends on the effective temperature, T_{eff}, and stellar mass as follows
$$\begin{array}{c}\hfill {\mathrm{\Gamma}}_{\mathrm{max}}={\mathrm{\Gamma}}_{\mathrm{max},0}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{{T}_{\mathrm{eff}}}{4800\phantom{\rule{0.166667em}{0ex}}\mathrm{K}}\right)}^{{\alpha}_{T}},\end{array}$$(22)
where Γ_{max, 0} = 0.1 μHz and α_{T} is a coefficient which depends on the stellar mass range (see Vrard et al. 2018). The dipolar mixed modes have, however, much smaller linewidths than their associated “pure” acoustic modes. This is mainly because their inertia is much larger as a consequence of the fact they behave as gravity modes in the inner layers. Indeed, the mode linewidth scales as the inverse of the mode inertia (see, e.g., Belkacem & Samadi 2013). Let ${I}_{n,\ell}^{m}$ (resp. ${\mathrm{\Gamma}}_{n,\ell}^{(m)}$) be the mode inertia (resp. mode linewidth) of a dipolar mixedmode and ${I}_{n,\ell}^{0}$ (resp. ${\mathrm{\Gamma}}_{n,\ell}^{(0)}$) that of a “pure” acoustic mode of the same radial order. We then have
$$\begin{array}{c}\hfill {\mathrm{\Gamma}}_{n,\ell}^{(m)}={\mathrm{\Gamma}}_{n,\ell}^{(0)}\phantom{\rule{0.166667em}{0ex}}\left(\frac{{I}_{n,\ell}^{0}}{{I}_{n,\ell}^{m}}\right),\end{array}$$(23)
where according to our previous assumption ${\mathrm{\Gamma}}_{n,\ell}^{(0)}={\mathrm{\Gamma}}_{\mathrm{max}}$ for any couple (n, ℓ). In Eq. (23), it is assumed that radiative damping in the radiative interior of red giants is negligible. The validity of this assumption has been thoroughly investigated by Grosjean et al. (2014).
To go further, we use the following relation from Goupil et al. (2013):
$$\begin{array}{c}\hfill \frac{{I}_{n,\ell}^{0}}{{I}_{n,\ell}^{m}}\simeq 1\frac{{I}_{\mathrm{core}}}{I}=1\zeta ,\end{array}$$(24)
where I_{core} is the contribution of the core to the mode inertia, and ζ is calculated according to Eq. (4) in Gehan et al. (2018). Finally, the rotational splitting for dipolar modes (the term δν_{rot} in Eq. (18)) is computed on the basis of Eq. (22) in Goupil et al. (2013) by neglecting the surface rotation (see e.g. Mosser et al. 2015; Gehan et al. 2018). Accordingly, we have
$$\begin{array}{c}\hfill \delta {\nu}_{\mathrm{rot}}=\frac{\zeta}{2}\phantom{\rule{0.166667em}{0ex}}\left(\frac{{\mathrm{\Omega}}_{\mathrm{core}}}{2\pi}\right),\end{array}$$(25)
where Ω_{core} is the core rotation rate (in rad/s).
The oscillation spectrum is then constructed by summing a Lorentzian profile for each mode. We include modes with radial orders ranging from n = 1 up to n = integer (ν_{c}/Δν), where ν_{c} is the cutofffrequency (see Eq. (28)), and with angular degrees from ℓ = 0 to ℓ = 3.
The simulator requires three main input parameters, ν_{max}, T_{eff} and Δν, from which all the other parameters are established using scaling relations, except ΔΠ_{1} and q which can be provided as optional inputs (otherwise no mixed modes are included). In case Δν is not provided, it is computed according to the scaling relation (Mosser et al. 2013)
$$\begin{array}{c}\hfill \mathrm{\Delta}\nu =0.274\phantom{\rule{0.166667em}{0ex}}{\nu}_{\mathrm{max}}^{0.757}.\end{array}$$(26)
The stellar mass used for the granulation scaling relations is determined by combining the scaling relation for ν_{max} and Δν (see Belkacem 2012; Mosser et al. 2010, and references therein):
$$\begin{array}{c}\hfill m={M}_{\odot}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{{\nu}_{\mathrm{max}}}{{\nu}_{\mathrm{max},\odot}}\right)}^{3}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{\mathrm{\Delta}\nu}{\mathrm{\Delta}{\nu}_{\odot}}\right)}^{4}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{{T}_{\mathrm{eff}}}{{T}_{\mathrm{eff},\odot}}\right)}^{3/2}.\end{array}$$(27)
Finally, the cutoff frequency ν_{c} is derived from the following scaling relation:
$$\begin{array}{c}\hfill {\nu}_{\mathrm{c}}={\nu}_{\mathrm{c},\odot}\phantom{\rule{0.166667em}{0ex}}\frac{g}{{g}_{\odot}}\phantom{\rule{0.166667em}{0ex}}\sqrt{\frac{{T}_{\mathrm{eff},\odot}}{{T}_{\mathrm{eff}}}},\end{array}$$(28)
where ν_{c, ⊙} = 5300 μHz.
4. Instrumental errors
Our objective here is to quantify the instrumental sources of error, namely the systematic error and the random noise, and to implement them into PSLS. For the former, a set of simulations at CCD pixel level is carried out while for the random noise we rely on the work made by Marchiori et al. (2019) as explained in Sect. 4.4.
4.1. The Plato instrument
PLATO is composed of 24 cameras (named normal cameras) working at a cadence of 25 s and two cameras (named fast cameras) working at a cadence of 2.5 s. Each group of cameras is composed of six normal cameras that see half of the full field of view (2200 square degrees). The fast cameras point towards the centre of the field of view, and provide the platform with pointing errors for the Attitude Control System. Four Charge Coupled Devices (CCDs) are mounted on the focal plane of each camera. The pixels have a size of 18 μm and their projected size in the sky represents approximately 15 arcsec.
Every three months, the platform is rotated by 90° in order to maintain the solar panel in the direction of the Sun. Due to the thermal distortion of the platform, changes in the pointing direction of each individual camera are expected during the uninterrupted threemonth observation sequences. These variations will lead to longterm star drifts on the focal plane of up to 0.8 pixels in three months. Furthermore, because of the large field of view, the kinematic aberration of light will induce drifts of the stellar positions of up to 0.5 pixels in three months at the edge of the field of view. Both effects add together and result in drifts of up to 1.3 pixels in three months (in the worst case, at the edge of field of view).
4.2. The Plato Image Simulator
To quantify the instrumental systematic errors, we generate timeseries of small imagettes with the Plato Image Simulator (PIS). This simulator, developed at the LESIAObservatoire de Paris since the early phases of the PLATO project, has very similar capabilities as the PLATOSim code (MarcosArenal et al. 2014). PIS can simulate imagettes representative of PLATO CCDs. It includes various sources of perturbations, such as shotnoise (photon noise), readout noise, background signal, satellite jitter, longterm drift, smearing, digital saturation, pixel response nonuniformity (PRNU), intra pixel response nonuniformity (IPRNU), charge diffusion, and charge transfer inefficiency (CTI). Since our goal is to quantify systematic errors, we turned off all random sources of noise in our instrumental simulations, except in the calculation of the NSR, see Sect. 4.4; these are the shotnoise, the readoutnoise, and the satellite jitter. CTI is simulated following Short et al. (2013) and activated for endoflife (EOL) simulations only. Charge diffusion within the CCD pixels is not activated because we still lack a reliable estimate of its amplitude (see the discussion in Sect. 7).
To take into account the impact of longterm drifts of the stellar positions, simulations are generated over 90 days and include a linear drift of 1.3 pixels in three months. To be more realistic, the instrumental point spread functions (PSF) used during these simulations include optical manufacturing errors and integration and alignment tolerances to the nominal design for the nominal focus position. These input PSFs do not include effects due to the detector or the spacecraft (such as the satellite jitter). However, most of them (like PRNU, IPRNU, CTI, and satellite jitter) are in any case included in PIS.
4.3. Simulation parameters and data sets
The flux of each simulated star behaves differently according to their magnitude, position over the CCD, and even position within a pixel (hereafter named intrapixel position). In order to cover the largest combination of these factors, we use PIS to run 630 artificial star simulations using a combination of:

9 stellar magnitudes (from V = 9 to V = 13 with a step of 0.5),

14 focal plane positions over the focal plan (from 1.41^{°} to 18.08^{°} from the optical centre),

5 intrapixel positions for each of the 14 focal plane positions.
The simulations are carried out using the parameters relevant for BOL and EOL conditions. Thus, regarding EOL simulations, the CTI is enabled and the mean optical transmission is assumed to be lower than the BOL one. The CTI model used by PIS requires specifying the number of trap species and their characteristics in terms of density, release time, and cross sections. To this end, Prod’homme et al. (2016) have studied CTI on a representative PLATO CCD that has been irradiated on purpose. This study allowed the authors to identify four trap species and to calibrate their corresponding parameters. We used the parameters derived by Prod’homme et al. (2016). However, the trap densities are rescaled so that the level of CTI reaches the mission specifications at the EOL. The adopted values of the simulation parameters are reported in Table 1.
Simulation parameters used with the PIS code.
4.4. Photometry extraction
Of the ∼120 000 targets observed by each camera during a given pointing, about 14 000 of them will have their 6 × 6 imagettes downloaded onground at a cadence of 25 s. For these targets, the photometry will be extracted onground on the basis of more sophisticated methods, which are not yet fully established. The photometry of the remaining targets will necessarily have to be performed onboard.
Before computing the photometry, we start with a basic preprocessing of the imagettes aiming to subtract the electronic offset and the background, convert ADU to electrons using the gain, and finally subtract the smearing for each column of the imagette.
Photometry extraction is performed onboard by integrating the stellar flux over a collection of pixels called the aperture or the mask. Different strategies for determining the most adequate aperture shape have been the subject of a detailed study (Marchiori et al. 2019), leading to the adoption of binary masks as the best compromise between NSR and stellar contamination ratio. For a given target, its associated binary mask is defined as the subset of the imagette pixels giving the minimum noisetosignal ratio. It is computed through the following scheme

Arrange all pixels n from the target imagette in increasing order of noisetosignal ratio NSR_{n}
$$\begin{array}{c}\hfill {\mathrm{NSR}}_{n}=\frac{\sqrt{{\sigma}_{{F}_{{T}_{n}}}^{2}+\sum _{k=1}^{{N}_{C}}{\sigma}_{{F}_{{C}_{n,k}}}^{2}+{\sigma}_{{B}_{n}}^{2}+{\sigma}_{{D}_{n}}^{2}+{\sigma}_{{Q}_{n}}^{2}}}{{F}_{{T}_{n}}}.\end{array}$$(29)

Compute the aggregate noisetosignal NSR_{agg}(m), as a function of the increasing number of pixels m = {1, 2, 3, …, 36}, stacking them conforming to the arrangement in the previous step and starting with the pixel owning the smallest NSR_{n}
$$\begin{array}{c}\hfill {\mathrm{NSR}}_{\mathrm{agg}}(m)=\frac{\sqrt{{\displaystyle \sum _{n=1}^{m}({\sigma}_{{F}_{{T}_{n}}}^{2}+{\displaystyle \sum _{k=1}^{{N}_{C}}{\sigma}_{{F}_{{C}_{n,k}}}^{2}+{\sigma}_{{B}_{n}}^{2}+{\sigma}_{{D}_{n}}^{2}+{\sigma}_{{Q}_{n}}^{2}})}}}{\sum _{n=1}^{m}{F}_{{T}_{n}}}.\end{array}$$(30)

Define as the aperture the collection of pixels m providing minimum NSR_{agg}(m).
In Eqs. (29) and (30), F_{T} is the target star’s mean flux, σ_{FT} the target star’s photon noise, F_{C} the contaminant star’s mean flux, σ_{FC} the contaminant star’s photon noise, σ_{B} the background noise from the zodiacal light, σ_{D} the overall detector noise (including readout, smearing and dark current noises) and σ_{Q} the quantization noise. Figure 1 illustrates how the NSR typically evolves as the binary mask gets larger following the above scheme. We note that the noise due to satellite jitter is not included in the definition of the mask (Eq. (30)). Including the contribution of the jitter noise in the definition of the mask is not trivial because its contribution depends on the final shape of the mask (see e.g. Fialho & Auvergne 2006). Nevertheless, it turns out that for PLATO, the jitter noise is small enough that its does not play a role in the mask shape, the dominant sources of noise being the photon noise for brighter stars and the background and readout noise for fainter stars. Accordingly, once the mask is defined, we include the jitter a posteriori in the estimation of the NSR.
Fig. 1. Typical NSR evolution curve as a function of increasing aperture size. Pixels with the smallest noisetosignal ratio are addedup successively. The collection of pixels giving the lowest aggregate NSR defines the binary mask for a given target. 
The NSR was estimated for a large sample of targets (so far about 50 000) with magnitudes ranging from 9 to 13. The targets and their associated contaminant stars were extracted from the Gaia DR2 catalogue (Gaia Collaboration 2018). In total about 3.5 million contaminant stars with magnitudes up to G = 21 were included in the calculation.
The calculation of the NSR takes into account the various sources of noise described above and also the fact that the shape of the PSF varies across the field of view. The latest version of the instrument parameters were also considered (details will be given in Marchiori et al. 2019). Typical values of the NSR are given in Table 2 for a single camera and 24 cameras as a function of the PLATO magnitude, P, which is defined in Marchiori et al. (2019) and is by definition directly connected to the flux collected by a PLATO camera. For comparison with the mission specifications (Rauer et al. 2014), we also provide the V magnitude, which is defined here as the flux collected in the Johnson V filter for a reference PLATO target of T_{eff} = 6000 K.
NSR as a function of target V and P magnitudes.
For comparison, we also reported the values of the NSR in the photon noise limit (i.e. when there is only the photon noise due to the target). The relative contribution of random noises that add (quadratically) to the target photon noise increase with increasing stellar magnitude from 20% at magnitude V = 8.5 up to 65% at V = 13.
Unless the NSR value is imposed by the user, the latter is obtained by interpolating the values given in Table 2 for a given V magnitude.
4.5. Mask update
An example of a lightcurve obtained with a fixed optimal binary mask is shown in Fig. 2 (top) for a target of magnitude V=11. Because of the longterm drift of the star and the fact that the mask is maintained at the same position during the threemonth observation sequence, we observe a significant longterm decrease of the stellar flux. In this worst case scenario (a displacement of 1.3 pixels in three months), the flux decreases by about 15%, which subsequently results in an increase of the NSR by about 8% (see Fig. 2 – bottom). The NSR increase obviously has an impact on the science objectives of the mission, in particular on the planet detection rate. Indeed, a higher NSR at a given magnitude reduces the number of targets for which the NSR is lower than a given threshold, which subsequently lowers the number of detected planets.
Fig. 2. Top: examples of lightcurves generated from a simulated timeseries of CCD imagettes. The red curve corresponds to the lightcurve generated with a fixed binary mask while the blue one includes a series of mask updates. The dotted vertical lines identify the times at which the masks were updated. Bottom: corresponding time variations of the NSR. 
To mitigate the impact of the longterm drift and to maintain the NSR as low as possible, the proposed solution is to update the mask when required during the threemonth observation sequences. An example is shown in Fig. 2 (top). We see in this example that the peaktopeak variation of the flux is maintained within 4% (top panel) while the variation of the NSR is maintained within less than 2% (lower panel). Therefore, the mask updates always guarantee that one reaches the best possible NSR. Furthermore, it is also found that the mask updates partially mitigate the impact of CTI.
It is interesting to note that some mask updates simultaneously reduce the flux and the NSR. This is because the NSR does not scale linearly with the flux. Indeed, due to the presence of the readout noise and the complex shape of the PSF, two masks collecting the same amount of flux can have a different number of pixels and hence different contributions of the readout noise.
Obviously, each mask update will introduce a discontinuity at a well known instant, which for a given target will be different from one camera to another. For instance in the example shown in Fig. 2, the binary mask has been updated seven times. It is however possible to reduce the number of updates by increasing the threshold above which a variation of the NSR since the last update must trigger a mask update. Furthermore, as explained below, the discontinuities induced by each update as well as the longterm flux variations induced by the longterm drifts can be efficiently corrected a posteriori onground.
4.6. Lightcurve correction
Knowing the PSF at any position across the field of view and the time displacements of a given target, it is possible – given its associated aperture mask – to reconstruct a synthetic lightcurve, which exactly mimics the time variation of the star flux induced only by the longterm drift over the CCD plane as well as the discontinuity induced by each mask update. The lightcurve correction then consists in building such a synthetic lightcurve assuming that the star has an unit intensity, then dividing the real stellar lightcurve by the synthetic one. The quality of this correction intrinsically depends on our ability to construct the PSF and to derive the stellar displacement in time. As explained in detail in Sect. 4.7, the stellar PSFs will be reconstructed during the inflight calibration phases on the basis of a microscanning sequence coupled with a dedicated inversion method.
Concerning the stellar displacements, the fast camera will provide information about the shortterm variations of the satellite attitude (i.e. satellite jitter) with a high cadence (2.5 s) and a sufficient accuracy. This information will then be directly translated in terms of the shortterm variations of the attitude of each given normal camera. Concerning the longterm displacements, centroids of a larger set of targets will be measured using the imagettes registered onboard at a cadence of 25 s. These centroids will be used to derive the attitude of each camera at any instant. The combination of the two sets of information will finally provide both the shortterm (i.e. jitter) and longterm timedisplacements of any target.
Finally, it has been established that the PRNU is a limiting factor for this correction. However, prior to the launch, the PRNU will be measured with an accuracy better than 0.1% (rms), which is sufficient to leave a negligible level of residual error in the corrected lightcurves (Samadi 2015).
Two examples of corrected (individual) lightcurves are displayed in Fig. 3 for a V = 11 PLATO target. The upper lightcurve corresponds to BOL observation conditions while the lower one to the EOL. It is clearly seen that the residual flux variations are larger at the EOL: for that particular target the peaktopeak flux variations is as high as about 1% at the EOL while it remains within about 0.2% at the BOL. This is explained by the combined effect of the CTI and the star drift. Indeed, as the star moves, the energy distribution in the different pixels vary with time and so does the CTI. This effect is named differential CTI.
Fig. 3. Examples of singlecamera lightcurves generated from a simulated timeseries of CCD imagettes and after correcting it for the longterm drift of the stellar position as explained in Sect. 4.6. We represent the relative flux variation in %. The red (reps. blue) curve corresponds to EOL (resp. BOL) observation conditions. The dotted vertical lines identify the times at which the masks were updated. 
The small discontinuities seen in the lightcurve occur each times the mask has been updated. These discontinuities are of the order 500 ppm. Hence, they remain small compared to the photon noise, which is about 2000 ppm for this target and for a single camera. It is also worth noting that for a given target observed with several cameras the instants at which the mask updates occur are different between the different cameras. Accordingly, the systematic errors induced by these updates are uncorrelated between the cameras and accordingly, their impacts on the final lightcurves (obtained after averaging several individual lightcurves) will be significantly reduced (see Sect. 4.10).
4.7. Point spread function reconstruction
One of the challenges with the PLATO mission is the relatively large size of the camera pixels (approximately 15 arcsec as projected on the fieldofview) compared to the typical size of the point spread functions (PSFs)^{7}. Accordingly, raw camera pictures do not provide a sufficient resolution of the PSFs, thus requiring the use of a specific strategy in order to obtain the PSFs with a subpixel resolution. In the PLATO mission, the adopted strategy is similar to the one applied to Kepler observations (Bryson et al. 2010): a microscanning sessions in which a series of imagettes with subpixel displacements are obtained (Green 2011). High resolution PSFs will then be reconstructed by inverting the imagettes along with a precise knowledge of the displacements. Such PSFs will be obtained for a number of reference stars across the fieldofview. The PSF at any position will then be obtained via interpolation using the reference PSFs. The resultant PSFs will subsequently be used in correcting the lightcurves sent down by PLATO as explained in Sect. 4.6.
4.7.1. Microscanning sessions
The microscanning sessions will typically last for 3 h and lead to a series of 430 imagettes composed of 6 × 6 pixels encompassing the target stars. The telescope will be pointing in a slightly different direction for each imagette resulting in small subpixel displacements of the target stars. A continuous microscanning strategy has been opted for, that is the position will be changing continuously throughout the manoeuvre rather than stopping for each imagette and then starting again (Ouazzani et al. 2015). The displacements do not need to fulfil stringent criteria in order to be suitable for the inversions, but only to form a path which roughly covers a pixel uniformly (for more details see Reese 2018a). Accordingly, this path has primarily been determined based on technological constraints. However, a precise knowledge of the displacements is essential for carrying out successful inversions. Various tests have shown that the fast cameras are able to obtain this information from the centreofbrightness of reference stars.
The displacements will form an Archimedean spiral such that the distance, D, between consecutive images is approximately constant, and the distance between consecutive spiral arms is $D\sqrt{3}/2$, thus leading to the formation of nearequilateral triangles depending on the relative positions of imagettes on consecutive arms. Furthermore, the spiral needs to approximately cover 1 pixel. The combination of these constraints leads to a spiral like the one illustrated in Fig. 4.
Fig. 4. Archimedean spiral used for the microscanning strategy. The dotted lines correspond to the CCD pixel borders. 
4.7.2. PSF inversions
In order to carry out the inversions, it is necessary to discretise the PSF by expressing it as a sum of basis functions:
$$\begin{array}{c}\hfill f(x,y)={\displaystyle \sum _{i}{a}_{i}{\varphi}_{i}(x,y),}\end{array}$$(31)
where the a_{i} are unknown coefficients which will be determined via the inversion, and the ϕ_{i} basis functions. Typical choices of basis functions include subpixel indicator functions, or Cartesian products of cubic Bsplines. The typical resolution used for these basis functions is 1/20th of a pixel (along both the x and y directions), given the number of imagettes from the microscanning session. This high resolution representation of the PSF then needs to be integrated over the pixels of the imagettes. Equating the resultant integrals with the observed intensities in these pixels leads to the following equation
$$\begin{array}{c}\hfill A\mathit{x}=\mathit{b},\end{array}$$(32)
where b is a vector composed of the observed intensities from the imagettes, x a vector composed of the coefficients a_{i}, and A the discretisation matrix. The inverse problem is then to extract the high resolution PSF, x, knowing A and b. Given that the number of unknowns does not necessarily equal the number of observables, this problem needs to be inverted in a leastsquares sense. Furthermore, some form of regularisation needs to be included in order to obtain wellbehaved solutions. Finally, the resultant highresolution PSF needs to remain positive. A sufficient (though not necessary) condition for this is to impose that the coefficients a_{i} are positive, provided the basis functions ϕ_{i} remain positive.
Two inversion techniques have been used for solving Eq. (32). The first is an iterative approach called the Multiplicative Algebraic Reconstruction Technique (MART; Censor 1981; Green & Wyatt 2006), which starts from a positive smooth solution and iteratively corrects it using one constraint at a time. Given that the corrections are applied in a multiplicative manner, the solution remains positive. The number of iterations is then used to control the degree of regularisation. The second approach is a regularised leastsquares approach with a positivity constraint on the coefficients. The regularisation term consists of a 2D Laplacian multiplied by a weight function which leads to a higher amount of regularisation in the wings of the PSF. Accordingly, cubic Bsplines are used with this approach given that these are continuously twicedifferentiable. This term is then multiplied by a tunable regularisation parameter. As shown in Reese (2018b), this second approach leads to better results in most cases (see an example in Fig. 5 bottom panel) and is accordingly the preferred approach.
Fig. 5. Top: original PSF. Bottom: PSF obtained by inversion on the basis of the microscanning technique (see Sect. 4.7). The dotted lines correspond to the CCD pixel borders. 
4.8. Analysis of systematic errors in terms of PSD
We compute the PSD associated with each corrected lightcurve, both for the BOL and EOL data sets. Two examples are shown in Fig. 6 at the BOL and the EOL for a star located at a given position in the field of view and at the subpixel position P_{0} (pixel corner). These PSDs are compared with the PLATO requirements in terms of allowed systematic errors at V = 11. At the EOL, the requirements are marginally exceeded in the frequency range [10 μHz–100 μHz]. This is a consequence of the presence of CTI. We stress that we expect to be able to correct for the CTI. However, this correction is not yet fully modelled and hence cannot yet be reliably quantified. Accordingly, the predictions for the EOL have to be considered conservative at this moment.
Fig. 6. PSD of the residual lightcurve obtained with two threemonth PIS simulations, one representative of the BOL (cyan) and the second of the EOL (pink). The results shown here correspond to a star of magnitude 11. The solid coloured line represents the fitted model defined in Eq. (33). The solid black line represents the PLATO requirements in terms of systematic errors translated for a single camera by assuming that they are uncorrelated between the different camera (see text). 
We find that the PSD of the residual lightcurve can satisfactory be fitted with a function of the form:
$$\begin{array}{c}\hfill \mathcal{I}(\nu )={H}_{1}\phantom{\rule{0.166667em}{0ex}}{\left(\frac{{\nu}_{1}}{\nu}\right)}^{{\alpha}_{1}}+\frac{{H}_{2}}{1+{\left(2\pi {\tau}_{2}\nu \right)}^{{\alpha}_{2}}},\end{array}$$(33)
where H_{1}, α_{1}, H_{2}, τ_{2} and α_{2} are the fitted parameters, and ν_{1} = 1/T_{1} with T_{1} = 90 days (three months). For convenience, we further define σ^{2} as the variance of the residual lightcurve, which is also the integral ℐ(ν). The quantity σ corresponds to the amplitude of the systematic errors and is related to the other parameters according to the relation
$$\begin{array}{c}\hfill {\sigma}^{2}=\frac{{H}_{1}{\nu}_{1}}{{\alpha}_{1}1}+\frac{{H}_{2}\phantom{\rule{0.166667em}{0ex}}}{2\phantom{\rule{0.166667em}{0ex}}{\tau}_{2}\phantom{\rule{0.166667em}{0ex}}sin(\pi /{\alpha}_{2})}.\end{array}$$(34)
We fit each residual lightcurve with the function given by Eq. (33). Depending on the parameters, we find that the parameter values significantly vary with the subpixel positions. This is not surprising since about 90% of the star’s intensity is concentrated in a square of 2.2 × 2.2 pixels (an example of such a PSF is displayed in Fig. 5). As a result, a change of the subpixel position of the star’s centroid induces important changes in the charge distribution. In contrast, at fixed subpixel positions, changes of the parameter values with the stellar field of view are in general weaker. Finally, the parameters controlling the amplitudes of the systematic errors (namely H_{1} and H_{2}) are found to strongly vary with the stellar magnitude.
Figure 7 highlights the impact of the star magnitude. Indeed, the 90th percentile of the quantity σ [in ppm] is displayed as a function of the star magnitude, both for BOL and EOL conditions. In general, the residual systematic errors increase with increasing star magnitude. As expected, the systematic errors at EOL are systematically much higher than at BOL by about a factor ten at magnitude 8.5 and down to about a factor four at magnitude 13. However, they hardly exceed 0.5% (rms) in the magnitude range considered here.
Fig. 7. Amplitude of the systematic errors (σ) as a function of the stellar magnitude. This quantity is computed according to Eq. (34). At each stellar magnitude, only the 90th percentile is displayed. 
4.9. Modelling the systematic errors in the time domain
The systematic errors were analysed in the previous section in terms of PSD because this is the most convenient way to compare directly with the mission requirements in terms of allowed systematic errors. Indeed, the latter are specified in terms of the PSD. However, modelling the systematic errors this way has the obvious consequence of destroying the phase of the instrumental or operational perturbations (e.g. the discontinuities induced by the mask updates or other effects). While this is in principle not a problem when the stellar signal is analysed in terms of the PSD (e.g. as this is typically done for the granulation or the solarlike oscillations), this can be misleading for the analysis taking place in the time domain, as for instance the detection and the characterization of planetary transits. To overcome this, we decide instead to model the systematic errors in the time domain.
Due to the quasiregular mask updates, the residual lightcurve is piecewise continuous (each piece corresponding to an interval of time where the aperture mask is unchanged). We find that each piece can be well reproduced by a third order polynomial. Accordingly, we decompose each generated instrument lightcurve as follows
$$\begin{array}{c}\hfill s(t)=\overline{s}\phantom{\rule{0.166667em}{0ex}}{\displaystyle \sum _{i=1}^{N}\mathrm{\Pi}\left(\frac{t{t}_{i}}{{d}_{i}}\right)\phantom{\rule{0.166667em}{0ex}}(1+{p}_{3,i}+{p}_{2,i}x+{p}_{1,i}{x}^{2}+{p}_{0,i}{x}^{3}),}\end{array}$$(35)
where $\overline{s}$ is the lightcurve timeaverage, N the number of masks used for a given imagette timeseries, i the mask index, t_{i} the time the mask is first applied or updated, d_{i} the time during which it is maintained, x ≡ (t − t_{i})/τ_{0}, τ_{0} a time constant (set arbitrarily to 90 days), p_{j, i} the polynomial coefficients associated with the mask i, and finally Π(x) a function defined as
$$\begin{array}{c}\hfill \mathrm{\Pi}(x)=\{\begin{array}{cc}\hfill 1& \phantom{\rule{0.333333em}{0ex}}\text{if}\phantom{\rule{0.166667em}{0ex}}0\le x<1\hfill \\ \hfill 0& \phantom{\rule{0.333333em}{0ex}}\text{if}\phantom{\rule{0.166667em}{0ex}}x<0\phantom{\rule{0.166667em}{0ex}}\phantom{\rule{0.333333em}{0ex}}\text{or}\phantom{\rule{0.166667em}{0ex}}x\ge 1.\hfill \end{array}\end{array}$$
While the coefficient p_{3, i} informs us about the amplitude of the discontinuity induced by a given mask i, the three other coefficients (p_{0, i}, p_{1, i} and p_{2, i}) inform us about the longterm variations of the instrument residuals obtained with that mask.
Each of the generated instrument lightcurve is fitted by the model given by Eq. (35). An example of such a fit is given in Fig. 8. In most cases, this polynomial model reproduces very well the main characteristics of the systematic errors, in particular the jumps induced by the mask updates as well as the longterm variations induced by the longterm star drifts.
Fig. 8. Example of a generated instrumental lightcurve (single camera) fitted with the piecewise polynomial decomposition of Eq. (35). The black line represents the generated lightcurve and the red one the result of the fit. 
4.10. Implementation into PSLS
The model for the systematic errors presented in the previous section is implemented into PSLS as follows: we have at our disposal a set of p coefficients for each stellar magnitude, focal plane position (i.e. PSF), and subpixel position. We first identify the positions (focal plane and subpixel) corresponding to the magnitude the closest to that of the star we want to simulate. For each position, the number of p coefficients depends on the number of masks used at that position. Then, each individual lightcurve simulated by PSLS is divided into quarters. For each quarter, we randomly select the set of coefficients p among the ensemble previously selected. We proceed in the same way for each quarter and for each individual camera. By proceeding this way, we simulate the fact that each star will have different PSFs and subpixel positions in the different cameras and that these PSFs and subpixel positions will change after the rotations of the spacecraft by 90^{°} every 3 months. An example of such simulated lightcurves is shown in Fig. 9.
Fig. 9. Simulated instrument residual lightcurves (systematic errors) over 90 days for a star of mangitude V = 11 and for the EOL conditions. The lightcurves are plotted in terms of relative variations and were generated using Eq. (35) and as explained in Sect. (4.10). Each dotted line corresponds to an individual lightcurve (here 24 in total) while the thick solid line corresponds to the lightcurve obtained by averaging the 24 simulated lightcurves. 
The above example also illustrates the benefit of averaging the lightcurves over several cameras. Indeed as shown in Fig. 9 averaging over, for example 24 cameras, substantially reduces the residual errors because the systematic errors are not always in phase and the mask updates do not always occur at exactly the same times. However, the figure also highlights some degree of correlation between the individual lightcurves. Indeed, it can clearly be seen that some lightcurves are close to being in phase. These correlations are expected as explained and discussed in Sect. 7.2.
5. Other signal components
5.1. Stellar granulation
The granulation background is simulated by assuming two pseudoLorentzian functions
$$\begin{array}{c}\hfill G(\nu )={\displaystyle \sum _{i=1,2}\frac{{h}_{i}}{1+{\left(2\pi {\tau}_{i}\nu \right)}^{{\beta}_{i}}},}\end{array}$$(36)
where h_{i} is the height, τ_{i} the characteristic timescale, and β_{i} the slope of the Lorentzian function. The values of h_{i} and τ_{i} are determined from the scaling relations established by Kallinger et al. (2014) with Kepler observations of red giants, subgiants and mainsequence stars. These scaling relations are a function of peak frequency ν_{max} of the oscillations and the stellar mass M. Following Kallinger et al. (2014), the values of the two slopes (β_{1} and β_{2}) are both fixed to four.
5.2. Stellar activity
The stellar activity signal is simulated assuming a Lorentzian function
$$\begin{array}{c}\hfill \mathcal{A}(\nu )=\frac{2\phantom{\rule{0.166667em}{0ex}}{\sigma}_{\mathrm{A}}^{2}\phantom{\rule{0.166667em}{0ex}}{\tau}_{\mathrm{A}}}{1+{\left(2\pi {\tau}_{\mathrm{A}}\nu \right)}^{2}},\end{array}$$(37)
where σ_{A} is the amplitude and τ_{A} is the characteristic timescale of the activity component. Both parameters have to be specified by the user (but see the discussion in Sect. 7).
5.3. Planetary transit
Planetary transit lightcurve are simulated on the basis of Mandel & Agol (2002)’s formulation and using the Python implementation by Ian Crossfield at UCLA^{8}. This model allows us to specify several parameters controlling the characteristics of the transit lightcurve. Among them, PSLS allows us to specify the planet radius, the orbital period, the semimajor axis and finally the orbital angle. We have adopted a quadratic limbdarkening law (cf. Sect. 4 of Mandel & Agol 2002) and assumed default values for the corresponding two coefficients (namely γ_{1} = 0.25 and γ_{2} = 0.75). However, these coefficients can be set by the user.
6. Simulated stellar oscillation spectra
As a preliminary remark, we stress that the goal of the simulator is not to provide stateoftheart modelling of a given target but rather to be able to mimic the main characteristics of objects of interest. Accordingly, we did not carry out a quantitative and extensive comparison between outputs of our simulator and lightcurves (or equivalently PSD) obtained from highprecision photometric observations, from space missions such as CoRoT and Kepler. However, to illustrate the quality and the relevance of the simulated lightcurves, we performed a qualitative comparison with Kepler observations. Three Kepler targets were selected according to the quality of the data and their evolutionary status: a main sequence star (16 Cyg B–KIC 12069449), a sub giant (KIC 12508433) and a giant on the Red Giant Branch (KIC 009882316). For each of them, a simulation was generated with stellar parameters and models as close as possible to the corresponding target.
6.1. Main sequence star
16 Cyg B (KIC 12069449) belongs to the Kepler legacy sample (Lund et al. 2017a,b). As input for PSLS, we considered a set of theoretical adiabatic mode frequencies computed with ADIPLS, using one of the stellar models considered in Silva Aguirre et al. (2017). The effective temperature and surface gravity were adjusted in accordance with the 1D stellar model while the seismic indices ν_{max} and Δν were taken from Lund et al. (2017a).
We generated an initial lightcurve assuming a V = 10.0 PLATO target observed with 24 cameras in EOL conditions and for a duration of 2 years. The choice of magnitude is motivated by the fact that we expect to derive stellar ages with the required accuracy (10%) with 24 cameras up to the magnitude V = 10.0 (Goupil 2017)^{9}. The two parameters controlling the activity component have been adjusted so that it matches that of the activity component seen in the 16 Cyg B Kepler lightcurve. The corresponding PSLS configuration file is given in Appendix A. The mode frequencies, linewidths, and heights used as input for the simulation are displayed in Fig. 10. The modes for which the frequencies significantly depart from the general trends are mixed modes. However, they have such low amplitudes that in practice they are not at all detectable.
Fig. 10. Top panel: Échelle diagram corresponding to the frequencies used as input for the simulations made for 16 Cyg B (KIC 12069449). A mean large separation of Δν = 118.9 μHz was assumed when plotting the échelle diagram. Bottom panel: corresponding mode linewidths (top) and mode heights (bottom). 
The corresponding simulated lightcurve is displayed in Fig. 11 while the corresponding PSD is plotted in Fig. 12, where we have depicted the various contributions to the PSD. As can been seen, the systematic errors start to dominate over the stellar signal only below ∼20 μHz. On the other hand, they remain negligible in the frequency domain where the solarlike oscillations and stellar granulation signal lie. As expected at that magnitude, the random noise (white noise) dominates the signal in this domain. Nevertheless, the presence of the oscillations in the PSD is clearly discerned when zooming and smoothing the PSD in this frequency domain (see bottom panel of Fig. 12).
Fig. 11. Simulated lightcurve for the main sequence star 16 Cyg B (KIC 12069449) with simulation parameters representative of a V = 10.0 PLATO target observed in EOL conditions with 24 cameras (see the details given in Sect. 6.1). The grey curve corresponds to the raw lightcurve while the black ones is the lightcurve averaged over one hour. 
Fig. 12. PSD of the simulated lightcurve of 16 Cyg B (KIC 12069449) shown in Fig. 11. Top: full PSD. The grey curve represents the raw PSD (i.e. unsmoothed PSD) while the black line corresponds to the PSD obtained after applying a running average over a width of 10 μHz. The coloured lines represent the various contributions to the signal (see the associated legend). Bottom: zoom in the frequency domain where solarlike oscillations are detected. Only the smoothed PSD is shown. 
The simulated PSD cannot be directly compared with Kepler observations for that star because PLATO and Kepler have different characteristics and furthermore 16 Cyg B is so bright that its image on the CCD is saturated. Therefore, to perform a comparison we adjusted the white noise level (equivalently the NSR value) so that it matches the level of the white noise seen at high frequency in the Kepler lightcurve. We compare in Fig. 13 the simulated PSD with the Kepler observations. Qualitatively, we note a fair agreement between the simulation and the observations. The figure however highlights some differences, in particular in terms of mode heights and the width of the oscillations envelope. As the characteristics of the oscillations are obtained through scaling relations, we do not except the match to be perfect, and in any case this is not the ultimate goal of the simulator.
Fig. 13. Comparison of a simulated PSD and the one obtained from Kepler observations of the main sequence star 16 Cyg B (KIC 12069449). The grey and black lines have the same meaning as in Fig. 12. The red curve corresponds to the smoothed PSD obtained from the observations. 
6.2. Subgiant star
The subgiant star KIC 12508433 observed by Kepler is among the subgiant stars studied in detail by Deheuvels et al. (2014). As an input for PSLS, we use the same stellar parameters as in this study as well as the set of theoretical mode frequencies that best fits the seismic constraints. As for 16 Cyg B (KIC 12069449), we adjusted the white noise level so that it matches the level of the white noise seen at high frequency in the corresponding Kepler lightcurve. The comparison between the simulated PSD and the one computed from the Kepler lightcurve is shown in Fig. 14. Here also, we have a good qualitative agreement between both PSDs. Nonetheless, some mismatch is visible by eye, especially concerning the mode heights and the width of the oscillation envelope.
6.3. Redgiant star
The red giant KIC 9882316 has been studied extensively since the Kepler era. Precise measurements of its seismic indexes (Δν, ν_{max}, ΔΠ and q) have been published for example in Mosser et al. (2015). We generated for this red giant a simulated lightcurve on the basis of the UP method (see Sect. 3.2). The latter requires specifying the seismic indexes as well as the effective temperature ; all these parameters are taken from Mosser et al. (2015). To illustrate the quality of the lightcurve expected for red giants with PLATO, we first perform a simulation for a V = 12.5 PLATO target observed with 24 cameras in EOL conditions for a duration of 2 years. The corresponding PSLS configuration file is given in Appendix A. We note that solarlike oscillations are also expected to be detectable in fainter red giants, but we limit ourselves to this magnitude because the systematic errors were not quantified for fainter stars. The PSD of the simulated lightcurve is displayed in Fig. 15, where we have also plotted the different contributions to the signal. As can been seen, the systematic errors remain negligible compared to the solarlike oscillations and stellar granulation. On the other hand, they dominate below ν ∼ 20 μHz.
Fig. 15. PSD of the simulated lightcurve for the Kepler red giant KIC 9882316 seen as a PLATO target of V = 12.5 in EOL conditions with 24 cameras. The curves have the same meaning as the top panel of Fig. 12. 
Finally, we compare the predictions made by PSLS with Kepler observations. We again adjust the white noise level to match the Kepler observations for that target and considered a simulation duration of 4 years. The comparison is shown in Fig. 16. The agreement between the simulation and the Kepler observations is rather good. In particular, we see that the mixedmode frequencies and heights are quite well reproduced.
Fig. 16. Same as Fig. 13 for the red giant star KIC 9882316 observed with Kepler. Top: entire oscillation spectrum. Bottom: zoom around the maximum peak frequency. Here we did not apply a running average over the PSD. The dotted red/blue/green vertical lines represent the frequency locations of the radial/dipole/quadrupole modes respectively. 
7. Discussion
We discuss in this section the limitations of the current approach and possible future improvements.
7.1. Instrument model
As far as the modelling of the instrument is concerned, there is still an important effect missing in the image simulator (PIS), which is the Brighter Fatter Effect (BFE hereafter). Indeed, there are several pieces of evidence showing that spot images using CCDs do not exactly scale with the spot intensity: bright spots tend to be broader than faint ones, using the same illumination pattern (see Guyonnet et al. 2015, and references therein). The BFE is fundamentally due to the selfelectrostatic interaction between charges in different pixels. This broadening, which mainly affects bright targets, would not be a problem as long as these interactions are stable in time. However this cannot be the case since the longterm drift of the stellar position changes the charge distribution in the different pixels. Analytical models (e.g.. Guyonnet et al. 2015) can be easily implemented into PIS, and that can subsequently be used to correct both the CCD imagettes and the lightcurves generated onboard. Such analytical models involve several free coefficients that can be calibrated onground with the test bench dedicated to the calibration of the flight PLATO CCDs. The BFE is not expected to evolve with time so that the parameters obtained with the onground calibration can be used throughout the mission. The calibration procedure for the PLATO CCD is not yet established but can in principle follow the one proposed in Guyonnet et al. (2015). As soon as we have at our disposal calibrated values of the BFE coefficients, it will be possible to update our simulations and derive new prescriptions to account for this additional source of systematic errors.
Charge diffusion within the CCD was neglected in this work since we still lack reliable estimates of its amplitude in the case of the PLATO CCD. However, charge diffusion is expected to a have nonnegligible impact on the performance since it enlarges somewhat the width of the PSF and leads to the suppression of the smallscale structures of the optical PSF. It has been shown for example by Lauer (1999) that in standard rearilluminated CCDs this phenomena can be modelled by performing the convolution of the optical PSF with a 2D Gaussian kernel with a given width, which strongly depends on the wavelength and type of CCD device. To what extent this model is applicable to the PLATO CCD and what typical width to use for representative PLATO targets are still open questions. Fortunately, tests on representative PLATO CCD are currently taking place at the ESTEC and will provide feedback on this issue that should allow us to improve the present performance assessment.
Besides the above mentioned effects taking place at the detector level, PLATO will be subject to many others perturbations that are not yet taken into account in the present simulator. Among them, we can in particular mention thermal trends after the rotations of the spacecraft by 90^{°} every 3 months, the regular thermal perturbations induced by the daily downlinks, the momentum wheels desaturations, and finally the residual outliers that would not have been detected by the outlier detection algorithms. All these perturbations are not yet well characterized but will be better known in the future, in particular with the deeper involvement of the prime contractor of the platform in the project and progress in the definition of the data processing pipeline.
7.2. Single to multiple instrument simulations
Strong correlations between the lightcurves coming from different cameras are expected. For instance, stellar drifts along the focal plane are expected to be strongly correlated between the cameras. Although for each given target, the associated PSF and aperture mask can differ between cameras, variations in the stellar flux induced by stellar drifts will present some degree of correlation, which only pixellevel simulations made for several cameras can quantify.
PSLS generates the instrument systematic errors of each individual lightcurve individually. However, it uses the model parameters derived from pixellevel simulations made for a single camera only (see Sect. 4.9). Each observed target will have different PSFs and subpixel positions in the different cameras with which it is observed. Accordingly, to simulate this diversity, PSLS randomly selects the model parameters derived at various positions (for a given star magnitude).
However, this approach is to some extent conservative. Indeed we use the systematic errors evaluated for the same camera. Each individual lightcurve will be corrected a posteriori onground on the basis of auxiliary data (such as the PSF) obtained by calibrating independently each individual camera. There are good reasons to believe that the systematic errors will be different from one camera to another. Indeed, the systematic errors made on each individual calibration are expected to be different because the cameras are not exactly identical. Indeed, the cameras do not have the exact same alignments of the CCD over the focal plane, same focal plane flatness, same PRNU, same optical manufacturing and alignment errors, etc. However, to confirm this it is required to simulate a statistically sufficient number of cameras with slightly different setups (results from a limited attempt can be found in Deru et al. 2017).
7.3. Stellar contamination
While the presence of contaminant stars was taken into account in our calculation of the NSR as a function of the stellar magnitude (see Sect. 4.4), this is not the case for the systematic errors. It is, in principle, possible to take into account the contaminant stars in the reconstruction of the stellar PSF and the generation of the threemonth imagette timeseries (Reese & Marchiori 2018). However, this is numerically challenging since due to the high diversity in terms of configuration, statistically reliable quantification of the impact of stellar contamination would require a much larger sample of simulations. Accordingly, we plan to perform, in the near future, simulations on the basis of a sufficiently large stellar field extracted from the Gaia DR2 catalogue.
7.4. Stellar activity and rotational modulations
Although the presence of stellar activity has little impact on solarlike oscillations, its presence is critical for the detection of planetary transits. At the present time, the parameters of the activity component still need to be specified by the user. Hence, our objective is to implement into the simulator some empirical descriptions of the magnetic activity sufficiently realistic to be representative of solarlike pulsators in the context of PLATO. To this end, we plan to analyse a large set of Kepler targets and derive from their spectra, in a similar way as for example in de Assis Peralta et al. (2018), two main characteristic parameters of the activity, namely the characteristic timescale and the amplitude associated with the activity component. Once these parameters are derived for a large sample of stars, we believe it will be possible to derive some relations between these parameters and some stellar parameters, such as the surface rotation period and the Rossby number which is the ratio of the rotation period and convective turnover time. Indeed, the differential rotation existing at the interface between the convective envelope and the internal radiative zone is believed to be at the origin of the stellar dynamo while convection is believed to be responsible for the diffusion of the magnetic field in the convective zone (see e.g. Montesinos et al. 2001, and references therein).
Finally, one other missing activityrelated signal is the rotational modulation due to the presence of rather large spots on the stellar surface. It is hence planned to implement in the near future some of the existing spot models (for a review on this problem see Lanza 2016). However, one difficulty is to have at our disposal representative prescriptions for the model parameters, for instance typically the number of spots, their sizes and their lifetimes. To our knowledge, such prescriptions do not exist yet. Therefore, as a starting point we plan to let the user chose these parameters.
8. Conclusion
We have presented here a lightcurve simulator, named the PLATO Solarlike Lightcurve Simulator (PSLS), that aims at simulating, as realistically as possible, solarlike oscillations together with other stellar signals (granulation, activity, planetary transits) representative of stars showing such pulsations. One of the specificities of this tool is its ability to account for instrumental and observational sources of errors that are representative of ESA’s PLATO mission. The latter were modelled on the basis of the Plato Image Simulator (PIS), which simulates the signal at the CCD pixel level. At the Beginning Of Life, we show that the systematic errors are always compliant with the specifications, whereas at the End Of Life they marginally exceed the specifications between 10 μHz and 100 μHz approximately (see Fig. 6) as a result of Charge Transfer Inefficiency (CTI). However, some mitigation options for the CTI are currently under study (e.g. charge injection, increasing the camera shielding). Although the procedure is not yet fully established, existing correction algorithms can be implemented in the context of PLATO (e.g. Short et al. 2013; Massey et al. 2014).
The PIS code is however not adapted to generating in a massive way simulated longduration lightcurves (e.g. up to two years in the case of PLATO). This is why a parametric description of the systematic errors expected in the time domain has been derived from the PIS simulations. This model reproduces both the residual longterm flux variations due to the instrument as well as the jumps induced by the maskupdates for those of the targets (the large majority of the targets of sample P5) for which photometry is extracted onboard. Implemented into PSLS, this parametric model enables us to mimic in a realistic and efficient way the instrument systematic errors representative of the PLATO multitelescope concept. Hence, with the inclusion of stellar signal components that are the most representative for the PLATO targets together with a realistic description of the instrument response function, this lightcurve simulator becomes an indispensable tool for the preparation of the mission. Its adaptation to other future space missions is in principle possible, provided that some analytical prescriptions for the instrumental and environmental sources of errors representative of the mission are available.
Lightcurves simulated with PSLS allow us to conclude that the systematic errors remain negligible above about 100 μHz and only start to dominate over the stellar signal below ∼20 μHz. Accordingly, they should not impact the core science objectives of PLATO. One the other hand, they can potentially impact the analysis of the signal below ν ∼ 20 μHz. In both cases, however, firm conclusions deserve dedicated studies, which are beyond the scope of the present work. It must further be made clear that the level of systematic errors predicted by the present modelling is, strictly speaking, only representative for those targets for which the photometry is extracted onboard (i.e. the large majority of the sample P5). For all the other samples, in particular the main sample (P1), the photometry will be extracted onground and thus will not suffer from the quasiregular mask updates. Therefore, a lower level of systematic errors are expected for these samples. Accordingly, the use of PSLS must be considered as a conservative approach for these samples.
This simulator is based on our current knowledge of the instrument and of the current development of the correction pipeline. Although already well advanced, this knowledge will improve in the near future as soon as a first flight model of the camera will be available and fully characterized (around the beginning of 2021). At that time, it will be relatively easy to update our pixellevel simulations and subsequently the parameters used by the model for the systematic errors as well as the NoisetoSignal Ratio (NSR) table.
The PSLS source code is available for download from the PSLS website (http://psls.lesia.obspm.fr) as well as from Zenodo.org (http://doi.org/10.5281/zenodo.2581107). The source code is free: you can redistribute it and/or modify it under the terms of the GNU General Public License (for more details see http://www.gnu.org/licenses). The present paper describes the version 0.8.
The additional factor of two comes from the fact we assume here a singlesided PSD while Baudin et al. (2005) assumed a doublesided one.
Acknowledgments
This work has benefited from financial support by CNES in the framework of its contribution to the PLATO mission. It has made use of data from the European Space Agency (ESA) mission Gaia (https://www.cosmos.esa.int/gaia), processed by the Gaia Data Processing and Analysis Consortium (DPAC, https://www.cosmos.esa.int/web/gaia/dpac/consortium). Funding for the DPAC has been provided by national institutions, in particular the institutions participating in the Gaia Multilateral Agreement. We acknowledge T. Prod’homme and D. Tiphéne for the useful discussions we had about various CCD effects. We thank the anonymous referee for his/her remarks which enabled us to improve significantly the simulator and the present article.
References
 Anderson, E. R., Duvall, T. L., & Jefferies, S. M. 1990, ApJ, 364, 699 [NASA ADS] [CrossRef] [Google Scholar]
 Appourchaux, T., Benomar, O., Gruberbauer, M., et al. 2012, A&A, 537, A134 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Appourchaux, T., Antia, H. M., Benomar, O., et al. 2014, A&A, 566, A20 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Appourchaux, T., Antia, H. M., Benomar, O., et al. 2016, A&A, 595, C2 [CrossRef] [EDP Sciences] [Google Scholar]
 Baglin, A., Auvergne, M., Barge, P., et al. 2006a, in The CoRoT Mission PreLaunch Status  Stellar Seismology and Planet Finding, eds. M. Fridlund, A. Baglin, J. Lochard, & L. Conroy, ESA SP, 1306, 33 [Google Scholar]
 Baglin, A., Auvergne, M., Boisnard, L., et al. 2006b, in 36th COSPAR Scientific Assembly, COSPAR Meet., 36 [Google Scholar]
 Ball, W. H., Chaplin, W. J., Schofield, M., et al. 2018, ApJS, 239, 34 [NASA ADS] [CrossRef] [Google Scholar]
 Ballot, J., Gizon, L., Samadi, R., et al. 2011, A&A, 530, A97 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Barban, C., Hill, F., & Kras, S. 2004, ApJ, 602, 516 [NASA ADS] [CrossRef] [Google Scholar]
 Baudin, F., Samadi, R., Goupil, M.J., et al. 2005, A&A, 433, 349 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Baudin, F., Samadi, R., Appourchaux, T., & Michel, E. 2007, ArXiv eprints [arXiv:0710.3378] [Google Scholar]
 Belkacem, K. 2012, in SF2A2012: Proceedings of the Annual meeting of the French Society of Astronomy and Astrophysics, eds. S. Boissier, P. de Laverny, N. Nardetto, et al., 173 [Google Scholar]
 Belkacem, K., & Samadi, R. 2013, in Lect. Notes Phys., eds. M. Goupil, K. Belkacem, C. Neiner, F. Lignières, & J. J. Green (Berlin: Springer Verlag), 865, 179 [NASA ADS] [CrossRef] [Google Scholar]
 Belkacem, K., Goupil, M. J., Dupret, M. A., et al. 2011, A&A, 530, A142 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Belkacem, K., Samadi, R., Mosser, B., Goupil, M. J., & Ludwig, H. G. 2013, in Progress in Physics of the Sun and Stars: A New Era in Helio and Asteroseismology, eds. H. Shibahashi, & A. E. LynasGray, ASP Conf. Ser., 479, 61 [NASA ADS] [Google Scholar]
 Benomar, O., Goupil, M., Belkacem, K., et al. 2018, ApJ, 857, 119 [NASA ADS] [CrossRef] [Google Scholar]
 Berthomieu, G., Toutain, T., Gonczi, G., et al. 2001, ESA SP464: SOHO 10/GONG 2000 Workshop: Helio and Asteroseismology at the Dawn of the Millennium, 411 [Google Scholar]
 Borucki, W. J., Koch, D., Basri, G., et al. 2010, Science, 327, 977 [NASA ADS] [CrossRef] [PubMed] [Google Scholar]
 Bryson, S. T., Tenenbaum, P., Jenkins, J. M., et al. 2010, ApJ, 713, L97 [NASA ADS] [CrossRef] [Google Scholar]
 Censor, Y. 1981, SIAM Rev., 23, 444 [CrossRef] [Google Scholar]
 Chaplin, W. J., Elsworth, Y., Howe, R., et al. 1997, MNRAS, 287, 51 [NASA ADS] [CrossRef] [Google Scholar]
 Chaplin, W. J., Elsworth, Y., Davies, G. R., et al. 2014, MNRAS, 445, 946 [NASA ADS] [CrossRef] [Google Scholar]
 ChristensenDalsgaard, J. 2008, Ap&SS, 316, 113 [NASA ADS] [CrossRef] [Google Scholar]
 Corsaro, E., Fröhlich, H.E., Bonanno, A., et al. 2013, MNRAS, 430, 2313 [NASA ADS] [CrossRef] [Google Scholar]
 de Assis Peralta, R., Samadi, R., & Michel, E. 2018, Astron. Nachr., 339, 134 [NASA ADS] [CrossRef] [Google Scholar]
 De Ridder, J., Arentoft, T., & Kjeldsen, H. 2006, MNRAS, 365, 595 [NASA ADS] [CrossRef] [Google Scholar]
 De Ridder, J., Barban, C., Baudin, F., et al. 2009, Nature, 459, 398 [Google Scholar]
 Deheuvels, S., Doğan, G., Goupil, M. J., et al. 2014, A&A, 564, A27 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Deru, A., Samadi, R., & Grolleau, E. 2017, Impacts of the Pointing Knowledge on the Longterm Drift Correction, Tech. Rep. PLATOLESIAPDCTN0029_i1.0, LESIA, Observatoire de Paris [Google Scholar]
 Duvall, Jr., T. L., Jefferies, S. M., Harvey, J. W., Osaki, Y., & Pomerantz, M. A. 1993, ApJ, 410, 829 [NASA ADS] [CrossRef] [Google Scholar]
 Dziembowski, W. A. 1971, Acta Astron., 21, 289 [NASA ADS] [Google Scholar]
 Fialho, F., & Auvergne, M. 2006, in The CoRoT Mission PreLaunch Status  Stellar Seismology and Planet Finding, eds. M. Fridlund, A. Baglin, & J. Lochard, ESA SP, 1306, 289 [NASA ADS] [Google Scholar]
 Gaia Collaboration (Brown, A. G. A., et al.) 2018, A&A, 616, A1 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Gehan, C., Mosser, B., Michel, E., Samadi, R., & Kallinger, T. 2018, A&A, 616, A24 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Gizon, L., Ballot, J., Michel, E., et al. 2013, Proc. Natl Acad. Sci., 110, 13267 [NASA ADS] [CrossRef] [Google Scholar]
 Gizon, L., & Solanki, S. K. 2003, ApJ, 589, 1009 [NASA ADS] [CrossRef] [Google Scholar]
 Goupil, M. 2017, Eur. Phys. J. Web Conf., 160, 01003 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Goupil, M. J., Mosser, B., Marques, J. P., et al. 2013, A&A, 549, A75 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Green, J. 2011, Microscanning, Tech. Rep. PLATOGSTN231LESIA_i1.0, LESIA, Observatoire de Paris [Google Scholar]
 Green, J. J., & Wyatt, L. R. 2006, J. Atm. Ocean. Technol., 23, 501 [CrossRef] [Google Scholar]
 Grosjean, M., Dupret, M.A., Belkacem, K., et al. 2014, A&A, 572, A11 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Guyonnet, A., Astier, P., Antilogus, P., Regnault, N., & Doherty, P. 2015, A&A, 575, A41 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Hekker, S., & ChristensenDalsgaard, J. 2017, A&ARv, 25, 1 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Huber, D., Bedding, T. R., Stello, D., et al. 2011, ApJ, 743, 143 [NASA ADS] [CrossRef] [Google Scholar]
 Huber, D., Chaplin, W. J., Chontos, A., et al. 2019, AJ, accepted [arXiv:1901.01643] [Google Scholar]
 Kallinger, T., Weiss, W. W., Barban, C., et al. 2010, A&A, 509, A77 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Kallinger, T., De Ridder, J., Hekker, S., et al. 2014, A&A, 570, A41 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Lanza, A. F. 2016, in Lect. Notes Phys., eds. J. P. Rozelot, & C. Neiner (Berlin: Springer Verlag), 914, 43 [NASA ADS] [CrossRef] [Google Scholar]
 Lauer, T. R. 1999, PASP, 111, 1434 [NASA ADS] [CrossRef] [Google Scholar]
 Lebreton, Y., Goupil, M. J., & Montalbán, J. 2014a, EAS Pub. Ser., 65, 99 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Lebreton, Y., Goupil, M. J., & Montalbán, J. 2014b, EAS Pub. Ser., 65, 177 [CrossRef] [Google Scholar]
 Lund, M. N., Silva Aguirre, V., Davies, G. R., et al. 2017a, ApJ, 835, 172 [CrossRef] [Google Scholar]
 Lund, M. N., Silva Aguirre, V., Davies, G. R., et al. 2017b, ApJ, 850, 110 [NASA ADS] [CrossRef] [Google Scholar]
 Mandel, K., & Agol, E. 2002, ApJ, 580, L171 [NASA ADS] [CrossRef] [Google Scholar]
 Marchiori, V., Samadi, R., Fialho, F., Paproth, C., & Santerne, A. 2019, A&A, submitted [Google Scholar]
 MarcosArenal, P., Zima, W., De Ridder, J., et al. 2014, A&A, 566, A92 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Massey, R., Schrabback, T., Cordes, O., et al. 2014, MNRAS, 439, 887 [NASA ADS] [CrossRef] [Google Scholar]
 Michel, E., Samadi, R., Baudin, F., et al. 2009, A&A, 495, 979 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Miglio, A., Chiappini, C., Mosser, B., et al. 2017, Astron. Nachr., 338, 644 [NASA ADS] [CrossRef] [Google Scholar]
 Miglio, A., Girardi, L., Rodrigues, T. S., Stello, D., & Chaplin, W. J. 2015, in Asteroseismology of Stellar Populations in the Milky Way, eds. A. Miglio, P. Eggenberger, & L. Girardi, Astrophys. Space Sci. Proc., 39, 11 [NASA ADS] [CrossRef] [Google Scholar]
 Montesinos, B., Thomas, J. H., Ventura, P., & Mazzitelli, I. 2001, MNRAS, 326, 877 [NASA ADS] [CrossRef] [Google Scholar]
 Mosser, B., & Miglio, A. 2016, IV.2 Pulsating Red Giant Stars, ed. CoRot Team, 197 [Google Scholar]
 Mosser, B., Belkacem, K., Goupil, M.J., et al. 2010, A&A, 517, A22 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Belkacem, K., Goupil, M. J., et al. 2011, A&A, 525, L9 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Elsworth, Y., Hekker, S., et al. 2012a, A&A, 537, A30 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Goupil, M. J., Belkacem, K., et al. 2012b, A&A, 540, A143 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Samadi, R., & Belkacem, K. 2013, in SF2A2013: Proceedings ofthe Annual meeting of the French Society of Astronomy and Astrophysics, eds. L. Cambresy, F. Martins, E. Nuss, & A. Palacios, 25 [Google Scholar]
 Mosser, B., Vrard, M., Belkacem, K., Deheuvels, S., & Goupil, M. J. 2015, A&A, 584, A50 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Pinçon, C., Belkacem, K., Takata, M., & Vrard, M. 2017, A&A, 600, A1 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Mosser, B., Michel, E., Samadi, R., et al. 2019, A&A, 622, A76 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Nigam, R., Kosovichev, A. G., Scherrer, P. H., & Schou, J. 1998, ApJ, 495, L115 [NASA ADS] [CrossRef] [Google Scholar]
 Ouazzani, R.M., Green, J. J., & Samadi, R. 2015, Eur. Phys. J. Web Conf., 101, 06050 [CrossRef] [Google Scholar]
 Prod’homme, T., Verhoeve, P., Beaufort, T., et al. 2016, in High Energy, Optical, and Infrared Detectors for Astronomy VII, Proc. SPIE, 9915, 99150U [CrossRef] [Google Scholar]
 Rauer, H., Catala, C., Aerts, C., et al. 2014, Exp. Astron., 38, 249 [NASA ADS] [CrossRef] [Google Scholar]
 Reese, D. R. 2018a, Testing and Choosing the Microscanning Path, Tech. Rep. PLATOLESIAPDCTN0045_i1.0, LESIA, Observatoire de Paris [Google Scholar]
 Reese, D. R. 2018b, The Weighted Positive RLS Inversion Method, Tech. Rep. PLATOLESIAPDCTN0037_i1.1, LESIA, Observatoire de Paris [Google Scholar]
 Reese, D. R., & Marchiori, V. A. 2018, PSF Inversions in the Presence of Contaminating Stars, Tech. Rep. PLATOLESIAPDCTN0039_i1.0, LESIA, Observatoire de Paris [Google Scholar]
 Reese, D. R., Chaplin, W. J., Davies, G. R., et al. 2016, A&A, 592, A14 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Roxburgh, I. W., & Vorontsov, S. V. 1997, MNRAS, 292, L33 [NASA ADS] [Google Scholar]
 Samadi, R. 2015, Photometric Impact of the Longterm Drift of the Star Position and Efficiency of its Correction, Tech. Rep. PLATOLESIAPDCRP0020_i1.0, LESIA, Observatoire de Paris [Google Scholar]
 Short, A., Crowley, C., de Bruijne, J. H. J., & Prod’homme, T. 2013, MNRAS, 430, 3078 [NASA ADS] [CrossRef] [Google Scholar]
 Silva Aguirre, V., Lund, M. N., Antia, H. M., et al. 2017, ApJ, 835, 173 [NASA ADS] [CrossRef] [Google Scholar]
 Sonoi, T., Samadi, R., Belkacem, K., et al. 2015, A&A, 583, A112 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Stello, D., Huber, D., Bedding, T. R., et al. 2013, ApJ, 765, L41 [NASA ADS] [CrossRef] [Google Scholar]
 Unno, W., Osaki, Y., Ando, H., Saio, H., & Shibahashi, H. 1989, Nonradial Oscillations of Stars, 2nd edn. (Tokyo: University of Tokyo Press) [Google Scholar]
 Van Eylen, V., Lund, M. N., Silva Aguirre, V., et al. 2014, ApJ, 782, 14 [NASA ADS] [CrossRef] [Google Scholar]
 Van Eylen, V., Dai, F., Mathur, S., et al. 2018, MNRAS, 478, 4866 [NASA ADS] [CrossRef] [Google Scholar]
 Vrard, M., Kallinger, T., Mosser, B., et al. 2018, A&A, 616, A94 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
Appendix A: Configuration file for the mainsequence star KIC 12069449 (16 Cyg B)
Appendix B: Configuration file for the red giant star KIC 9882316
All Tables
All Figures
Fig. 1. Typical NSR evolution curve as a function of increasing aperture size. Pixels with the smallest noisetosignal ratio are addedup successively. The collection of pixels giving the lowest aggregate NSR defines the binary mask for a given target. 

In the text 
Fig. 2. Top: examples of lightcurves generated from a simulated timeseries of CCD imagettes. The red curve corresponds to the lightcurve generated with a fixed binary mask while the blue one includes a series of mask updates. The dotted vertical lines identify the times at which the masks were updated. Bottom: corresponding time variations of the NSR. 

In the text 
Fig. 3. Examples of singlecamera lightcurves generated from a simulated timeseries of CCD imagettes and after correcting it for the longterm drift of the stellar position as explained in Sect. 4.6. We represent the relative flux variation in %. The red (reps. blue) curve corresponds to EOL (resp. BOL) observation conditions. The dotted vertical lines identify the times at which the masks were updated. 

In the text 
Fig. 4. Archimedean spiral used for the microscanning strategy. The dotted lines correspond to the CCD pixel borders. 

In the text 
Fig. 5. Top: original PSF. Bottom: PSF obtained by inversion on the basis of the microscanning technique (see Sect. 4.7). The dotted lines correspond to the CCD pixel borders. 

In the text 
Fig. 6. PSD of the residual lightcurve obtained with two threemonth PIS simulations, one representative of the BOL (cyan) and the second of the EOL (pink). The results shown here correspond to a star of magnitude 11. The solid coloured line represents the fitted model defined in Eq. (33). The solid black line represents the PLATO requirements in terms of systematic errors translated for a single camera by assuming that they are uncorrelated between the different camera (see text). 

In the text 
Fig. 7. Amplitude of the systematic errors (σ) as a function of the stellar magnitude. This quantity is computed according to Eq. (34). At each stellar magnitude, only the 90th percentile is displayed. 

In the text 
Fig. 8. Example of a generated instrumental lightcurve (single camera) fitted with the piecewise polynomial decomposition of Eq. (35). The black line represents the generated lightcurve and the red one the result of the fit. 

In the text 
Fig. 9. Simulated instrument residual lightcurves (systematic errors) over 90 days for a star of mangitude V = 11 and for the EOL conditions. The lightcurves are plotted in terms of relative variations and were generated using Eq. (35) and as explained in Sect. (4.10). Each dotted line corresponds to an individual lightcurve (here 24 in total) while the thick solid line corresponds to the lightcurve obtained by averaging the 24 simulated lightcurves. 

In the text 
Fig. 10. Top panel: Échelle diagram corresponding to the frequencies used as input for the simulations made for 16 Cyg B (KIC 12069449). A mean large separation of Δν = 118.9 μHz was assumed when plotting the échelle diagram. Bottom panel: corresponding mode linewidths (top) and mode heights (bottom). 

In the text 
Fig. 11. Simulated lightcurve for the main sequence star 16 Cyg B (KIC 12069449) with simulation parameters representative of a V = 10.0 PLATO target observed in EOL conditions with 24 cameras (see the details given in Sect. 6.1). The grey curve corresponds to the raw lightcurve while the black ones is the lightcurve averaged over one hour. 

In the text 
Fig. 12. PSD of the simulated lightcurve of 16 Cyg B (KIC 12069449) shown in Fig. 11. Top: full PSD. The grey curve represents the raw PSD (i.e. unsmoothed PSD) while the black line corresponds to the PSD obtained after applying a running average over a width of 10 μHz. The coloured lines represent the various contributions to the signal (see the associated legend). Bottom: zoom in the frequency domain where solarlike oscillations are detected. Only the smoothed PSD is shown. 

In the text 
Fig. 13. Comparison of a simulated PSD and the one obtained from Kepler observations of the main sequence star 16 Cyg B (KIC 12069449). The grey and black lines have the same meaning as in Fig. 12. The red curve corresponds to the smoothed PSD obtained from the observations. 

In the text 
Fig. 14. Same as Fig. 13 for the subgiant star KIC 12508433 observed with Kepler. 

In the text 
Fig. 15. PSD of the simulated lightcurve for the Kepler red giant KIC 9882316 seen as a PLATO target of V = 12.5 in EOL conditions with 24 cameras. The curves have the same meaning as the top panel of Fig. 12. 

In the text 
Fig. 16. Same as Fig. 13 for the red giant star KIC 9882316 observed with Kepler. Top: entire oscillation spectrum. Bottom: zoom around the maximum peak frequency. Here we did not apply a running average over the PSD. The dotted red/blue/green vertical lines represent the frequency locations of the radial/dipole/quadrupole modes respectively. 

In the text 
Current usage metrics show cumulative count of Article Views (fulltext article views including HTML views, PDF and ePub downloads, according to the available data) and Abstracts Views on Vision4Press platform.
Data correspond to usage on the plateform after 2015. The current usage metrics is available 4896 hours after online publication and is updated daily on week days.
Initial download of the metrics may take a while.