Issue 
A&A
Volume 644, December 2020



Article Number  A171  
Number of page(s)  8  
Section  Stellar structure and evolution  
DOI  https://doi.org/10.1051/00046361/202038222  
Published online  16 December 2020 
Velocityintensity asymmetry reversal of solar radial pmodes
^{1}
LESIA, Observatoire de Paris, PSL Research University, CNRS, Université Pierre et Marie Curie, Université Paris Diderot, 92195 Meudon, France
email: jordan.philidet@obspm.fr
^{2}
Zentrum für Astronomie der Universität Heidelberg, Landessternwarte, Königstuhl 12, 69117 Heidelberg, Germany
^{3}
GEPI, Observatoire de Paris, PSL Research University, CNRS, Université Pierre et Marie Curie, Université Paris Diderot, 92195 Meudon, France
Received:
21
April
2020
Accepted:
28
October
2020
The development of spaceborne missions has significantly improved the quality of the measured spectra of solarlike oscillators. Their pmode line profiles can now be resolved, and the asymmetries inferred for a variety of stars other than the Sun. However, it has been known for a long time that the asymmetries of solar pmodes are reversed between the velocity and the intensity spectra. Understanding the origin of this reversal is necessary in order to use asymmetries as a tool for seismic diagnosis. For stars other than the Sun, only the intensity power spectrum is sufficiently resolved to allow for an estimation of mode asymmetries. We recently developed an approach designed to model and predict these asymmetries in the velocity power spectrum of the Sun and to successfully compare them to their observationally derived counterpart. In this paper we expand our model and predict the asymmetries featured in the intensity power spectrum. We find that the shape of the mode line profiles in intensity is largely dependent on how the oscillationinduced variations of the radiative flux are treated, and that modelling it realistically is crucial to understanding asymmetry reversal. Perturbing a solarcalibrated grey atmosphere model, and adopting the quasiadiabatic framework as a first step, we reproduce the asymmetries observed in the solar intensity spectrum for lowfrequency modes. We conclude that, unlike previously thought, it is not necessary to invoke an additional mechanism (e.g. nonadiabatic effects, coherent nonresonant background signal) to explain asymmetry reversal. This additional mechanism is necessary, however, to explain asymmetry reversal for higherorder modes.
Key words: methods: analytical / Sun: helioseismology / Sun: oscillations / stars: atmospheres / stars: oscillations / stars: solartype
© J. Philidet et al. 2020
Open Access article, published by EDP Sciences, under the terms of the Creative Commons Attribution License (https://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
The power spectral density of solarlike oscillations is expected to feature Lorentzian peaks centred on their eigenfrequencies. However, observations show that their line profiles are slightly asymmetric (Duvall et al. 1993). This asymmetry is primarily due to the fact that stochastic excitation occurs in a localised region just beneath the surface of the star. Several studies have consequently used observed line profile asymmetries to infer properties of the turbulent source of excitation of solar pmodes, in particular its radial position and its multipolar nature (see e.g. Roxburgh & Vorontsov 1997; Nigam et al. 1998). These prior studies used parametrised models, and aimed to find bestfit values for their free parameters by applying fitting procedures to individual peaks in the observed spectrum. Philidet et al. (2020) followed a different approach, which consisted in modelling mode asymmetry without fitting any free parameters to the available observational data. Instead, they developed an analytical model of stochastic excitation, coupled with a 3D hydrodynamical simulation of the stellar atmosphere. This allowed the authors to reproduce the asymmetries of solar pmodes as measured in the observed velocity power spectrum, and to subsequently demonstrate the role of the spatial extent of the mode driving region, together with the differential properties of turbulent convection (namely the variation of the injection lengthscale below and above the photosphere).
The recent measurement of pmode asymmetries in solarlike oscillators by Benomar et al. (2018), using Kepler observations, opened the way to constrain the properties of stochastic excitation, and therefore of turbulent convection, throughout the HR diagram. Unlike in the solar case, however, only observations made by Kepler in intensity have the resolution necessary for mode asymmetry to be inferred. But it is well known that asymmetries are very different between velocity and intensity observations (Duvall et al. 1993; Toutain et al. 1997). More precisely, line profiles in the velocity power spectrum have more power on their lowfrequency side, whereas line profiles in the intensity power spectrum have more power on their highfrequency side. This is known as the asymmetry reversal puzzle.
Several hypotheses have been proposed to explain this reversal, but no consensus has emerged. Duvall et al. (1993) suggested that modal entropy fluctuations could affect intensity asymmetries while leaving asymmetries in velocity unaffected. Following this argument, Rast & Bogdan (1998) quantified these nonadiabatic effects, and found that radiative cooling has a negligible impact on line profile asymmetry, so that it can hardly explain the asymmetry reversal. Gabriel (1998) then remarked that in order for such heat transfers to impact line asymmetry, it is necessary that they affect the wave equation beyond the second order, which was not the case in the model of Rast & Bogdan (1998).
Shortly afterwards, another candidate was found to explain the asymmetry reversal puzzle. Roxburgh & Vorontsov (1997) remarked that adding a coherent, nonresonant background (i.e. a signal with a very broad spectrum but whose Fourier component close to an oscillating mode would be coherent with it, and would therefore be able to interfere with it) to a resonant signal could affect its line profile, and thus its asymmetry. They argued that the overshooting of turbulent eddies into the lower layers of the atmosphere should act as a coherent nonresonant background in the velocity signal, while keeping the intensity signal unaffected, thus explaining the asymmetry reversal. On the other hand, Nigam et al. (1998) argued that both signals contain a coherent background component, and that the asymmetry reversal stems from the fact that it is much stronger in the intensity signal than in the velocity signal. Subsequently, several studies have undertaken the task of estimating the level of correlated background in the intensity signal using the observed asymmetry reversal (e.g. Kumar & Basu 1999; Chaplin & Appourchaux 1999; Severino et al. 2001; Barban et al. 2004).
Yet another candidate to explain asymmetry reversal was recognised by Georgobiani et al. (2003). They noticed that pmodes featured in the velocity and intensity power spectra of 3D hydrodynamic simulations of the stellar uppermost layers have opposite asymmetries when they are computed at fixed optical depth, but identical asymmetries when they are computed at fixed geometrical depth. They therefore proposed the following picture: the velocity and intensity line profiles are intrinsically proportional to one another, but the height of unity optical depth, at which the intensity fluctuations are observed, oscillates with the mode. Since there is a strong temperature gradient there, the observed background temperature also oscillates, which adds a component to the resonant intensity signal. They showed that this added component tends to reduce the amplitude of the intensity fluctuations. However, because the κ − T relation is highly nonlinear at the photosphere, this reduction is not uniform over the entire line profile, and thus it changes its asymmetry. Since there is no equilibrium velocity gradient, there is no corresponding additional component in the velocity signal, and the velocity asymmetry remains unaffected.
At the core of these models lies the assumption that the gas temperature at the photosphere and the effective temperature are equal, and therefore have equal relative fluctuations. This assumption means that the velocity and intensity line profiles should have the same asymmetry, so that the key to understanding the asymmetry reversal puzzle must be sought elsewhere. While this assumption is not problematic when it is used as a photospheric boundary condition in the framework of fully nonadiabatic calculations (Dupret et al. 2002), it becomes more questionable when used to justify that luminosity and temperature eigenfunctions are simply proportional to one another. In this context, our objective is to question this assumption, and to show that the radiative flux reacts in a more complex way to temperature variations, which has a crucial impact on line profile asymmetry in the intensity spectra. To this end, we extend the model of Philidet et al. (2020) for intensity observations. We show that, unlike previously thought, source localisation impacts velocity and intensity observations differently, so that an additional physical mechanism is not necessary to account for asymmetry reversal, except maybe at high frequency.
This paper is structured as follows. In Sect. 2 we describe the steps necessary for the adaptation of our model to intensity observations. We then present its predictions pertaining to asymmetry reversal in Sect. 3, and discuss these results in Sect. 4.
2. Modelling the intensity power spectrum
In order to adapt our pmode stochastic excitation model to intensity observations, it is first necessary to model the intensity Green’s function associated with radial pmodes. In Philidet et al. (2020), the wave equation was written in terms of a wave variable Ψ_{ω}, related to the velocity fluctuations through
where ρ is the equilibrium density, c is the sound speed, ω the angular frequency, j the imaginary unit. The notation refers to Fourier transform in time. The radial inhomogeneous wave equation then reads
where V(r) is the acoustic potential, Γ_{ω} is the frequencydependent damping rate of the oscillations, and S(r) is a source term proportional to the divergence of the fluctuating Reynolds stresses. The damping rates Γ_{ω} are inferred from observations; we use the same values as those presented in Table 1 of Philidet et al. (2020).
For a given value of ω, convolving the Green’s function in Eq. (2) with the source term S(r) allows us to predict the value of the power spectrum in terms of Ψ_{ω}. Then the velocity power spectrum is given by Eq. (1). Following the same approach, the goal of this section is to relate the intensity fluctuations to the wave variable Ψ_{ω}, so that from the Ψ_{ω} power spectrum we have access to the intensity power spectrum.
2.1. Intensity fluctuations in a grey atmosphere
Because the pmode intensity power spectrum is observed close to the photosphere, we only need to model the oscillationinduced intensity variations in this region. In order to model these variations, we treat the atmosphere as a grey atmosphere. This is justified, in part, by the fact that the observed intensity power spectrum corresponds to the continuum intensity, on which absorption spectral lines have little impact.
A grey atmosphere is, by definition, in radiative equilibrium. When studying pmodedriven intensity fluctuations, working under the radiative equilibrium assumption is justified by the large gap existing between the modal period and the local thermal timescale. The period of the modes is of the order of several minutes, while the thermal timescale is about ten seconds at the photosphere. As such, the radiative flux reacts almost instantly to the oscillations induced by the pmodes, and the atmosphere remains at radiative equilibrium at all times. One of the consequences of radiative equilibrium is that the radiative flux is uniform, and its relative fluctuations are proportional to the relative fluctuations of the effective temperature T_{eff}. The equality between the relative luminosity fluctuations at the photosphere and at the observation height of the modes is further supported by the fact that the modes are observed very close to the photosphere. The goal of the present section is therefore to relate the variations of T_{eff} to the gas fluctuations brought about by the oscillating modes, and in particular to the gas temperature fluctuations. In doing so, we follow the same treatment of pmodeinduced atmospheric perturbation as Dupret et al. (2002).
In a grey atmosphere, the temperature of the gas is given by a unique function of the optical depth τ and effective temperature T_{eff}, expressed by means of the Hopf function q(τ) (Mihalas 1978)
An arbitrary relation T = T(τ, T_{eff}) can be perturbed as
where the fluctuations of the optical depth can be expressed as
where κ is the Rosseland mean opacity and ξ_{r} the radial displacement of the gas.
Taking the partial derivative of Eq. (4) with respect to τ, and eliminating dδτ/dτ alternatively through Eqs. (4) and (5), we find
Isolating the perturbation of the effective temperature, this can be rearranged as
When the temperature law as given by Eq. (3) is used, Eq. (7) reduces to
where we have introduced
and ′ and ″ respectively refer to the first and second derivatives with respect to τ. The first term in the brackets can be rearranged as
Finally, using Eqs. (8) and (10), the fluctuations of the effective temperature can be written
The fluctuations in the effective temperature do not depend on τ, and therefore neither does the righthand side of Eq. (11), even though its individual terms do. The atmosphere being in radiative equilibrium, and the height of observation being fairly close to the photosphere, the radiative flux is uniform and equal to its value at the photosphere. This also holds true for the fluctuations of the radiative luminosity, which, by definition of the effective temperature, are therefore given by
which, thanks to Eq. (11), becomes
where we have introduced
Finally, we neglect the Lagrangian perturbations of the convective luminosity L_{C} compared to those of the radiative luminosity L_{R}. Including the convective contribution in this model would require a nonlocal, timedependent treatment of turbulent convection; furthermore, the oscillations would have to be treated in a nonadiabatic framework. Until subsequent refinements are made to this model, and as a first approximation, we therefore consider δL = δL_{R}, in which case we have
In the following we adopt a solarcalibrated Hopf function, which is based on a numerical solution to the nonLTE radiative transfer equation derived by Vernazza et al. (1981) to match the observed solar spectrum. This Hopf function is furthermore consistent with 3D hydrodynamic atmospheric simulations provided by CO^{5}BOLD, which we use to model the source term in Eq. (2). The Hopf function reads (see Sonoi et al. 2019)
In Fig. 1, we plot the quantity x(τ) against τ, where the Hopf function given by Eq. (16) is adopted. As expected, x(τ) is much smaller than unity at high optical depth. This is in accordance with the condition that the Hopf function must reduce to a constant in the deeper layers of the star. At lower optical depth, however, x(τ) is no longer negligible. The height of observation of the continuum intensity power spectrum (τ ∼ 2/3, vertical dashed line in Fig. 1) lies halfway between these two extreme cases; we therefore account for the quantity x(τ) in the following, even though it should not be of much significance.
Fig. 1.
Quantity x(τ) defined by Eq. (14) as a function of optical depth τ, when the Hopf function given by Eq. (16) is adopted. The vertical dashed line corresponds to the radius of the photosphere (τ = 2/3), where the intensity power spectrum is observed. The τaxis is oriented from left to right, so that the surface is on the left side of the figure, and the deeper layers on the right side. 
On a side note, comparing Eq. (15) to the perturbed radiative diffusion equation (see Eq. (21.15) of Unno et al. 1989)
it can be seen that the intensity fluctuations of a grey atmosphere with an arbitrary Hopf function q(τ) reduce to their diffusive counterpart when the following condition is met:
In particular, in the limit where the Hopf function is linear in τ (another common approximation in stellar atmospheres, leading to the widely used EddingtonBarbier relations, for instance), x(τ) strictly vanishes, and the luminosity fluctuations of the grey atmosphere are identical to the expression obtained in the diffusion approximation. We note, however, that this is only true of the fluctuating part of the luminosity. Even if x(τ) vanishes, the total luminosity of the grey atmosphere is not equal to the total luminosity obtained in the diffusion approximation.
2.2. Relating the intensity fluctuations to the Ψ_{ω} variable
Using the perturbed equation of state and the perturbed continuity equation, Eq. (15) can be rewritten in terms of fluid displacement and temperature fluctuations:
Here H_{T} ≡ dlnT/dr^{−1} is the temperature scale height, κ_{ρ} ≡ (∂lnκ/∂lnρ)_{T}, κ_{T} ≡ (∂lnκ/∂lnT)_{ρ}, and x is the value of the quantity x(τ), defined by Eq. (14), at the considered optical depth.
We can then write the temperature fluctuations as a function of fluid displacement. While it is known that nonadiabatic effects are important at the top of the convection zone, they are considerably complicated to account for in the treatment of solarlike oscillations (in particular, including them in this formalism would require going beyond the second order in Eq. (2)). As a first step we therefore choose to neglect their impact on pmode asymmetry, and we place ourselves in the quasiadiabatic approximation. Further discussion regarding the validity of this assumption can be found in Sect. 4.2. In this approximation, the relative temperature fluctuations are proportional to the relative density fluctuations, which are related to the fluid displacement through the perturbed continuity equation. In turn, the fluid displacement is related to the velocity variable through , and the velocity variable to the variable Ψ_{ω} through Eq. (1). This finally leads to
with
and
where ∇_{ad} is the adiabatic gradient and Γ_{1} is the gas adiabatic index.
Equation (20) shows that the intensity fluctuations cannot be described as being simply proportional to the wave equation variable Ψ_{ω}, but that they also depend on its first and second derivatives. It can be seen, for instance from the last two terms in the righthand side of Eq. (19), that this is because the radiative flux is sensitive to the temperature gradient. In prior studies tackling the issue of asymmetry reversal, it is always either explicitly argued, or implicitly assumed, that the Green’s function associated with intensity (or its pressure proxy) and velocity are proportional to one another (see e.g. Kumar & Basu 1999). This relation would, with the above notations, correspond to a case where only one of the coefficients A_{L}, B_{L}, or C_{L} is nonzero. In particular, synthetic spectrum models usually assume that the effective temperature fluctuations are equal to the actual temperature fluctuations, in which case only B_{L} ≠ 0 (see Sect. 4.1 for a more detailed discussion).
2.3. Intensity power spectral density
The remainder of the procedure is identical to the one detailed in Philidet et al. (2020). More precisely, to derive Ψ_{ω} we convolve the Green’s function G_{ω} and the source term S associated with the inhomogeneous wave equation (Eq. (2)). This is done by considering only the contribution of source localisation to the pmode asymmetries; in particular, we do not account for the contribution of correlated noise, although it was in our previous study. We also assume that the only source term in Eq. (2) stems from fluctuations of the turbulent pressure. Finally, using the resulting Ψ_{ω} in Eq. (20) leads to
where ⟨⟩ denotes ensemble average, and the function I_{ω} is defined as
where the Einstein convention on index summation is used for the indices i and j, the superscript star (^{⋆}) denotes complex conjugation, Re denotes the real part of a complex quantity, and X_{ω}, and are defined in terms of the Green’s function as
where the variables r_{o} and r_{s} in the Green’s function refer to the radius of observation and the radius of the source respectively. We note that the coefficients A_{L}, B_{L}, and C_{L} in Eq. (23) are only evaluated at the height of observation of the modes. This means, as we pointed out above, that we only need to model the oscillationinduced radiative flux variations at the photosphere, whereas the effect of the spatial extent of the source is entirely contained within the function I_{ω}. In particular, this is the reason why the value of the quantity x(τ) is only important at the height of observation (illustrated by the vertical dashed line in Fig. 1).
It is worth mentioning that Eq. (23) does not involve any further modelling than when the velocity power spectrum is calculated. Except for additional equilibrium thermodynamic quantities, both the Green’s function and the fourthorder correlation term in Eq. (24) were already modelled in Philidet et al. (2020). In other words, this means that modelling the contribution of source localisation to asymmetries in intensity does not require additional physical constraints, nor does it require new input parameters to be introduced, provided the nonadiabatic terms (not accounted for in this model) indeed remain small in the stellar superficial layers.
3. Results for intensity asymmetries and comparison with observations
3.1. Numerical computation of intensity asymmetries
The system comprised of (23) to (25) constitutes a closed, semianalytical form of the intensity power spectrum. The equilibrium quantities involved, as well as the turbulent quantities needed as inputs for the analytical model of turbulence, are all extracted from a 3D hydrodynamic simulation of the solar atmosphere computed using the CO^{5}BOLD code, which, after horizontal and time average, we patched on top of a 1D solar model provided by the evolutionary code CESTAM (for more details, see Manchon et al. 2018). Once the intensity power spectrum is calculated, we fit the obtained synthetic line profiles using the following formula (Nigam & Kosovichev 1998):
Here x = 2(ω − ω_{0})/Γ_{ω0} is the reduced pulsation frequency, ω_{0} the angular eigenfrequency, and Γ_{ω0} the linewidth of the mode. The parameter B corresponds to the asymmetry parameter. The terms positive and negative asymmetry refer to the sign of B, and in the special case B = 0 we recover a Lorentzian line profile.
In order to compare our results to observational data, we used the numerical spectrum model developed in Philidet et al. (2020). It contains only one parameter in the form of λ (see their Sect. 2.3.2 for a definition), which illustrates the relative uncertainty pertaining to the temporal spectrum associated with the turbulent cascade in the solar superficial layers. Physical arguments allow us to constrain the value of this parameter (see e.g. Samadi & Goupil 2001); to be consistent with these constraints, they retained the value λ = 0.5. This led to a satisfactory quantitative agreement between their model and observations in the velocity spectrum. Here, we retain the same value for λ, and compare the resulting intensity asymmetries to observations; there is therefore no parameter adjustment in what follows.
3.2. Observational datasets
To compare the asymmetries predicted by the model with observations, we use the same observational data as for the velocity power spectrum in Philidet et al. (2020). These data points were extracted from the spectrum analysis conducted by Barban et al. (2004) on observations made by the GONG network. We used these observations because they are particularly fitting for the study of asymmetry reversal; the GONG network provides velocity and intensity measurements simultaneously. We recall that the spectral analysis of Barban et al. (2004) considers nonradial modes (15 < l < 50), whereas our model was developed for radial modes. However, the dependence of asymmetry on angular degree is very weak, and the asymmetry observations collapse to a slowly varying function of frequency, so long as l ≲ 100 (see e.g. Vorontsov & Jefferies 2013) Therefore, the frequencydependence of asymmetry for the modes observed by GONG is expected to be almost identical to that of radial modes.
To obtain the asymmetries in the intensity spectrum, Barban et al. (2004) used approximately one year of GONG data, allowing us to resolve about 600 modes. Following Severino et al. (2001), they simultaneously fitted the velocity spectrum, intensity spectrum, and I–V cross spectrum (both coherence and phase difference), which is known to yield more reliable results. The observed asymmetries we used in velocity and intensity are not obtained independently, but through the same fitting procedure. The model used for the spectral analysis, however, considered that the asymmetry was entirely due to a coherent nonresonant background component, so that their results were presented in terms of noise level and phase differences. This is a different mathematical description for the same line profile shape as given by Eq. (26). In order to extract the asymmetry parameter B as defined by Eq. (26), we reconstructed the line profiles using the bestfit values obtained by Barban et al. (2004), and then fitted these reconstructed line profiles using Eq. (26) instead.
We also consider intensity asymmetries inferred from HMI observations, and extracted from the spectral analysis procedure described in Korzennik (2005). The asymmetry profile B(ν) resulting from this spectral analysis, while in agreement with the values inferred by Barban et al. (2004), shows less dispersion, and thus allows for a more robust comparison of our results with observations. The dataset used contains four periods of 72 days each. In Korzennik (2005) the asymmetries are already directly given in terms of a parameter α, which is easily related to the parameter B through B = α/2. We only considered angular degrees between l = 0 and l = 20, and we averaged the values of B over bins of width 30 μHz.
3.3. Modelled asymmetries compared with observations
Our model allows us to predict the mode asymmetries in both the velocity and intensity spectra simultaneously. However, since we focus on the results pertaining to the Sun’s velocity power spectrum in Philidet et al. (2020), in this paper we focus on the subsequent analysis of the Sun’s intensity power spectrum.
Figure 2 showcases the comparison between the asymmetries predicted by our model and those inferred from observations, both in velocity and intensity. It is clear that our model predicts a reversal of the asymmetries between these two observables, except for the higher order modes (ν ≳ 3.6 mHz). It is also clear that a quantitative agreement is found with observations for modes with ν ≲ ν_{max}, where ν_{max} ∼ 3 mHz is the frequency of maximum height in the pmode power spectrum. This shows that the localisation of the source, which is the primary cause of asymmetry in the velocity spectrum, is sufficient to explain a large portion of the asymmetry reversal.
Fig. 2.
Asymmetry profile B(ν) obtained by the numerical spectrum model with λ = 0.5, in the intensity power spectrum (solid red line) and in the velocity power spectrum (solid blue line). Both are compared to the asymmetry profile B(ν) inferred from observations by Barban et al. (2004) in the intensity (red crosses) and the velocity power spectra (blue crosses), respectively. The green crosses correspond to the asymmetry measured by Korzennik (2005) in the intensity power spectrum. 
However, our model fails to account for the intensity asymmetry of the higher order modes, with ν ≳ ν_{max}. While it consistently predicts slightly negative asymmetries for these modes, observations tend to show that they actually feature strong positive asymmetry. This shows that other mechanisms must be invoked to fully explain the asymmetry reversal throughout the entire pmode spectrum. For instance, unlike the velocity power spectrum, our intensity power spectrum model does not contain the contribution of the correlated background. It is widely thought that this contribution is negligible in velocity data; in turn, the results presented in Fig. 2 indicate that it is also negligible in intensity data for lowfrequency modes, but that it may no longer be the case for highfrequency modes. Furthermore, the nonadiabaticity of the oscillations is not taken into account in our study; we discuss this approximation in Sect. 4.2. The opacity effect, as it was called by Severino et al. (2008), could also play a role. Finally, the fluctuations of the convective flux may add a nonnegligible contribution to the total intensity fluctuations, whereas we only considered the fluctuations of the radiative flux in Eq. (17). The relative importance of both kinds of fluxes depends on the height at which the modes are observed. In particular, the higher the radius of observation, the more prominent the radiative flux.
4. Discussion
4.1. Understanding the asymmetry reversal puzzle
As already mentioned in Sect. 2, the reason why source localisation leads to different asymmetries in the intensity and velocity power spectra is the fact that the relation that links the intensity fluctuations to the velocity fluctuations (or, equivalently, to the variable Ψ_{ω}) is not a simple linear relation, but involves its first and second derivatives as well. As we also mentioned above, this is because the radiative flux depends primarily on the temperature gradient, and not only on the absolute value of the temperature. There can be partial cancellation between the three terms on the righthand side of Eq. (20), leading to line profiles that are not simply proportional to each other.
In contrast, using simpler approximations to model the intensity fluctuations leads to much simpler relations between δL/L and v_{osc}, which, precisely because of their simplicity, are unable to predict any asymmetry reversal. In the following we illustrate this by considering that δT_{eff}/T_{eff} = δT/T at the photosphere. In that simple case the intensity fluctuations can be written
It is readily shown that the second term on the righthand side of Eq. (27) is negligible for solar pmodes close to the surface. In turn, the temperature fluctuations are, in the quasiadiabatic approximation, proportional to the pressure fluctuations. In this simple model pressure fluctuations are therefore a suitable proxy for intensity fluctuations. Then, using the perturbed continuity equation, the intensity fluctuations are related to the variable Ψ_{ω} through a relation similar to Eq. (20), but with
We compare in Fig. 3 the velocity and intensity asymmetry profiles B(ν) obtained when the relation δT_{eff}/T_{eff} = δT/T is adopted at the photosphere. As can readily be seen, the asymmetries are not reversed. This is because in this simplified model only one term is retained in the relation between the two types of fluctuations.
Fig. 3.
Predicted asymmetry profiles B(ν) when the relation δT_{eff} = δT is assumed. The solid red line shows the velocity asymmetries (since they are unaffected by the intensity fluctuation modelling, it is identical to the solid blue line in Fig. 2). The dashed red line corresponds to the intensity asymmetries obtained by using Eq. (27) in place of Eq. (20). 
The relation between the intensity and velocity Green’s functions is therefore a crucial key to tackling the issue of asymmetry reversal. In many studies on the subject, various approximations were made to model this relation. For instance, when dealing with asymmetry reversal, Duvall et al. (1993) split the wave variables into dynamical variables, such as velocity, and thermal variables, such as temperature or brightness. They then implicitly consider that each set of variables is characterised by one Green’s function, and in particular that temperature and intensity fluctuations are proportional to one another, which is analogous to Eq. (27). Adopting Eq. (27), as shown by Dupret et al. (2002), does not substantially alter predictions regarding intensity fluctuations, provided temperature fluctuations are described in a fully nonadiabatic framework. However, the use of a simple Newton’s cooling law to model nonadiabaticity renders it invalid. Rast & Bogdan (1998), Nigam et al. (1998), Kumar & Basu (1999) made similar assumptions regarding the intensity fluctuations, all of which are equivalent to considering the approximation δT_{eff}/T_{eff} = δT/T, without the necessary nonadiabatic framework.
On the other hand, Roxburgh & Vorontsov (1997) used the same Green’s function for velocity and intensity, but considered different source terms. More specifically, they added a frequencyindependent source term for the velocity fluctuations, which they did not consider for the intensity fluctuations. In other words, they considered that the only difference between the velocity and intensity fluctuations is the addition of a coherent, nonresonant background component in the velocity signal. Likewise, in Chaplin & Appourchaux (1999), the authors considered proportional Green’s functions for velocity and intensity. All these assumptions are equivalent to considering that the coefficients B_{L} and C_{L} in Eq. (20) are zero, thus only retaining the coefficient A_{L}.
Prior studies on asymmetry reversal thus have this in common; they use simplifying approximations to model the intensity fluctuations, so that their equivalent of Eq. (20) only contains one nonvanishing coefficient (either A_{L} or B_{L}, depending on the authors). This is the reason why, in their models, source localisation alone was not able to explain the different sense of asymmetry observed in velocity and intensity.
4.2. Quasiadiabatic approximation
As we mentioned above, our model describes the oscillations in the quasiadiabatic framework, in the sense that, in establishing the wave equation given by Eq. (2), we neglect all heat transfers, both in the homogeneous part (the full, nonadiabatic wave equation is of fourth order, whereas ours is only secondorder) and in the source term (we only considered mechanical work exerted by fluctuations of the turbulent pressure, and left out the effect of turbulent entropy fluctuations). As pointed out by Gabriel (1998), increasing the order of the wave equation is likely to cause asymmetries in different observables to drift further apart. Thus, in order to predict the shape of the mode line profiles as realistically as possible, one should go beyond the quasiadiabatic approximation and perform fully nonadiabatic computations. However, as a first step, we adopted this approximation in this study.
The quasiadiabatic approximation is notoriously questionable in the superficial layers of solarlike oscillators, and more specifically in the superadiabatic region (Samadi et al. 2015; Houdek & Dupret 2015), because the thermal timescale over which heat transfers typically occur in this region is neither much smaller, nor much greater than the period of the oscillations, but rather coincide with it. Thus, modal entropy fluctuations are nonzero, and should, in a fully nonadiabatic framework, be included in the equation of state along with their corresponding evolution equation. The difference is seen, for example, in the phase difference between velocity and intensity modal fluctuations; while the quasiadiabatic approximation yields a phase difference of π/2 between the two, the observed phase difference varies significantly with frequency (Barban et al. 2004).
Therefore, in adopting the quasiadiabatic approximation, we do not overlook its shortcomings, but rather consider this a first step to a novel approach, which is still likely to shed light on the issue of asymmetry reversal. The impact of nonadiabaticity is perhaps best illustrated with mode amplitudes. In discarding modal entropy fluctuations from the oscillation model, predicted intensity amplitudes are severely overestimated compared to their observed counterparts.
This is illustrated in Fig. 4, where we show the amplitudes predicted by our model as well as the observed solar mode amplitudes, both for velocity and intensity. Predicted mode amplitudes are accessed from the same fitting procedure described in Sect. 3; the amplitude squared of a mode indeed corresponds to the area under the curve of its spectral power density, and is therefore given by
Fig. 4.
pmode amplitudes A, as defined by Eq. (29), as a function of mode frequency ν. The legend is identical to that of Fig. 2: crosses correspond to amplitudes inferred from observations, using the spectral analysis of Barban et al. (2004) (each cross represents an individual doublet (n, l)), whereas solid lines correspond to the prediction of our model; blue element pertain to velocity, red elements to intensity. The amplitudes are given in m.s^{−1} for velocity, and in ppm for intensity. 
where A is the mode amplitude and Γ_{ω} its linewidth, and H_{0} is defined by Eq. (26). We note that mode amplitudes defined in this way are intrinsic amplitudes, and do not account for visibility factors. As for the observed amplitudes, we use the results of the same spectral analysis conducted by Barban et al. (2004) that we used to compare asymmetries in Sect. 3.
It can be seen from Fig. 4 that while our model reproduces the amplitudes in velocity to a satisfactory extent, the intensity amplitudes are overestimated by an order of magnitude (approximately a factor of 5). In particular, it appears that the overestimation factor only slightly depends on frequency. This overestimation is a known shortcoming of the quasiadiabatic approximation, whose alleviation, as we mentioned above, would require going beyond a secondorder wave equation. We note, however, that simply because nonadiabatic effects have an important impact on mode amplitude does not mean that the impact on asymmetries is as critical. Asymmetries are only sensitive to differential, frequencydependent alterations of the line profiles, and remain unchanged under an overall reduction factor. An alternative approach would be to obtain an equivalent of Eq. (11) by replacing δτ/τ in Eq. (4) by its integral expression obtained through Eq. (5). Since this method does not rely on τderivatives, it is likely to be less affected by departure from adiabaticity; however, the integral form of δτ/τ renders the resulting equivalent of Eq. (23) impractical to use.
5. Conclusion
In this paper we extended the semianalytical synthetic power spectrum model developed in Philidet et al. (2020) to predict the radial pmode asymmetries in intensity observations. We treated the pmodeinduced fluctuations of the radiative flux by perturbing a grey atmosphere model with a solarcalibrated Hopf function. We showed that the dependence of the radiative flux on the temperature gradient, and not simply on the absolute value of the temperature, has a profound impact on the shape of the line profiles in the intensity spectrum. We find quantitative agreement between our predicted asymmetries and the corresponding observations for lowfrequency modes, both in velocity and intensity simultaneously. We conclude that no secondary physical mechanism is necessary to explain the reversal between asymmetries in velocity and intensity, at least for ν ≲ ν_{max}.
Our model is unable, however, to explain asymmetry reversal for higher order modes. Secondary mechanisms can be invoked there. The nonadiabatic effects invoked by Duvall et al. (1993), the correlated background effect invoked by Nigam et al. (1998), and the impact of the convective flux fluctuations are all viable candidates. The fact that these discrepancies are restricted to highfrequency modes in intensity suggests that nonadiabaticity is at least partly responsible. As a concluding remark, we point out that radiative transfers, even if they are not sufficient to reverse asymmetries at the highfrequency end of the pmode spectrum, still have a significant impact on the line profiles. As a result, in investigating the impact of any other physical mechanism on asymmetry reversal, this intrinsic difference between velocity and intensity line profiles must still be accounted for.
The main limitation of the model presented in this study is the quasiadiabatic approximation, which is not valid in the superficial layers of the star. Although it sheds some light on the asymmetry reversal problem, any further improvement of this model will therefore need to go beyond this approximation and consider a nonadiabatic wave equation instead. We postpone this refinement to a later study.
Acknowledgments
The authors wish to thank the anonymous referee for his/her useful comments, which helped considerably improve this manuscript. J.P, K.B and R.S acknowledge financial support from the “Programme National de Physique Stellaire” (PNPS) of CNRS/INSU and from the “Axe Fédérateur Etoiles” of Paris Observatory. H.G.L. acknowledges financial support by the Sonderforschungsbereich SFB 881 “The Milky Way System” (subprojects A4) of the German Research Foundation (DFG).
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All Figures
Fig. 1.
Quantity x(τ) defined by Eq. (14) as a function of optical depth τ, when the Hopf function given by Eq. (16) is adopted. The vertical dashed line corresponds to the radius of the photosphere (τ = 2/3), where the intensity power spectrum is observed. The τaxis is oriented from left to right, so that the surface is on the left side of the figure, and the deeper layers on the right side. 

In the text 
Fig. 2.
Asymmetry profile B(ν) obtained by the numerical spectrum model with λ = 0.5, in the intensity power spectrum (solid red line) and in the velocity power spectrum (solid blue line). Both are compared to the asymmetry profile B(ν) inferred from observations by Barban et al. (2004) in the intensity (red crosses) and the velocity power spectra (blue crosses), respectively. The green crosses correspond to the asymmetry measured by Korzennik (2005) in the intensity power spectrum. 

In the text 
Fig. 3.
Predicted asymmetry profiles B(ν) when the relation δT_{eff} = δT is assumed. The solid red line shows the velocity asymmetries (since they are unaffected by the intensity fluctuation modelling, it is identical to the solid blue line in Fig. 2). The dashed red line corresponds to the intensity asymmetries obtained by using Eq. (27) in place of Eq. (20). 

In the text 
Fig. 4.
pmode amplitudes A, as defined by Eq. (29), as a function of mode frequency ν. The legend is identical to that of Fig. 2: crosses correspond to amplitudes inferred from observations, using the spectral analysis of Barban et al. (2004) (each cross represents an individual doublet (n, l)), whereas solid lines correspond to the prediction of our model; blue element pertain to velocity, red elements to intensity. The amplitudes are given in m.s^{−1} for velocity, and in ppm for intensity. 

In the text 
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