Testing gravity with galaxy-galaxy lensing and redshift-space distortions using CFHT-Stripe 82, CFHTLenS and BOSS CMASS datasets

The combination of Galaxy-Galaxy Lensing (GGL) and Redshift Space Distortion of galaxy clustering (RSD) is a privileged technique to test General Relativity predictions, and break degeneracies between the growth rate of structure parameter $f$ and the amplitude of the linear power-spectrum $\sigma_8$. We perform a joint GGL and RSD analysis on 250 sq. degrees using shape catalogues from CFHTLenS and CFHT-Stripe 82, and spectroscopic redshifts from the BOSS CMASS sample. We adjust a model that includes non-linear biasing, RSD and Alcock-Paczynski effects. We find $f(z=0.57) =0.95\pm0.23$, $\sigma_8(z=0.57)=0.55\pm0.07$ and $\Omega_{\rm m} = 0.31\pm0.08$, in agreement with Planck cosmological results 2018. We also estimate the probe of gravity $E_{\rm G} = 0.43\pm0.10$ in agreement with $\Lambda$CDM-GR predictions of $E_{\rm G} = 0.40$. This analysis reveals that RSD efficiently decreases the GGL uncertainty on $\Omega_{\rm m}$ by a factor of 4, and by 30\% on $\sigma_8$. We use an N-body simulation supplemented by an abundance matching prescription for CMASS to build a set of overlapping lensing and clustering mocks. Together with additional spectroscopic data, this helps us to quantify and correct several systematic errors, such as photometric redshifts. We make our mock catalogues available on the Skies and Universe database.


Introduction
Since its inception, general relativity theory (GR) has been constantly tested, starting with observations in the solar system and in our Galaxy (see e.g. Damour 2000). At cosmological scales, the advent of wide field survey experiments currently yields very high precision measurements in both the early and late ages of the universe. A Universe dominated by cold dark matter and a cosmological constant in the context of GR (hereafter ΛCDM−GR model) reproduces all these observations with very high accuracy and for this reason, the model is often referred to as the standard reference model. The catalogues are available at the CDS via anonymous ftp to cdsarc.u-strasbg.fr (130.79.128.5) or via http://cdsarc. u-strasbg.fr/viz-bin/qcat?J/A+A/627/A137 and at http:// www.skiesanduniverses.org However, some slight tensions are emerging between predictions based on the cosmic microwave background measurements from the Planck mission at redshift z = 1089 and measurements at redshifts z < 1 obtained from galaxy clustering or gravitational lensing. In particular with Planck, the amplitude of the matter power spectrum σ 8 is larger and the Hubble constant H 0 is smaller than what is estimated at redshifts z < 1 at about 2σ confidence level (C.L.; Planck Collaboration XIII 2016; Beutler et al. 2014;Alam et al. 2017;Hildebrandt et al. 2017;DES Collaboration 2018). Although systematic errors in the analyses can explain a significant fraction of these discrepancies, they might nonetheless suggest some issues with our understanding and modelling of the expansion of the Universe, or of the large-scale structure formation probed by galaxy clustering and gravitational lensing.
The common approach to test ΛCDM−GR at cosmological scales is either to measure the expansion history H(z) of the Universe (e.g. Betoule et al. 2014;Alam et al. 2017;Magaña et al. 2015), or to measure the growth of structures traced by the velocity or density fields in redshift space (e.g. de la Torre et al. 2013;Tully et al. 2016;Martinet et al. 2018). In this paper, we combine galaxy-galaxy lensing (GGL) and RSD to test both aspects simultaneously at redshift z = 0.57. The amplitude of GGL measurements is sensitive to H(z) and the density field, whereas RSD probes the growth of structure f (z) through galaxy peculiar velocities. The combination of these two observables has demonstrated its effectiveness at isolating the independent effects of the growth rate of structure f (z), the amplitude of the matter power spectrum σ 8 , and the dark energy equation of state parameter w involved in H(z) calculation (Simpson et al. 2013;de la Torre et al. 2017;Joudaki et al. 2017). Zhang et al. (2007) proposed an alternative method to test deviations to GR. Assuming small scalar perturbations around the Friedmann-Lemaître-Robertson-Walker metric (FLRW) in the conformal Newtonian gauge ds 2 = −a(τ) 2 [1 + 2Ψ]dτ 2 + a(τ) 2 [1 − 2Φ]dx 2 , where a is a scale factor, τ is the conformal time, and x are comoving coordinates, these authors proposed a statistics E G sensitive to the gravitational slip between the two gravitational potentials Φ and Ψ as follows: where all quantities are estimated at the redshift of interest. Reyes et al. (2010) proposed an associated observational estimator E G = Υ gm /βΥ gg (see below in Sect. 6.4), which converges to E G in the large-scale limit where the galaxy bias b and the distortion parameter β = f /b converge to constant values. The small-scale filtered galaxy-matter cross-correlation Υ gm probed with GGL is sensitive to both b and ∇ 2 (Φ − Ψ) since photons traverse equal quantity of space and time. The galaxy-velocity cross-correlation βΥ gg probed with RSD is sensitive to galaxy bias and the Newtonian potential Ψ. In GR and in absence of anisotropic stress, Φ = −Ψ so lensing is sensitive of 2∇ 2 Φ. In the linear regime, the Poisson equation relates the potential to the matter density contrast δ, such that ∇ 2 Φ = −∇ 2 Ψ = 3 2 Ω m0 H 2 0 a −1 δ. This estimator therefore converges to E G = Ω m0 f in the standard model. In their seminal paper, Zhang et al. (2007) predicted deviations from GR with four alternative models: ΛCDM, flat (Dvali et al. 2000, hereafter DGP), f (R) gravity , and TeVeS/MOND (Bekenstein 2004). Apart from the TeVeS/MOND model, which introduces a wavelength difference between dynamical and lensing power-spectra, all other models add at most 10% deviations compared to GR predictions. Leonard et al. (2015) reached similar conclusions with other models based on the empirical extension of the Poisson equations with the commonly used parameters Σ(a) and µ(a) (Amendola et al. 2008;Ferreira & Skordis 2010). Most importantly, these authors found that details of the analysis (e.g. integration length along the line of sight for projected estimators) could mimic deviations similar to those predicted with alternative models of gravity, thus the need for a careful study of these biases. In any case with 20%-30% precision, current datasets are not yet at the level of accuracy required to observe these deviations, and unsurprisingly no deviation to GR predictions has been detected so far (Blake et al. 2016;Pullen et al. 2016;de la Torre et al. 2017;Alam et al. 2017;Amon et al. 2018).
Nowadays, cosmological analyses require measurements with exquisite control of systematic errors, at all levels from data acquisition to cosmological model inference. The wide range of expertise needed to reach the requirements is demonstrated by the size of the on-going and forthcoming cosmological experiments such as Dark Energy Survey (Dark Energy Survey Collaboration 2005), the Kilo Degree Survey (Hildebrandt et al. 2017), the Hyper-Suprime Cam survey (Aihara et al. 2018), the extended Baryonic Oscillation Sky Survey (Dawson et al. 2013), the Prime Focus Spectrograph project (Sugai et al. 2012), the Dark Energy Survey Instrument project (DESI Collaboration 2016a,b), the Large Scale Synoptic Telescope (LSST Dark Energy Science Collaboration 2012), and the Euclid mission Laureijs et al. (2011).
In this paper, we extend the Leauthaud et al. (2017) analysis (hereafter L17), by adding RSD measurements of CMASS galaxies from the Baryon acoustic Oscillation Spectroscopic Survey (BOSS) to GGL measurements in the CFHT-Stripe 82 and CFHT-LS fields. Thanks to refined simulations, we precisely quantify systematic errors, and thus manage to reconcile real and simulated measurements of clustering and lensing. The work presented builds on the theoretical model and joint RSD and GGL analysis developed in de la Torre et al. (2017, hereafter DLT17).
The outline of the paper is as follows. First we present our galaxy bias model, and its inclusion in standard clustering and lensing estimators. Next, we present our datasets and measurement estimators. Our tests on simulations are presented in Sect. 5, and our estimates of the cosmological parameters in Sect. 6. Finally, we present our measurement of E G and conclude. Systematic errors are discussed in the Appendix. Unless otherwise mentioned, we express the GGL projected densities Σ gm and distances in comoving coordinates. We assume the fiducial ΛCDM−GR cosmology with flat universe, Ω m = 0.31, h = 0.6777, Ω b = 0.048, σ 8 = 0.82 (Planck Collaboration XIII 2016).

Method
In the following, we compute the RSD two-point galaxy correlation functions in configuration space. We decomposed the three-dimensional galaxy separation vector s into polar (s, µ) or Cartesian (r p , π) coordinates in the frame defined by the line of sight and the normal to it, where s is the norm of s, µ is the cosine of the angle between s and the line of sight, π and r p are the projections of s on the line of sight and its normal, respectively. In the flat-sky approximation, the transformation between Cartesian and polar coordinates is µ = π/s, r p = √ s 2 − π 2 (Fisher et al. 1994). Conversely, the GGL formalism is defined in real space, where the separation vector r is decomposed into Cartesian coordinates (R, χ), where χ and R are the projections of r on the line of sight and its normal, respectively. In GGL, the radial window function of integration is hundreds of h −1 Mpc, and the effects of RSD can safely be neglected (Baldauf et al. 2010). Hereafter, we assume that R in the model corresponds to r p in the observations.

Galaxy bias model
In this work, we want to measure the growth rate f and amplitude of the matter power spectrum σ 8 with GGL and galaxy-clustering measurements. These measurements are not typically estimated at the same scale. While the GGL signal typically emerges in the range of transverse distances 0.1 < r p < 20 h −1 Mpc, the galaxy clustering signal rises between 10 < r p < 100 h −1 Mpc. To maximize the overlap between these two observables in the non-linear regime, we adopted the fourth order perturbation model in the initial density field as proposed by McDonald & Roy (2009). Assuming homogeneity and isotropy in the density field, they derived the following expression for the halo-matter power spectrum: where P δδ and P lin represent the non-linear and linear matter power spectra respectively; P b 2 ,δ and P b s 2 ,δ are the one-loop power spectra between the density field δ, its derivative and the variance of the tidal tensor field s(x). The term b 3nl σ 2 3 (k) includes various third order terms of the galaxy bias model (see McDonald & Roy 2009, for more details). Assuming coevolution between the halo and matter density fields, and the bias being purely local in Lagrangian space at initial conditions, Baldauf et al. (2012) computed the second order halo density field in both Eulerian and Lagrangian space and found the relation b s 2 = −4/7(b 1 − 1). Under the same assumptions as above to compute b s 2 , Saito et al. (2014) obtained the relation b 3nl = 32/315(b 1 − 1). The analytical expressions for all these terms are given in Appendix A of DLT17.

Galaxy-galaxy lensing model
The measured GGL differential excess surface density is defined as where the mean projected surface density can be read as and Σ gm (R) is the projected surface density defined as a function of the galaxy-matter cross-correlation function (Dvornik et al. 2018) where the mean matter density ρ m = Ω m ρ c = 3Ω m0 H 2 0 /8πG is constant in comoving coordinates. The galaxy-matter crosscorrelation function ξ gm is obtained from the Fourier transform of the galaxy-matter power spectrum P gm (k) defined above.
In practice, we used an FFTLog unbiased Hankel transform with parameter µ = 1 2 in logarithmic space to perform the Fourier transform 1 . We truncated the power spectrum at k min = 10 −5 and k max = 1000 to minimize cut-off aliasing during the FFT operation, and we spline-interpolated the resulting correlation function to obtain the desired binning.

Redshift space distortions model
In this work, we used the Taruya et al. (2010) model to describe the RSD effect. In the ideal case in which galaxies are perfect tracers of the matter density field, this model takes the form where θ is the divergence of the velocity field defined as θ = −∇·v/(aH f ). The values P δδ , P θθ , and P δθ are the non-linear matter density, velocity divergence, and density-velocity divergence power spectra, respectively; C A (k, µ, f ) and C B (k, µ, f ) terms derive from the general anisotropic power spectrum of matter and their expressions are given in Taruya et al. (2010) and de la Torre & Guzzo (2012). The damping function D(kµσ v ) essentially (but not only) describes the Fingers of God effect on the two-point correlation function, and we modelled it as a Lorentzian damping in Fourier space, i.e.
where σ v represents an effective pairwise velocity dispersion that we fitted for and then treated as a nuisance parameter. This model can be generalized to the case of biased tracers, by including our bias model. Hence, we obtain (Beutler et al. 2014;Gil-Marín et al. 2014) where, In the above equations P b 2 ,δ , P b s 2 ,δ , P b 2 ,b 2 , P b 2 ,b s 2 , P b s 2 ,b s 2 and σ 2 3 (k) are one-loop integrals, of which analytical expressions can be found in Appendix A of DLT17. We computed the linear matter power spectrum P lin using the class Bolzmann code (Lesgourgues 2011), and the non-linear matter power spectrum P δδ using the semi-analytic prescriptions HALOFIT (Smith et al. 2003;Takahashi et al. 2012). To predict the velocity spectra P θθ and P δθ , we use the nearly universal fitting functions from Bel et al. (2019), already used in DLT17 and Pezzotta et al. (2017). These are built such that they converge to P lin at large scales, but reproduce non-linearities at small scales. Pezzotta et al. (2017) highlighted that adding a redshift dependency with σ 8 (z) such that and was helping. The coefficients (p 1 = 1.906, p 2 = 2.163, p 3 = 2.972, p 4 = 2034) were deduced from a fit to measurements performed on the DEMNUni simulations (dark energy and massive neutrino universe). These two fitting functions are accurate within 5% to the measurements in simulations and appear to be insensitive to the presence of neutrinos (Carbone et al. 2016).
The overall degree of non-linearity in these terms is therefore solely controlled by σ 8 (z), which is left free when fitting the model to observations. Although these fitting functions possibly duplicate a fraction of the high-order modes included in the perturbation theory model above, we demonstrate in DLT17 and in Sect. 5 below that it does not bias significantly our cosmological estimates given data uncertainties.
Finally, we obtain the multipole moments of the anisotropic correlation functions in configuration space where j (x) is the spherical Bessel function and P s (k) is the anisotropic power-spectrum multipole moment of order defined as where L (x) are the Legendre polynomial of order .
At linear scales, f and σ 8 are degenerate, but extending to non-linear scales with the Taruya et al. (2010) 8 , and f 3 σ 4 8 appear in the calculation of the correction terms C A and C B , and hence help break the degeneracy. Accordingly, in our model ( f , b 1 , b 2 , σ v , σ 8 ) are treated as separate parameters in the fit (de la Torre & Guzzo 2012).

Spectroscopic redshift uncertainties
It is worth mentioning that redshift errors can potentially affect the anisotropic RSD signal. They have the same effect as galaxy random motions in virialized objects. We model the redshift errors by multiplying the anisotropic power spectrum by the Fourier transform of a Gaussian damping function of the form such that our predicted signal can be finally written as Bolton et al. (2012) measured the error on the estimated spectroscopic velocities, thanks to multiple observations of the same CMASS galaxies, and found approximately δ v = 32 km s −1 , which translates to σ z = 0.797 h −1 Mpc in comoving distances at redshift z = 0.57 with our fiducial cosmology. This effect is therefore negligible, but we included it to have a cleaner estimate of σ v .

Suppressing small-scale modelling uncertainties
Although considered as sufficient for galaxy-clustering analysis, we find that our weak-lensing (WL) model deviates from our measurements with simulated data at scales r p ∼ 3 h −1 Mpc (see Fig. 7 in DLT17). In order to damp the contribution of any signal below a given cut-off radius R 0 , we computed the annular differential excess surface density (ASAD) estimator from the data (Baldauf et al. 2010). For the lensing observable ∆Σ gm (r p ), it is given by and for the galaxy clustering These two estimators become useful to estimate E G in the following. We derive the projected correlation w p (r p ) from the projection of the multipole decomposition of the correlation function in redshift space ξ s (s) The α 2 coefficients are given in Baldauf et al. (2010) We integrate along the line of sight up to π max = 40 h −1 Mpc to match the integration length used with the data (see the estimators Sect. 4.2). According to Singh et al. (2019), they found consistent results whether they use π max = 50 h −1 Mpc or 100 h −1 Mpc. Given the low number CMASS galaxies in this analysis, we set π max = 40 h −1 Mpc to minimize the noise.
The ASAD can also be predicted from theory. For the lensing part, Υ gm (r p , R 0 ) is obtained by filtering the cross-correlation function ξ gm (r) with the window function W Υ (x, r p , R 0 ) (Baldauf et al. 2010) defined as where Θ(x) is the Heaviside step function. In a similar manner, we computed Υ gg (r p , R 0 ) by simply replacing ξ gm (r) by ξ gg (r) in Eq. (23). We included the RSD effect in the calculation of Υ gg (r p ). In both cases, we integrated in logarithmic scale up to r max = 100 h −1 Mpc. We note that we do not include intrinsic alignment in our modelling. This choice is motivated by the marginal constraints obtained in Joudaki et al. (2017) on the amplitude of this effect A IA = 1.67 +0.50 −0.49 , with small-scale cut on γ t at θ > 12 arcmin. Since we applied the small-scale Υ filter, we anticipate very little constraint on this parameter as well, at a significant additional computing cost.

Alcock-Paczynski effect
We may mention that additional distortions can occur in the correlation functions owing to possible differences between the true and the fiducial cosmological models used to compute the distances. This effect was first identified by Alcock & Paczynski (1979; hereafter AP) as a means to constrain the cosmological model. However these distortions degenerate with the RSD effect and considerably limit the constraining power of the AP effect (Ballinger et al. 1996;Matsubara & Suto 1996).
Fortunately, the scale-dependence of the AP and RSD effects differ and thus allow us this degeneracy to break (Seo & Eisenstein 2003;Blake et al. 2011;Chuang & Wang 2012).
In this work, we adopted the AP model proposed by Xu et al. (2013). The isotropic and anisotropic distortions are expressed respectively as where quantities computed with the fiducial cosmology as denoted with primes. Those parameters modify the transverse and the radial distances such that Given these distortions, the observed redshift-space monopole and quadrupole expressed in configuration space become The GGL estimator becomes

Data
In our GGL analysis, the lenses are the CMASS galaxies and the sources are galaxies in the CFHTLens and CFHT-Stripe 82 WL catalogues. Lenses have spectroscopic redshifts and sources have photometric redshifts. For each lens, we can then discard all uncorrelated foreground sources and use the background sources to estimate the lensing signal. The final GGL measurement is the average of the signals for each lens.

CFHTLens catalogue
In 2013, the CFHTLenS team released a public WL catalogue covering an area of 154 sq. deg in four wide fields (W1, W2, W3, and W4; Erben et al. 2013;Heymans et al. 2012). So far, the depth of the input CFHT Legacy Survey imaging is unrivaled, with a 5σ point source limiting magnitude i AB ∼ 25.5. The lensfit algorithm is used to measure the shape of every object detected with i AB < 24.7. Then, we selected galaxies with good shape measurements (fitclass = 0 and weight > 3). We obtained photometric redshifts from five optical band photometry u, g, r, i, z and reach a precision of about 5% up to z ∼ 1 (Hildebrandt et al. 2012). Galaxy-galaxy lensing measurements can be significantly biased by inaccurate photometric redshifts (Nakajima et al. 2012). We computed the photometric redshift bias estimator b z , based on spectroscopic and photometric catalogues matched in position, and averaged over the CMASS redshift distribution (see appendix details). Since the spectroscopic calibration sample is significantly shallower than the photometric sample, we discarded galaxies fainter than the 90% completeness limit of the spectroscopic sample (see below), i.e. we only kept galaxies brighter than i AB < 24. After this selection, we obtained b z = +0.003 ± 0.003, b z = −0.014 ± 0.004 and b z = +0.022 ± 0.003 in fields W1, W3, and W4, respectively. We discarded field W2 because it only contains 200 CMASS galaxies on its northern edge.
Our final catalogue contains 3.5 millions galaxies over an effective area of about 127 sq. deg. The galaxy density 2 is n eff = 7.0 galaxies arcmin −2 . The median redshift is z med = 0.70.  Gunn et al. 2006) stripe 82 region, with a 5σ point-source magnitude limit i AB ∼ 24.1, and a mean seeing of 0.6 . The effective area is 129.2 sq. deg after masking out bright stars and other image artefacts (L17). We used a new version 3.0 of the shape catalogue that has shapes measured with lensfit down to magnitude i AB < 24.7. This new version benefits from internal calibration in lensfit based on image simulations inherited from the CFHTLenS project. Shape measurements are accurate at the 2% level, without relying on any additional linear correction. In addition, this new catalogue contains about 40% more galaxies, mostly because of a better handling of galaxy de-blending and instrument artefacts in lensfit (L. van Waerbeke, priv. comm.).

CFHT-Stripe 82 catalogue
Photometric redshifts in the original version of the catalogue (Bundy et al. 2015) were computed with BPZ (Benítez 2000) using ugriz from the Stripe 82 co-adds (Annis et al. 2014) and U JHK from UKIDSS. We use nearest-neighbour interpolation in sky coordinates, i magnitude, and g − r, r − i, i − z colour space to get photometric redshifts for the new galaxies. We verified that the redshift distribution is unchanged. We applied the same procedure as in the CFHTLS fields to estimate the bias due to photometric redshifts in our GGL measurements. However, given the relatively shallow spectroscopic survey coverage of the CS82 field compared to CFHTLS fields (90% completeness reached at i AB = 22.5), we are forced to select galaxies only down to i AB < 22.5. Although this cut is quite severe, it allow us to confidently model and correct photometric redshift bias in this field. The lack of deeper spectroscopic information prevents us from exploiting the complete WL catalogue. For i AB < 22.5 sources and CMASS lenses, we find a bias b z = −0.028 ± 0.006. In contrast to L17, we apply no cut based on the odd quality flag because we find it has no impact on our lensing measurements given our stringent cut in magnitude. Our final catalogue contains 2.2 million galaxies. The galaxy density is n eff = 4.7 galaxies arcmin −2 . The median redshift is z median = 0.53.

Spectroscopic dataset: BOSS CMASS sample
The BOSS spectroscopic survey (Eisenstein et al. 2011) is a programme of the SDSS project. The constant (stellar) mass 2 We use the definition n eff = 1 (CMASS) galaxy sample is one of the galaxy samples observed in this survey. This sample consists of galaxies selected with SDSS photometry, such that they lie in the redshift range 0.43 < z < 0.7 and represent a sample of galaxies approximately volume-limited in stellar mass (Reid et al. 2016). Early clustering analysis found that CMASS galaxies lie in massive haloes and have a mean halo mass of 2.6 × 10 13 h −1 M , a large-scale bias of b ∼ 2.0, and a satellite fraction of 10% (White et al. 2011).
We used the public DR12v5 version of the CMASS catalogue (Alam et al. 2015). The galaxy surface density is about 100 deg −2 (Reid et al. 2016). We only considered CMASS overlapping with our four lensing fields, i.e. covering an area 250 sq. deg. Our catalogue of lenses contains 28 039 CMASS galaxies, distributed as reported in Table 1. The redshift distribution of CMASS galaxies compared to CS82 and CFHTLens lensing sources is shown in Fig. 1.
In spite of a careful photometric selection, the observed CMASS galaxy sample remains contaminated by various observational effects (Ross et al. 2012). We took these into account by applying the galaxy weights w g = w star w see (w z f + w cp − 1) as defined in Ross et al. (2017). We also included the Feldman et al. (1994, hereafter FKP) weights with the parameter P 0 = 20 000 h −3 Mpc 3 (Ross et al. 2012), such that the noise in the power spectrum is minimum at the baryon acoustic oscillation scale k = 0.1 h Mpc −1 . Although not optimal for our study focussed on small-scale clustering, this value of P 0 allows for a consistent comparison with previous measurements. For consistency, we take the same value of P 0 for our mock catalogues and data. Finally, we used the DR12v5_random0 catalogues trimmed to the regions overlapping with WL data.

Galaxy-galaxy lensing estimation
We computed ∆Σ gm (r p ) using the estimator ∆Σ gm (r p ) = N l,s l,s Σ cr (z l , z s )w l,s + (r p ) N l,s l,s w l,s − N r,s r,s Σ cr (z r , z s )w r,s + (r p ) where r p is the comoving transverse distance between the lens and the source at redshifts z l and z s , respectively. The subscript "r" denotes the random catalogue of lensing objects. Our number of random objects N r is ten times the number of lenses N l . Their redshift distribution n(z) is that from CMASS galaxies (Nuza et al. 2013). The subtraction of the random signal decreases the variance at large scales (Singh et al. 2017;Shirasaki et al. 2017). The value + represents the tangential component of a source ellipticity around a lens. The weight w l,s = Σ −2 cr (z l , z s )w s is the product of the shape measurement weight w s from lensfit and the critical density. This inverse variance scheme downweights pairs which are close in redshift (Mandelbaum et al. 2006). The critical lensing density Σ cr (z l , z s ) in comoving units is defined as where D S , D LS , D L are the observer-source, lens-source, and observer-lens angular diameter distances 3 We used the bestfit estimate of the photometric redshift to compute the distances, instead of the full probability distribution, as suggested in Blake et al. (2016). However, our approach described below and based on full ray-tracing simulations consistently takes this simplification into account.

Anisotropic galaxy clustering estimation
We computed the two-point galaxy correlation function in the polar and Cartesian coordinate systems. The anisotropy in the signal is due to the RSD effect we are after. The estimator is the same in each coordinate system and is defined as where (x, y) = (s, µ) or (r p , π). GG, GR and RR are the normalized number of pairs between galaxy-galaxy, galaxy-random, and random-random, respectively, at a given separation. We compressed the information contained in ξ(s, µ) by projecting it on the Legendre polynomials using the expressions for the correlation-function multipole moments where L is the Legendre polynomial of order . We used the monopole and quadrupole = (0, 2) only because the higher order non-null multipoles are too noisy. We also computed the projected correlation function w p (r p ) by projecting ξ(r p , π) along the line of sight such that where we find the optimal value π max = 40 h −1 Mpc to minimize the noise due to the limited number of pairs in our fields.

Joint lensing and clustering likelihood
We performed a maximum-likelihood analysis to derive the cosmological parameters from the GGL and RSD measurements. In each field i, we measured the data vector d i = (ξ i 0 , ξ i 2 , Υ i gm ) and we computed the likelihood function per field L i such that where m is the model prediction, andΦ i is the precision matrix estimated from the simulations. Our four fields are statistically uncorrelated, and therefore the global likelihood is just the product of the individual likelihoods for each field, i.e.
Field W4 partly overlaps with field S82, but this overlapping represents <6% of the total area. In addition, CFHTLens catalogue used for W4 goes deeper than CS82 catalogue used for S82, thus decreasing further the correlation between the two fields.

Light cones and lensing mock catalogues
In order to accurately estimate large-scale variance and possibly unveil new systematic errors, we produce light cones with the same geometry as the observed fields. We used the Big-Multidark N-body simulation, as it appears to be a good compromise between particle resolution and cosmological volume (m p = 2.5 × 10 10 h −1 M , L box = 2.5 h −1 Gpc, Planck cosmology with h = 0.6777; Klypin et al. 2016). Following the approach described in Giocoli et al. (2016), we simulated four fields, CS82, W1, W3, and W4, which have light cones extending up to redshift z = 2.3 for the CFHT-LS fields and z = 2 for CS82. We computed lensing properties, such as deflected positions, shear, and convergence, by ray tracing through 25 lens planes separated by 161 h −1 Mpc comoving (Giocoli et al. 2016) using the GLAMER 4 code. The spatial resolution of the lensing maps is 6 arcsec.

Lensing properties
We simulated lensing catalogues of sources including survey mask, intrinsic shape, and photometric redshift noises. For survey mask, we placed the source galaxies are the location of observed sources. Thus, we naturally reproduced the footprint and the holes around bright stars and other artefacts of the real WL catalogue. Effects due to the intrinsic clustering of sources in projection were also included. We got the shear properties for each source by spatially interpolating the values from the shear maps computed with GLAMER. For sources intrinsic ellipticities, we randomly drew observed ellipticites obs from the WL 4 Gravitational Lensing with Adaptive Mesh Refinement (Metcalf & Petkova 2014).
catalogue, that we multiply by a random orientation φ int , such that int 1 = obs cos(2φ int ) and int 2 = obs sin(2φ int ).

Photometric redshifts
To simulate photometric redshifts with catastrophic failures, we designed a method related to that described in Lima et al. (2008), also referred as the direct calibration method (DIR) in the Kilo Degree Survey (KIDS, Hildebrandt et al. 2017). We start by estimating the true redshift distribution n true (z) for our CFHTLens (i AB < 24) and CS82 (i AB < 22.5) WL catalogues from our spectroscopic calibration sample described in Appendix A. In practice, we computed the histograms of the WL and spectroscopic (ZP) catalogues in the magnitude-color space where N is the number of sources per bin. We assume all sources in a bin have the same weight. Finally, we obtain the true distribution in redshift bin i with the following sum: A drawback of this approach is that if spectroscopic selection does not cover part of the redshift range, then it truncates n true (z). However, we see in the following that the coverage is sufficient for our purpose.
Then, we compute the joint probability P(z BPZ , z spec ) for each field, as shown in Fig. 2. We observe that the spectroscopic redshift completeness at z < 0.5 in field W1 and W4 is very low because most of the redshifts come from the CMASS sample. Fortunately, this has little impact on our simulation of photometric redshift noise because our analysis focusses on the crosscorrelation of CMASS galaxies with lensing sources at z > 0.5. We also observe that the scatter in the z BPZ of CS82 field is almost twice as large as in field W3, and differs between the three CFHTLens fields. This justifies our field-by-field treatment of the photometric redshift noise. Finally, we assign photometric redshifts to the simulated sources by randomly drawing a photometric redshift from P(z BPZ , z spec ), where we assume the spectroscopic redshift z spec is the true redshift that was assigned at the beginning of the procedure.

Spectroscopic CMASS mock catalogues
We adopted the sub-halo abundance matching (SHAM) procedure described in Rodríguez-Torres et al. (2016) to produce CMASS mock catalogues. Starting from the Rockstar public catalogues (Behroozi et al. 2013) 5 , we computed a scattered peak velocity V scat peak = (1 + N(0, σ SHAM ))V peak , where N is the normal distribution, and σ SHAM = 0.31. We also simulated the CMASS incompleteness in stellar mass and redshift, based on the stellar mass function (SMF) from the Portsmouth sed-fit DR12 stellar mass catalogue with Kroupa initial mass function (Maraston et al. 2013). We binned the catalogue in 12 redshift intervals between 0.43 < z < 0.7 and in 18 stellar mass bins between 10.5 < log 10 (M * /M ) < 12.3. Thus, we obtained a tabulated SMF that we can interpolate in stellar mass and redshift. Finally from cumulative stellar mass and halo mass functions, we constructed a number density matching such that n gal (> M i * ) = n halo (> V scat peak,i ). Since different cosmologies were assumed in the Portsmouth catalogue and in the BigMultidark simulations, h = 0.73 and h = 0.6777 respectively, we renormalized the stellar masses to the BigMultidark cosmology. As shown in Fig. 3, our number densities for each of the four fields are in good agreement with the measurements from Anderson et al. (2012).
We also include the effect of peculiar velocities by summing together in redshift-space the halo position r c and the peculiar velocity vector v in real space using the relation s = r c + v·r a H(z real ) , wherer is the line-of-sight unit vector, a is the scale factor, and H(z real ) is the Hubble parameter at redshift z real , the redshift corresponding to r c . Finally, we masked the borders of the square simulated fields W3 and W4 to reproduce their complex geometry, and we computed the FKP weights, assuming the same P 0 = 20 000 h −3 Mpc 3 as in the data. Since data have been corrected for fiber collision, redshift failure, stellar density, and seeing, we did not simulate these effects.

Bias due to photometric redshift noise
We computed successively the lensing signal for catalogues with and without photometric redshift noise, and compare the measurements in Fig. 4. We find that the large photometric scatter observed in field S82 (Fig. 2)  10% in the lensing signal at scales R < 10 h −1 Mpc, whereas the CFHTLens fields seem insignificantly affected. We argue that this might explain the discrepancy highlighted in L17 between lensing measurements obtained with real and mock data. Indeed, in the following, we show that our lensing measurements with mock data contaminated by photometric redshift noise are in agreement with real data.

Bias from small-scale modelling
We used the simulation to quantify the bias in the estimation of the cosmological parameters f and Ω m due to our model prediction of the small scales. Successively, we cut data points of ξ 0 and ξ 2 at scales s min = 11.2, 14.1, and 17.8 h −1 Mpc, and Υ gm at scales R 0 = 1.0 and 1.5 h −1 Mpc. Overall, we find that the values s min = 17.  compromise between systematic bias and statistical precision as can be seen in Fig. 5.

Covariance matrices
To obtain an unbiased estimate of the precision matrices, we need minimal errors in the covariance matrices and therefore a large number of mock catalogues. Noise in the covariance matrices increases the errors on the model parameter estimation (see e.g. Taylor & Joachimi 2014). Unfortunately, we were limited by the size of our simulation box L = 2 h −1 Gpc. Escoffier et al. (2016) proposed a method to increase the number of mocks, based on Jackknife resampling of the mock catalogues (see Table 2). Following their prescription, we split each catalogue into N JK spatial subregions and measured the clustering and lensing signals in each Jackknife subsample using estimators given in Eqs. (34) and (32). The covariance matrix for each mock catalogue is then where the mean vector is obtained from the Jackknife samples In addition, given our limited number of independent mock catalogue N m , we increase their number for lensing by resampling N r times the observed lensing ellipticity distribution function, and the photometric redshifts distribution. We find this strategy to efficiently improve the accuracy of the covariance matrix for the lensing, especially at small scales. The final covariance matrix is therefore obtained by averaging the Jackknife covariance matrices  Finally, we computed the precision matrix Escoffier et al. (2016) have shown that this expression provides an unbiased estimate of the true precision matrix.
In spite of our resampling strategy, our covariance matrices are still noisy. Therefore, we adopted the tapering method proposed by Paz & Sánchez (2015) to damp the noise by a filter function beyond a given tapering scale T p . This technique is based on the assumption that correlation between pairs of data points far apart is negligible and little information is lost by treating these points as being independent. Although very efficient, it is commonly accepted that this method might inadvertently remove non-Gaussian terms (Paz & Sánchez 2015). However this effect is beyond the scope of this analysis given our data and the range of scales investigated in this work. In Fig. 6, we observe that large tapering yields errors similar to no tapering. In contrast, small tapering zeros all off-diagonal terms, and can also lead to overestimated errors. We find the errors on f and Ω m to reach a minimum value at the tapering scale T p ∼ 12 h −1 Mpc. We adopted this scale in the rest of this analysis. We should note that all measurements were performed with s min = 14.1 h −1 Mpc and R 0 = 1.5 h −1 Mpc. However, we repeated some measurements with our final set-up (s min = 17.8 h −1 Mpc and R 0 = 1.0 h −1 Mpc) and find that these parameters have almost no impact on the tapering scale behaviour. The covariance and precision matrices obtained before and after tapering at this scale are shown in Fig. 7. We can observe that A137, page 9 of 17 A&A 627, A137 (2019) the noise in the off-diagonal terms is significantly reduced after tapering. This is particularly obvious between clustering and lensing, which cover very different range of scales.

Cosmological results
The quality tests and errors assessment that we performed with the simulations give us confidence that our dataset can lead to reliable cosmological constraints.

Galaxy-clustering and galaxy-galaxy lensing measurements
In Figs. 8 and 9, we show our RSD and GGL measurements, along with our theoretical predictions, assuming the fiducial   Fig. 9. Filtered Υ gm and non-filtered ∆Σ GGL measurements with mocks (shaded regions), ∆Σ and Υ data (blue and orange points respectively), and theory with a linear bias parameter b 1 = 1.8 (dashed line). Black dots in S82 panel represent ∆Σ measurements from L16, and Υ gm measurements from Alam et al. (2017) in CFHTLS panels. parameters of the simulation, and a constant linear bias b 1 = 1.8. We find a good agreement within 1σ C.L. between mocks, data, and theoretical predictions for all fields. We notice that the quadrupole of the correlation function measurement in the field W3 is lower than the 1σ C.L., and that the GGL measurement in the field W4 is lower than 1σ C.L. at scales R < 1 h −1 Mpc. For field W3, we found that setting σ 8 (z = 0.57) = 0.9 and b 1 = 1.5 could reconcile predictions with measurements, thus suggesting a sample variance effect. These values are within the 3σ C.L. of the RSD-only fit of the data (see Fig. 10). For field W4, we attribute the discrepancy to our poor modelling of baryonic or lensing effects at small scales, which average out too slowly in the data to reproduce the simulated dark-matter only profile. Nonetheless, the overall good agreement gives us confidence that we can proceed with the cosmological analysis.

Growth of structure and background constraints
We estimate the cosmological parameters f , σ 8 , and Ω m by combining ξ 0 , ξ 2 , and Υ gm measurements. The power of this combination to break the degeneracy between f and σ 8 has already been demonstrated (see e.g. DLT17, Joudaki et al. 2017). In this paper, we move one step further by estimating Ω m as well from the data. Figure 10 shows the independent lensing, clustering, and combined constraints on these parameters. Best-fit values and 1σ error estimates are reported in Table 3. A corner plot with all the parameters involved in the fit is reported in Fig. A.2. On the one hand, we find that GGL alone constrains Ω m at 45% and σ 8 at 22%. It provides no constraint on the structure growth rate f . On the other hand, RSD also constrains σ 8 at 20% but leaves Ω m completely unconstrained as expected from the model. When used in combination, GGL and RSD measurements yield 12% precision constraint on σ 8 , i.e. almost as if the two datasets were independent. In fact, Fig. 10 shows that the well-known WL degeneracy between Ω m and σ 8 intersects almost perpendicularly with the constraint on σ 8 from RSD.
In Fig. 11, we present our estimate of the growth rate f , and compare to other measurements. In spite of having a wider area, we obtain a constraint similar to that found in DLT17 with VIPERS. Clearly, the number of RSD tracers determines the precision. In both analysis, we have about 28,000 galaxies in the range 0.5 < z < 0.7. Regarding WL, the number densities of background sources at z > 0.7 in both analysis are similar. We  √ Ω m /0.3 -0.87 ± 0.18 0.72 ± 0.08 E G --0.33 ± 0.10 f σ 8 (z = 0.57) 0.53 ± 0.14 0.50 ± 0.86 0.51 ± 0.12 σ 8 (z = 0) 0.78 ± 0.26 0.70 ± 0.12 0.73 ± 0.08 have n eff = 3.45 in CFHTLS fields and n eff = 2.33 in CS82 and CFHTLS fields combined. We also compare our results with analyses performed on the full CMASS sample. Singh et al. (2019) performed a joint analysis with Planck cosmic microwave background lensing and SDSS galaxy lensing and obtained three times tighter constraints than ours. Their results are in agreement with ours at the 1σ C.L.
Finally, combining CMASS power spectrum and bispectrum, Gil-Marín et al. (2017) also obtained very competitive constraints at redshift z = 0.57 in agreement with ours. These two estimates find a tension on f with Planck predictions at z = 0.57. Interestingly, this tension was also observed in other RSD analysis with the CMASS sample, but not with the LOWZ sample (e.g. Alam et al. 2017;Beutler et al. 2014).

Comparison with other measurements
From MCMC, we can derive new parameter constraints, defined as a combination of single parameters. In particular, we look at the quantity S 8 = σ 8 √ Ω m /0.3, very common in gravitational lensing analyses. We find S 8 = 0.72 ± 0.08, which is in agreement with the value estimated in L17, but 2 − 3σ smaller than the cosmic microwave background measurements S 8 = 0.832 ± 0.013 (Planck Collaboration VI 2018). Similarly, our estimate of σ 8 = 0.73 ± 0.08 is 2 − 3σ smaller than the measurement σ 8 = 0.8111 ± 0.0060 from the Planck collaboration 2018. Our results are also in agreement with KIDS shear peaks statistics S 8 = 0.75 ± 0.059 (Martinet et al. 2018;Shan et al. 2018), KIDS tomographic WL S 8 = 0.745 ± 0.039 (Hildebrandt et al. 2017), and DES cosmological constraints from WL and clustering S 8 = 0.783 +0.021 −0.025 . We note that our fit only performed with RSD measurements yield an estimate of σ 8 = 0.78 ± 0.26, in better agreement with Planck estimates.
Our model also contains a second order biasing term, but our estimated value b 2 = −0.04 ± 0.53 is not sufficient to discuss the non-linearity of the CMASS sample. We note that Gil-Marín et al. (2017) found b 2 = 0.606 ± 0.069, which is in agreement with us.
Finally, we also include Alcock-Paczynski effect in our model, but found no significant constraint given the data, α = 1.01 ± 0.05 and = 0.00 ± 0.05. We note that no significant constraint could either be obtained by Gil-Marín et al. (2017) with the full CMASS DR12 sample.
To conclude, we demonstrated the effectiveness of combining RSD and GGL to break the degeneracies between the amplitude of the large-scale structure fluctuations σ 8 and their growth rate f at redshift z = 0.57. We also found that the constraints on the cosmic matter density Ω m , usually derived with WL, could be significantly improved by combining with RSD. Given the data, our measurements are still in agreement with Planck predictions.

Measuring E G
To corroborate the information obtained with the analysis in the previous section and probe any deviation to ΛCDM−GR predictions, we estimate E G , as defined in Reyes et al. (2010). The E G estimator is function of projected scale r p , and is defined as (Zhang et al. 2007) This estimator is particularly interesting because it apparently just relies on observations. However, we show in the following that this might not be the case in practice.
Indeed, the E G estimator suffers from a few downsides. First, this estimator relies on a previous determination of β. However, statistical and systematic error propagation into E G error might be awkward, unless proper correction terms and covariance matrices are determined from ad hoc mock catalogues of lensing and clustering. Although seldom the case in the past, this is becoming more and more common (Blake et al. 2016;Amon et al. 2018;Singh et al. 2019). Second, it is assumed that galaxy bias is linear, scaleindependent, and the galaxy density field is fully correlated to the underlying matter density field, i.e. the cross-correlation factor r cc = 1. Of course, these assumptions hold in the linear regime, but the scale at which they break depends on the galaxy sample. Using CMASS mock catalogues, several authors have shown that they hold in the range 5 < r p < 60 h −1 Mpc (Baldauf et al. 2010;White et al. 2011;Amon et al. 2018;Singh et al. 2019). This depends on the requested precision on the model though, and recent works have proposed to take non-linearity and other effects into account with normalizing functions derived from simulations (Alam et al. 2017;Singh et al. 2019). The multiplication of these correction terms nonetheless tend to reveal the limitation of the E G estimator.
Marta Pinho et al. (2018) have noted that E G depends not only on gravity but also on the background (e.g. quantified with the matter density Ω m0 in ΛCDM). Although it is always possible to predict E G for different cosmological models (see e.g. Zhang et al. 2007, in which predictions are computed for ΛCDM, Flat DGP, f (R) gravity, TeVeS/MOND), a discrepancy with the observations therefore does not specifically point to a failure of GR, but can also be attributed to the background. In this respect, these authors claim that an estimator such as η, based on independent estimates of f σ 8 (z), H(z), E G might be more appropriate. To our point of view, adjusting an actual model including modified gravity parameters might be as helpful.
In spite of these limitations, E G has become quite popular recently, mostly because of the advent of wide field imaging and spectroscopic surveys. This estimator has been measured several times, but no significant deviation from ΛCDM−GR has been found so far. In particular with the CMASS sample at redshift z = 0.57, Amon et al. (2018) found E G = 0.26±0.08, Blake et al. (2016) found E G = 0.30 ± 0.07, Pullen et al. (2016) found E G = 0.24 ± 0.06, Alam et al. (2017) found E G = 0.42 ± 0.06, and Singh et al. (2019) found E G = 0.39 ± 0.05. The dispersion in the estimates reveal that the method is probably not fully mature yet, and deserves further investigation, in particular regarding the observational biases such as photometric redshifts. Figure 12 shows our measurements of E G as a function of scale. We estimate β = 0.41 ± 0.15 from our fit to the RSD Planck+15 Ω m = 0.27 Fig. 13. Measurements of E G at various redshifts. Effective redshifts of the measurements have been slightly shifted for clarity. measurements only. Although it is difficult to compare our work with other works because authors use different models, this value is larger but statistically consistent with that found with the full CMASS sample β = 0.34 ± 0.02 from Amon et al. (2018). For each bin of E G (r p ), we add in quadrature the errors on the ratio U i = Υ i gm /Υ i gg derived from the data and the error on β = f /b 1 derived from the fit, with the following chain rule formula: Using the MCMC samples from the fit of the GGL and RSD measurements, we use our model to reconstruct the ratio U i . We also determine the correlation coefficients ρ(β, U i ) ∼ 0.3, i.e. β and U i are significantly correlated. We average in the scale range 10 < r p < 60h −1 Mpc, and we find E G = 0.48 ± 0.15 for CFHTLens field only, and E G = 0.43 ± 0.11 for CFHTLens and CS82 fields combined, i.e. a 30% improvement in precision for a 100% increase in area. In the average E G calculation, we consider the full covariance matrix between the E G points estimated from our simulations in Sect. 5.1. We note finally that our current precision does not justify applying scale-dependent bias, redshift weighting, or integration window corrections since their effect is less than 5% at the scales we consider (see Alam et al. 2017;Singh et al. 2019).
To put our measurement in context, we collected the E G measurements at different redshifts from the literature in Fig. 13. Overall, we observe a trend of E G values lower than predicted by Planck 2018. In the appendix, we forward model the E G signal based on the MCMC samples output from the joint fit of the GGL and RSD measurements on mocks. Figure A.1 shows that the probability distribution function of the E G estimator is skewed towards low values. Taking its mean value then necessarily leads to a biased-low estimation of E G (r p ). This result confirms the previous claim from Alam et al. (2017), and might also explain why so many E G measurements are below the Planck 2018 predictions.

Conclusions
Understanding the current acceleration of the expansion of the Universe is one of the major goal of cosmology today. The combination of GGL and RSD is a remarkable avenue to distinguish the effect of gravity due to large-scale structures, and the effect of some scalar field on the background expansion rate.
In this work, we have demonstrated the power of this combination applied to the well-studied CMASS galaxy sample at the effective redshift z = 0.57. Using a comprehensive set of lensing and galaxy mock catalogues, we investigated several sources of systematic biases and determined the confidence limits for our datasets. In particular, we found that thanks to spectroscopic data, we could correct the bias due to photometric redshift uncertainty for galaxies brighter than i AB < 22.5, and i AB < 24 in our CFHT-S82 and CFHTLens WL catalogues, respectively. These conservative magnitude cuts allow us to match our GGL measurements in the CFHT-S82 and CFHTLS fields, although at the cost of drastically reducing the number of WL sources. This conclusive remark highlights the crucial need of spectroscopic redshifts to calibrate the photometric redshift faint galaxies.
Building on this encouraging result, we pursue a cosmological analysis of the combined dataset. Thanks to the joint GGL and RSD constraints, we efficiently break the degeneracy between galaxy bias b 1 , matter density Ω m , matter power spectrum amplitude σ 8 , and the structure growth rate f at z = 0.57. We find astrophysical CMASS parameters and cosmological parameters in agreement with measurements previously obtained by other authors (White et al. 2011;Beutler et al. 2014;Chuang et al. 2013;Gil-Marín et al. 2017;Joudaki et al. 2017) and with Planck 2018 predictions in the frame of the ΛCDM−GR model. Finally, we combine GGL and RSD measurements to estimate E G . By averaging in the range of scales 10 < r p < 60 h −1 Mpc, we find E G (z = 0.57) = 0.43 ± 0.11, which is in perfect agreement with Planck 2018 prediction E G = 0.40. Also, we use our mocks to characterize the statistical properties of E G , and find that it has an asymmetric probability distribution, which tends to underestimate its mean value. This might explain part of the low values found in previous analysis. We also find that the reconstructed value of E G = Ω m0 / f derived from the fit of the GGL and RSD measurements results in a value with smaller errors bars than that obtained directly from the data. More importantly, this value naturally includes the cross-correlation terms between β and Υ gg .
Back in 2012, Gaztañaga et al. (2012) was already advocating that overlapping lensing and spectroscopic surveys were 100 times more constraining on the dark energy equation of state and cosmic growth history parameter γ. Although it might not be the cleanest way to test gravity, the recent progress in estimating E G at different redshifts with different tracers comes as a confirmation. In the future, wider imaging and spectroscopic surveys will result in very tight constraints on cosmological parameters. In contrast, it will probably take us more time to fully profit from smaller but deeper imaging surveys. Deep imaging surveys are helpful for many reasons, but also introduce additional systematic errors on the lensing side, in particular with respect to blending (Harnois-Déraps et al. 2018;Euclid Collaboration 2019). Nonetheless, both strategies lead to very exciting perspectives regarding our understanding of the dark sector.
Masking. In order to assess the impact of missing tiles and large-scale masking (e.g. due to very bright stars), we compute the density of CS82 galaxies on a grid with pixel size ∼1 deg. Then, we randomly draw mock galaxies in the field such that the overall redshift distribution and total number of sources matches observations. Finally, we down-sample this catalogue according the density fluctuations attributed to masking. We find that masking increases the statistical noise in the GGL measurement by about 20% at all scales. However we could not identify any obvious systematic bias related to masking.
Photometric redshifts bias. Mandelbaum et al. (2008) and Nakajima et al. (2012) proposed an alternative method to estimate the bias introduced by photometric redshifts on GGL measurements. These authors proposed to estimate the bias b z (z lens ) between photometric redshifts ∆Σ and spectroscopic redshifts ∆Σ measurements, The summation is performed over the subset of source galaxies with both spectroscopic and photometric redshifts. We adapted the original expression from Mandelbaum et al. (2008) such that the inverse critical densities Σ −1 cr = 4πG c 2 D L (1 − D L D S ) converges to zero when the source redshift becomes smaller than z lens . The value w j is the weight on source galaxy j in the lensing catalogue. In order to estimate the effective bias on our GGL measurements with CMASS galaxies, we need to integrate the bias function b z (z lens ) over the CMASS redshift distribution p(z lens ) such that b z = dz lens p(z lens )w l (z lens )b z (z lens ) dz lens p(z lens )w l (z lens ) , (A.2) where the weight on each lens placew l = D −2 L (1 + z lens ) −2 j w j Σ −2 cr is correcting for the fact that the number of sources involved in a given aperture in physical coordinates includes more objects at lower than at higher redshifts. We bootstrapped our catalogues to estimate the uncertainties on our bias estimates.
We also adapted our code to assess the improvement obtained by using the photometric redshift probability of each source galaxy p(z s ) instead of maximum-likelihood values. The critical densities then becomẽ b z = −0.031 ± 0.005. Nonetheless, using the best-fit redshifts provided by BPZ still yields the smallest bias.
Catastrophic photometric redshifts. In order to assess the impact of catastrophic redshifts on the lensing measurements, we computed the two-dimensional probability p(z LP |z ANNZ ) of obtaining a photometric redshift with Le Phare given a photometric redshift obtained with neural network. Assuming this later to be the true redshift, we degraded the true redshifts in our mocks to reproduce the catastrophic outlier effects. Overall, we found that catastrophic redshifts could bias the lensing signal by about b z = +0.03. This is in agreement with our estimations above with spectroscopic redshifts and the estimates found in Leauthaud et al. (2017).
Asymmetric posterior on. E G It is very typical that observational estimators obtained from a ratio of observables have asymmetric probability distribution function. Indeed using our simulations, we found that E G is systematically lower than ΛCDM−GR predictions, with a long tail towards larger values of E G , as shown in Fig. A.1. When applying the usual E G = Υ gm βΥ gg estimator on our mocks, we also find mean values smaller than expected, although still in statistical agreement. We note finally that 1σ constraints are tighter with the fit than with the usual E G estimator. Given that Amendola et al. (2013) have demonstrated that E G is probably not as effective as anticipated in some particular cosmological models, and Alam et al. (2017) and Singh et al. (2019) have started to apply bias corrections to this estimator based on mock catalogues built with fiducial cosmological models, we think it might be as efficient and clean to fit the correlation functions, and derive E G by marginalizing over the model parameters, or simply compare Ω m0 and f to their ΛCDM+GR predictions.