Constraints on and from the potential-based cluster temperature function
The abundance of galaxy clusters is in principle a powerful tool to constrain cosmological parameters, especially and , due to the exponential dependence in the high-mass regime. While the best observables are the X-ray temperature and luminosity, the abundance of galaxy clusters, however, is conventionally predicted as a function of mass. Hence, the intrinsic scatter and the uncertainties in the scaling relations between mass and either temperature or luminosity lower the reliability of galaxy clusters to constrain cosmological parameters. In this article, we further refine the X-ray temperature function for galaxy clusters by Angrick et al., which is based on the statistics of perturbations in the cosmic gravitational potential and proposed to replace the classical mass-based temperature function, by including a refined analytic merger model and compare the theoretical prediction to results from a cosmological hydrodynamical simulation. Although we find already a good agreement if we compare with a cluster temperature function based on the mass-weighted temperature, including a redshift-dependent scaling between mass-based and spectroscopic temperature yields even better agreement between theoretical model and numerical results. As a proof of concept, incorporating this additional scaling in our model, we constrain the cosmological parameters and from an X-ray sample of galaxy clusters and tentatively find agreement with the recent cosmic microwave background based results from the Planck mission at 1-level.
keywords:cosmology: theory – methods: analytical – dark matter – cosmological parameters – galaxies: clusters: general
Since the evolution of galaxy clusters is mainly driven by gravity and dark-matter (DM) physics, galaxy clusters provide in principle reliable information about cosmological parameters, especially on the density of matter in the Universe and the amplitude of initial density perturbations, expressed by and , respectively. The usual procedure is to fit a theoretically motivated X-ray temperature function to X-ray samples obtained by analysing surveys conducted with X-ray telescopes like XMM Newton and Chandra.
The statistics of DM haloes, however, could conventionally only be analytically predicted based on masses, but measurements yield usually the X-ray temperature and luminosity. This implies that scaling relations between mass and other observables have to be calibrated relying on other cluster observables like e.g. weak-lensing shear, which reduces the power of the theoretical prediction by introducing additional sources of scatter. Additionally, the mass of a galaxy cluster is a global quantity and hence ill-defined since galaxy clusters have neither a fixed boundary with a regular shape nor a well-defined centre.
Angrick & Bartelmann (2009) developed an approach to derive the X-ray temperature function from the statistics of perturbations in the cosmic gravitational potential and the relation between potential depth and X-ray temperature. Using an extension of the ellipsoidal-collapse model of Bond & Myers (1996) by Angrick & Bartelmann (2010), Angrick & Bartelmann (2012) refined their X-ray temperature function by replacing spherical- with ellipsoidal-collapse dynamics and including an analytical merger model that takes the temporal temperature increase due to mergers statistically into account.
The goal of this paper is to further refine the merger model and analyse how the agreement between their analytical prediction and numerical realizations of the temperature function depends on the temperature definition used when setting up the halo catalogue inferred from a numerical simulation. We also want to analyse how constraints on and using the potential-based temperature function are affected if differences between the theoretically motivated X-ray temperature that enters via the virial theorem and temperatures that are actually inferred from measurements with X-ray telescopes are taken into account.
The structure of this paper is as follows: In Sect. 2, we summarize the main ingredients of the cluster temperature function built upon the statistics of the cosmic gravitational potential including the ellipsoidal-collapse model by Bond & Myers (1996), slightly extended by Angrick & Bartelmann (2010), and the refined analytic merger model based on the model by Angrick & Bartelmann (2012).
In Sect. 3, we give an overview of the fully hydrodynamical numerical simulation we base our analysis upon and introduce the temperature definitions we work with in the remainder of this work.
We contrast our theoretical model to results from this numerical simulation for different temperature definitions in Sect. 4 and analyse how taking into account a relation between these differently defined temperatures improves the agreement between semi-analytic model and simulations.
We present our constraints on both parameters in Sect. 6 and quantify how a relation between the X-ray temperature from the model and the one inferred from measurements affects constraints on both parameters. Additionally, as a proof of concept, we compare to recent results from the Planck mission.
Finally, we give a short summary in Sect. 7 and provide an outlook on how to proceed further with our potential-based temperature function.
2 Theoretical background
In this section, we will give short overviews of the main ingredients that are needed to construct the X-ray temperature function without reference to mass.
2.1 The ellipsoidal-collapse model
Let with be the dimensionless principal axes of a homogeneous ellipsoid, where the are the ellipsoid’s physical semi-major axes, and is the size of a spherical top-hat corresponding to a mass with the cosmological background density .
Their evolution is described by the following three coupled differential equations,
where is the scale factor of the Universe, its expansion function, and its derivative with respect to , and are the dimensionless density parameters of matter and the cosmological constant, respectively, in units of the critical density today and .
Here, is the density contrast of the evolving ellipsoid, is the th component of the internal shear given by
and the denote the components of the external shear, which we approximate by the so-called hybrid model,
where is the scale factor of turn-around of the th axis, is the linear growth factor of matter perturbations, and the are the eigenvalues of the Zel’dovich deformation tensor (Zel’dovich, 1970). Using the hybrid model, we take into account that the ellipsoid’s evolution is initially tightly bound to its vicinity until each axis finally decouples at its turn-around.
The initial conditions of equation (1) are given by the Zel’dovich approximation,
since for a small initial scale factor chosen to be . Note that in this ellipsoidal-collapse model, the reference frames of both the ellipsoid and the gravitational shear coincide.
The initial values of the at are given by
where is the square root of the matter power spectrum’s variance filtered with a circular top-hat function on the scale given by
Here, is the halo’s virial mass, is the gravitational constant, is the Hubble constant, is the matter power spectrum and is the Fourier transform of .
To derive equation (6), we implicitly used that the most probable values for the initial ellipticity and the prolaticity are the best choices to describe a statistical average of haloes with mass .
According to equation (1), the evolution of the three axes continues until the smallest axis finally collapses first. At that point, the halo’s density would formally be infinitely large, and the evolution of the other two axes could no longer be followed. But physically, the ellipsoid’s collapse should be stopped before due to virialization.
A proper virialization condition can be derived for each axis from the tensor virial theorem. It reads
If the former expression is fulfilled for the th axis, its collapse is stopped by hand, i.e. is set constant and to zero for the further evolution. The ellipsoid is considered to be completely collapsed when the condition (8) is fulfilled for the largest axis . This defines the virialization scale factor .
The critical overdensity and the virial overdensity with respect to the critical density are given by
respectively. Note that both and are mass dependent in this model unlike results from the spherical-collapse model!
2.2 The X-ray temperature function without reference to mass
In the following, we will shortly describe how to evaluate the cluster temperature function derived from the statistics of minima in a Gaussian random field and incorporating ellipsoidal-collapse dynamics. For a detailed derivation, see Angrick & Bartelmann (2009, 2012).
Based on the statistics of Gaussian random fields (Bardeen et al., 1986), the number density of minima in the cosmic gravitational potential as a function of the linear potential depth and the potential’s Laplacian can be derived analytically and is given by
Here, the with are the spectral moments of the potential power spectrum defined as
and . The window function in the former equation is given by
where with , which is the Fourier transform of the functional form of a homogeneous sphere’s gravitational potential.
The lower integration boundary in equation (13) is chosen for each pair such that the number density (10) is maximized. This effective high-pass filter removes large modes of the potential and also of its gradient so that the potential of an object is defined with respect to its local environment and small objects with are brought to rest and are therefore counted correctly. These objects correspond to minima in the non-linearly evolved potential which, however, are not present in the linearly evolved one.
The potential power spectrum is related to the matter power spectrum by
To obtain the number density of minima in the gravitational potential that belong to collapsed structures, we have to integrate equation (10) over accordingly,
where is Heaviside’s step function and the critical Laplacian is given by
Since galaxy clusters are highly non-linear objects, we have to relate the linear potential, , to a non- linear one, . This is realized by comparing the potential in the centre of a homogeneous ellipsoid at the time of virialization to the linearly propagated potential. The result is
where is the initial overdensity inside the collapsing halo chosen such that the last axis virializes at . Note that the ratio depends on both and through the axes since the ellipsoidal-collapse model is initialized with the scale . However, since we need to relate a single linear potential to a non-linear one, we marginalize over the dependence on by
where is a function of and via equation (18).
The non-linear potential depth can be related to an X-ray temperature via the virial theorem if we average over sufficiently many particle orbits. For particles near the centre, this yields
where is Boltzmann’s constant, is the proton mass and represents the mean molecular weight and is defined as
where and are the primordial hydrogen and helium mass fractions, respectively, so that .
2.3 The influence of mergers on the temperature function
So far, we have only taken into account virialized structures for which the relation (20) holds. However, due to hierarchical structure formation, smaller DM haloes merge to form larger haloes. Since these mergers induce a rise in the X-ray temperature function (see e.g. Randall, Sarazin & Ricker, 2002), we will include this effect statistically in our framework by a simple parameter-free merger model. The following model slightly extends the model by Angrick & Bartelmann (2012) to account for the change of the cluster temperature function with redshift.
Starting from the number density of virialized galaxy clusters at a given temperature and redshift, , we calculate two correction terms. First, we add the clusters that reach a temperature only due to a temperature boost induced by a merger, and second, we subtract those that would have a temperature if they were virialized, but have a temperature higher than due to a merger.
Denoting the first contribution by and the second by , the final halo population can be modelled as
where is given by
In the two former equations, there are various quantities that have to be defined in the following.
The merger rate yields the number of mergers of haloes with mass with other haloes in the mass range and in the redshift range and is given by
(Lacey & Cole, 1993), where , (cf. equation 7), and . Here, is the critical overdensity of the spherical-collapse model. Heaviside’s -function in equation (24) ensures that so that mergers between two objects with masses and are only counted once by demanding that the mass ratio between main and merging object is always larger than unity.
The redshift interval is connected to the sound-crossing time by
are the cluster’s mean radius and the sound speed, respectively.
The theoretical temperature-mass relation for virialized ellipsoidal haloes is given by
Dirac’s delta-distribution in equation (24) ensures that only those clusters contribute to the integral whose temperature is the sum of their temperature based on virial equilibrium, , and a temperature increase due to the merger given by
where is the mean potential on the surface of an ellipsoid with mass , virialized at redshift ,
can be calculated accordingly from equation (25) using equation (26) for , equation (27) for , and inverting equation (29) to arrive at . Note that in equation (25), is simply the cluster’s virial temperature .
3 The simulation
Hydrodynamical simulations are important numerical tools to describe in detail the evolution of cosmic structures in the Universe taking into account gas physics. In this section we describe in detail the numerical set-up adopted in this work. In particular, we will describe the simulations used, how haloes were extracted and how we built the halo catalogues with their X-ray properties.
The hydrodynamical simulation used in this work is part of a bigger set of simulations (BINGS, Baryons in non-Gaussian simulations) originally proposed to study the effect of baryons in cosmologies with non-Gaussian initial conditions. They represent an extension of the DM only simulations analysed to study several aspects of the large-scale structures of this kind of cosmologies (Grossi et al., 2009). In addition, the DM-only simulations with the same cosmological parameters and box size have been already employed for studies on the SZ effect and X-ray emission (Roncarelli et al., 2010). For this work, we use exclusively the simulation run with Gaussian initial conditions, also in the light of recent observations of the cosmic microwave background (CMB) by the Planck mission (Planck Collaboration XIII, 2015).
The simulations are based on the parallel cosmological TreePM-SPH code Gadget-2 (Springel, 2005) using an entropy-conserving formulation of smoothed-particle hydrodynamics (SPH; Springel & Hernquist, 2002). The simulation run includes radiative cooling, star formation with associated feedback processes (Springel & Hernquist, 2003) and heating by a uniform, time-dependent ultraviolet background. The simulation also takes into account a multiphase model for star-formation and feedback processes due to supernovae-driven galactic winds (Springel & Hernquist, 2003; Di Matteo et al., 2008).
The numerical set-up assumes a box of 1.2 Gpc comoving with DM and gas particles. The underlying cosmological model is a standard cold dark matter model with the cosmological parameters derived by the 5 yr WMAP results. We report them in Table 1. DM particles have a mass of , and gas particles have a mass of (at the redshift of the initial conditions, ). The gravitational force is computed assuming a Plummer-equivalent softening length of kpc. The evolution of particles is followed till the present time (). To create the initial conditions of our simulation, the transfer function by Eisenstein & Hu (1998) was used.
|Hubble parameter (100 km s Mpc)||0.72|
|Amplitude of fluctuations at 8 Mpc||0.8|
|Total matter density||0.26|
|Dark energy density||0.74|
|Cubic box length ( Mpc)||1200|
|Total number of particles|
|Mass of DM particles ()|
|Mass of gas particles at ()|
Haloes were initially identified with a Friend-of-Friend algorithm (Davis et al., 1985) with linking length times the mean interparticle distance and in a second step, using the SUBFIND algorithm (Springel et al., 2001; Dolag et al., 2009), we evaluated spherical-overdensity masses for each halo centred at the deepest potential point. We computed two different overdensities, and times the critical density. The corresponding radii are and , respectively. We extracted our catalogues at different redshifts, namely , , , , and , and considered only objects with at least 100 DM particles to incorporate only haloes in the further analysis whose X-ray profiles are resolved well enough..
To evaluate the X-ray properties of each halo, we took into account all its gas particles, computed the relevant quantities for each individual particle and summed them up to have the integrated value for the object considered. For what concerns us, we will limit our discussion to the evaluation of the halo temperature. Starting from the internal energy of a given SPH particle, we evaluate its temperature with the following relation,
For a given object we can define three different temperatures: the mass-weighted one, , (Kang et al., 1994; Bartelmann & Steinmetz, 1996; Mathiesen & Evrard, 2001), the emission-weighted one, , (Kang et al., 1994; Mathiesen & Evrard, 2001), and the spectroscopic-like temperature (Mazzotta et al., 2004). They are defined as
respectively, where is the density and is the integration volume (in this case the volume of the halo). In the following, we will consider a spherical integration volume with either or as a radius and indicate the corresponding temperature as, e.g., or , respectively.
Since the halo density is not simulated as a continuous quantity, we can replace the integration with a sum over all particles such that the operative definitions of the three different temperatures become
where and are the mass of the th particle and the SPH estimate of the density at its position, respectively.111Note that there are more complicated definitions of the emission-weighted temperature, involving in its definition the cooling function (Bryan & Norman, 1998; Frenk et al., 1999; Muanwong et al., 2001; Borgani et al., 2004). However, since we will not use the emission-weighted temperature in the further discussion, we limit ourselves to the more simplified definition (34) here.
The mass-weighted temperature (equation 33) has a relevant physical meaning since it is proportional to the total thermal energy of the cluster. However, it may differ significantly from what an observer would measure via an X-ray spectral analysis since the bremsstrahlung emissivity is proportional to the square of the gas density: the emission-weighted temperature (equation 34) takes this bias into account. The spectroscopic-like temperature (equation 35), introduced by Mazzotta et al. (2004), besides the emissivity bias, accounts also for the gas temperature gradient along the line of sight together with the shape of the energy response function of Chandra and XMM-Newton X-ray detectors.222When calculating and , it is necessary to remove cold SPH particles ( keV) from the computation to exclude the contribution of the cold dense phase of the ICM that has negligible emissivity.
4 Analytical model versus simulation
In the following, we want to compare the results of our analytical model from Sect. 2 with results from the simulation presented in the previous section based on the two temperature definitions and in the analysis, where ‘cut’ in the superscript refers to the fact that the volume corresponding to the inner 15 per cent of the sphere’s radius is cut out from the integration to obtain . The reason for cutting out the inner part will become clear shortly.
In Fig. 1, we show the X-ray temperature function based on together with our semi-analytical prediction for five different redshifts. The theoretical curve matches the numerical results from the simulation very well for lower temperatures. At temperatures keV, however, the theoretical prediction lies above the temperature function from the simulation. A reason for the latter might be that haloes with a high X-ray temperature and therefore also a large mass are not well resolved in the simulation due to the limited number of large-scale modes in the simulation.
Since the X-ray temperature in our model is derived from the thermal energy of the virialized cluster and the mass-weighted temperature is proportional to the cluster’s thermal energy, is the definition used in the simulation that matches best the one in our model and hence is the appropriate quantity in this case.
In Fig. 2, we show the X-ray temperature function based on as inferred from the simulation together with our semi-analytic prediction since X-ray observers often fit the spectrum of a galaxy cluster in the interval . The theoretical prediction underestimates the number density of haloes at temperatures keV, whereas for higher temperatures the theoretical curve lies above the results from the simulation at low redshifts. This might be another hint at missing high-mass objects in the simulation and incomplete statistics. Overall, the theoretical curve seems too flat compared to the numerical one inferred from the simulation.
To relate the temperature that is measured by observers () to the one that our model is based on (), we fitted a relation for each of the five different redshifts of the form
based on the cluster catalogue extracted from our simulation. The fitting parameters and therefore vary with redshift. We used only those clusters for the fit that fulfil both keV and for both and , where is the mass of the cluster’s DM component. The cut in mass corresponds to the requirement of having a halo that consists of at least 100 particles. The fitted functions (39) together with the data points the fits are based on are shown for various redshifts in Fig. 3.
The resulting fitting parameters and can be found in Table 2. Except for , the parameter is very close to 3 keV. Additionally, the higher the redshift, the closer to unity is the parameter . The rms of the deviations of individual clusters from the fitting relation (39) is with 0.21 keV largest for and with 0.12 keV smallest for and hence relatively small.
Based on the relation (39), we recalculated our theoretical prediction by scaling the temperature function accordingly, i. e. given , we calculated and used this temperature as input for equation (22). In doing so, an additional factor had to be taken into account. The comparison between the rescaled theoretical temperature prediction and the one inferred from the simulation based on can be found in Fig. 4.
After a temperature rescaling in the theoretical prediction for the X-ray temperature function, the agreement between the theoretical predictions and the numerical results based on is much better for all redshifts. Thus, by taking the redshift-dependent temperature conversion (equation 39) into account, our theoretical model based on the statistics of gravitational-potential perturbations is consistent with numerical results that mimic as well as possible the X-ray temperature function inferred by real observations.
5 Constraining cosmological parameters
Based on the results from the previous section, we want to determine the cosmological parameters and from a cluster sample by Vikhlinin et al. (2009), which was also considered in the Planck 2013 analysis of the Sunyaev-Zel’dovich (SZ) effect (Planck Collaboration XX, 2014), using our theoretical model for the X-ray temperature function together with a proper temperature scaling dependent on redshift based on equation (39). The statistical analysis is very similar to the one already presented in Angrick & Bartelmann (2012).
This section is meant as a proof of concept. To reliably constrain cosmological parameters in the future, one should stick to empirical relations between the potential of a cluster and its temperature, e.g. by combining data from gravitational lensing and X-ray temperature measurements, and not rely on relations inferred only from hydrodynamical simulations. See also the end of Sect. 7 for more details.
5.1 The sample
The sample by Vikhlinin et al. (2009) consists of two subsamples, one at high and one at low redshift, based on ROSAT PSPC All-Sky (RASS) and 400 deg data. The low-redshift sample is based on archival Chandra data and consists of 49 clusters with flux erg s cm in the 0.5–2 keV band from several samples of RASS with a total area of 8.14 sr (26722 deg). The redshift coverage is with , and temperatures are in the range as inferred from their spectra measured in multiple annuli with Chandra.
The high-redshift sample consists of 36 clusters from the ROSAT 400 deg survey (Burenin et al., 2007) further analysed with Chandra in the redshift range with and a redshift-dependent flux limit in the 0.5–2 keV band. For , the limiting flux is erg s cm, whereas for , the flux limit corresponds to a minimal X-ray luminosity of erg s. The temperatures of the clusters are in the range as inferred from their spectra measured with Chandra in the region , where is the radius that encloses a mean overdensity of 500 times the critical density of the Universe.
The effective differential search volume as a function of mass and cosmological parameters , and km s Mpc for both subsamples was made available in electronic form on a grid by A. Vikhlinin. To convert it to a function of temperature, we used the best-fitting values of the mass–temperature relation of Vikhlinin et al. (2009),
where and .
5.2 The fitting procedure
Since the errors on the cluster number counts are Poissonian, we used the statistic of Cash (1979) for unbinned data to find the best-fitting values for and , assuming a spatially flat universe, hence . In the next section, we compare with the results from the 2015 data release of the Planck Collaboration so that we set the baryon density parameter , the index of the primordial power spectrum and as inferred from the TT,TE,EE+lowP data (Planck Collaboration XIII, 2015). To include baryonic effects, we used the transfer function by Eisenstein & Hu (1998) when computing the power spectrum .
The statistic is defined as
where is the total number of objects expected from the sample assuming a theoretical model, and is the theoretically expected differential number density of the th cluster in the sample with temperature and redshift . The sum extends over all sample members.
Although the cosmological parameters in the further discussion will slightly differ from their numerical values in our cosmological simulation, we assume that the temperature relation (39) does not change significantly so that we could still use the best-fitting values from Table 2. To take the listed uncertainties into account, we convolved with a normal distribution of the form
where is given by equation (39). Both and in that relation depend on redshift as follows. Let and be two consecutive redshifts for which the former relation can be deduced from the simulation. For a redshift with , the values of the parameters and as well as their errors are linearly interpolated from their values at and (cf. Table 2). To properly take the errors on the parameters and into account, the standard deviation was set to
due to Gaussian error propagation. Thus, the expected number of objects in each subsample is given by
where the subscripts ‘low’ and ‘high’ denote the low- and the high-redshift subsample, respectively. The integral boundaries depend on the subsample and are given in Sect. 5.1 for and . The integration over has to be done over the whole valid range of .
Finally, the expected differential number density of the th cluster is simply given by the convolution
where is the measurement error of the th cluster.
To jointly fit both the low- and the high-redshift cluster samples of Vikhlinin et al. (2009), we had to add the two contributions, resulting in
We searched for minima of the statistic as a function of the two cosmological parameters and , which enter both via and the volume factor .
Cash (1979) showed that one can create confidence intervals for the statistic exactly in the same way as it can be done for a fit using properties of the distribution. Following the work by Lampton, Margon & Bowyer (1976), intervals with confidence are implicitly given solving
for , where is the density of the distribution with degrees of freedom determined by the number of parameters. For 68 per cent confidence and , it follows that , while for 95 per cent confidence, . Using the minimum of the statistic, , we could simply calculate the 68 and 95 per cent confidence contours by searching for points in the parameter space for which and , respectively.
In Fig. 5, we compare the 68 and 95 per cent confidence contours for the parameters and inferred with our semi-analytic cluster temperature function to the respective confidence contours from the Planck 2015 data release (Planck Collaboration XIII, 2015) based on the TT,TE,EE+lowP data both including the temperature relation (39) and excluding it by setting in equations (44) and (45) for the latter case.
Taking the temperature conversion from to into account when fitting our theoretical X-ray temperature function to the X-ray sample by Vikhlinin et al. (2009) shifts the confidence contours to smaller values for and to larger values for compared to the case where such a temperature conversion based on the difference between measured and theoretically motivated temperature is neglected. Additionally, the sizes of both the 68 and the 95 per cent contour are smaller if the temperature conversion is included.
The Planck constraints are in agreement with our results incorporating the redshift-dependent temperature conversion (39) at 1-level, whereas the results without the temperature conversion are in agreement with the Planck results only at the 2-level. Hence, discriminating between the temperature that is actually inferred from an X-ray measurement (similar to ) and theoretically motivated temperature consistent with the virial theorem (similar to ) seems crucial when our potential-based X-ray temperature function is used to constrain cosmological parameters.
7 Summary & conclusions
In the first part of this article, we further refined the X-ray temperature function for clusters based on the cosmic gravitational potential by Angrick & Bartelmann (2009, 2012) by incorporating the redshift evolution of the temperature function for virialized structures (equation 22) into our analytical merger model. We then compared our theoretical model to X-ray temperature functions inferred from a fully hydrodynamical simulation based on two different temperature definitions at five different redshifts: (1) the mass-based temperature inside , , (2) the spectroscopic like temperature inside with the inner part cut out, . The main results can be summarized as follows:
Our theoretical temperature function is in very good agreement with the numerical one based on except for relatively high temperatures which is presumably due to resolution effects of the simulation in the high-mass regime.
Compared to the numerical temperature function based on , our theoretical X-ray temperature function underestimates the abundance of objects over a large temperature range for all redshifts examined.
For each redshift separately it is possible to find a relatively tight relation of the form , where both and are fitting parameters depending on . The rms of the deviations of individual clusters in the simulation from the above relation reaches from 0.12 keV at to 0.21 keV at .
Scaling the temperature of our theoretical temperature function according to the above relation for each redshift and then comparing it to the numerical temperature function based on yields very good agreement between both functions.
The second part of this article was meant as a proof of concept. Here, we used the redshift-dependent temperature scaling found in the first part for our theoretical model to fit it to an X-ray sample by Vikhlinin et al. (2009) and constrain the cosmological parameters and . For comparison we also fitted these parameters without taking the aforementioned temperature conversion into account. The main results are the following:
Incorporating the temperature conversion shifts the confidence contours in the - plane towards smaller values of and larger values of . Additionally, the size of the contours is reduced.
We find agreement at 1-level between the purely CMB-based TT,TE,EE+lowP results from the Planck 2015 data release (Planck Collaboration XIII, 2015) and our theoretical model incorporating the temperature conversion, whereas the two only agree at 2-level with each other if the temperature conversion is neglected.
Concluding, it seems necessary to establish an empirical relation between the potential and the X-ray temperature of a cluster since relying solely on a scaling inferred from a hydrodynamical simulation may not allow to constrain cosmological parameters reliably enough. Combining data from gravitational lensing and X-ray observations of both relaxed and merging galaxy clusters could be a promising way to find such a relation since gravitational lensing probes the gravitational potential of a cluster projected along the line-of-sight, whereas one can infer the temperature of its intracluster medium (ICM) from X-ray spectra.
Once such an empirical relation is established, we will use our potential-based temperature function on more recent and bigger samples of X-ray clusters to constrain and from cluster cosmology with higher accuracy and reliability. However, finding a well-defined physical and analytical model for this relation would be even more desirable since it would allow directly the modelling of the temperature abundance of galaxy clusters, thus avoiding additional sources of scatter.
We thank Klaus Dolag for providing the initial conditions of the simulation and Margherita Grossi for the code to run them. Simulations and cluster catalogues were created on the Intel SCIAMA High Performance Compute (HPC) cluster which is supported by the ICG, SEPNet and the University of Portsmouth.
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