Issue 
A&A
Volume 574, February 2015



Article Number  A86  
Number of page(s)  11  
Section  Numerical methods and codes  
DOI  https://doi.org/10.1051/00046361/201323181  
Published online  29 January 2015 
Logtransforming the matter power spectrum
^{1}
MaxPlanckInstitut für Astrophysik,
KarlSchwarzschildStr. 1,
85748
Garching,
Germany
email:
maksim@mpagarching.mpg.de
^{2}
LudwigMaximiliansUniversität München,
GeschwisterSchollPlatz
1, 80539
München,
Germany
Received: 3 December 2013
Accepted: 10 December 2014
We investigate whether nonlinear effects on the largescale power spectrum of dark matter, namely the increase in smallscale power and the smearing of baryon acoustic oscillations, can be decreased by a logtransformation or emulated by an exponential transformation of the linear spectrum. To that end we present a formalism to convert the power spectrum of a lognormal field to the power spectrum of the logarithmic Gaussian field and vice versa. All ingredients of our derivation can already be found in various publications in cosmology and other fields. We follow a more pedagogical approach providing a detailed derivation, application examples, and a discussion of implementation subtleties in one text. We use the formalism to show that the nonlinear increase in smallscale power in the matter power spectrum is significantly smaller for the logtransformed spectrum which fits the linear spectrum (with less than 20% error) for redshifts down to 1 and k ≤ 1.0 h Mpc. For lower redshifts the fit to the linear spectrum is not as good, but the reduction of nonlinear effects is still significant. Similarly, we show that applying the linear growth factor to the logarithmic density leads to an automatic increase in smallscale power for low redshifts fitting to thirdorder perturbation spectra and Cosmic Emulator spectra with an error of less than 20%. Smearing of baryon acoustic oscillations is at least three times weaker, but still present.
Key words: methods: data analysis / largescale structure of Universe
© ESO, 2015
1. Introduction
In cosmology and astrophysics densities are often described as a combination of the mean density and fluctuations around it, (1)where the density contrast field δ is often small and accurately described by a Gaussian random field. However, as soon as large overdensities occur (δ> 1) a description of δ by Gaussian statistics does not suffice, since δ cannot go below minus one. A prominent example of such a density is the largescale structure, where the overdensity is accurately described by Gaussian statistics at early epochs, but becomes highly nonlinear at later epochs and small scales. In these nonlinear regimes the density is much more accurately described by lognormal statistics, i.e., log (1 + δ) following Gaussian statistics. This has already been noted by Hubble (1934) and Hamilton (1985) and theoretically investigated by Coles & Jones (1991). Nbody simulations calculated by Kayo et al. (2001) are also in agreement with a lognormal distribution. However, as Carron (2011) showed, correlation functions and spectra contain very limited information in the case of highly nonlinear lognormal statistics as there are other distribution functions that would produce the same moments. For a perturbative treatment of the power spectrum of log (1 + δ) see Wang et al. (2011). Another example is the density in turbulent and isothermal clouds, which is very accurately described by a lognormal distribution (see, e.g., Passot & VázquezSemadeni 1998 or Nordlund & Padoan 1999).
In many cases, however, only the linear power spectrum (the power spectrum of δ) is available (e.g., from observations or simulations). It is therefore useful to convert a linear power spectrum into a logarithmic power spectrum (and vice versa). In this work we derive such a conversion formula under the assumption that the power spectrum is the power spectrum of the underlying statistical process. This condition is not necessarily met if the power spectrum is calculated from observational data or simulations, but in most cases the formula works nevertheless. Formulas relating the correlation functions of Gaussian and lognormal fields are widely known throughout several fields. In cosmology we refer the reader to Coles & Jones (1991), Politzer & Wise (1984), and Percival et al. (2004). The first goal of this paper is to provide a pedagogical introduction along with application examples enabling the reader to directly apply the derived formulas in a numerical setting while avoiding normalization and prefactor mistakes which can drastically influence the outcome due to the nonlinearity of the exponential and logarithmic functions. The second goal is to apply the presented formalism to investigate how much a logtransformation of the largescale density reduces the nonlinear enhancement of smallscale power for decreasing redshifts.
The remainder of this paper is structured as follows. First, we go through the derivation of the conversion formalism in Sect. 2 in which we state all definitions explicitly before the calculation. Second, we apply the conversion to the largescale matter spectrum in Sect. 3 to test the validity of the lognormal approximation of the cosmic matter density. Finally, we conclude this paper with a summary and outlook in Sect. 4.
In the Appendix, we describe how to generate lognormal random field following a given spectrum (Appendix A). Furthermore, we present a consistent discretization of the conversion formulas (Appendix B) their spherical harmonics equivalent (Appendix C). We also discuss in greater detail a number of aspects from Sect. 3 in Appendix. D, e.g., how the choice of gridding affects the results.
2. The conversion
2.1. Notation and definitions
We denote the lognormal field at position x by ρ(x) and the underlying Gaussian field by s(x), (2)where s is dimensionless and the units of ρ as well as a proportionality constant are in ρ_{0} and m ≡ log ρ_{0}. In this work, log denotes the natural logarithm.
The field s is assumed to follow a Gaussian distribution with zero mean^{1}, (3)with u being the dimensionality of space and . S(x,y) is the autocorrelation function of s. It is defined as (4)Here, denotes integration over the full phase space of s. The inverse of S is defined by the relation (5)where δ_{D}(x − z) is the udimensional Dirac delta distribution.
In Fourier space, we denote position vectors by k or q. Fourier transformed fields are denoted by their argument (e.g., s(k)). We define the Fourier transformations over continuous position space as (6)If a field obeys statistical homogeneity its autocorrelation function depends only on the separation, S(x,y) = S(x − y), and is therefore diagonal in Fourier space, (7)The quantity P_{s}(k) is the statistical power spectrum of s.
The autocorrelation function and statistical power spectrum of ρ are defined analogously, (8)In the second line we used that ρ obeys statistical homogeneity, too.
2.2. Converting the logarithmic power spectrum to the linear power spectrum – the forward conversion
Suppose the statistical power spectrum of s, P_{s}(k), and the mean m are known. We are looking for the statistical power spectrum of ρ(x) = e^{s(x) + m}. The autocorrelation functions are related by (9)since is Gaussian. Using the statistical homogeneity of C_{ρ} and S, we write (10)This relation between the correlation function of a Gaussian and lognormal field is well known in cosmology (see, e.g., Coles & Jones 1991). Combined with Eqs. (7)and (8)this yields (11)and therefore (12)Equation (12)is our forward conversion formula.
If P_{s}(k) is isotropic, the equation can be simplified in spherical coordinates, since in that case the argument of the exponential function is isotropic in x, too. In the threedimensional isotropic case, integration of the angular part yields (13)where we denoted P(k) ≡ P(q)_{ q  = k}. While this equation only has onedimensional integrals, its numerical evaluation involves some subtleties, which is why we perform the numerical calculations in this work using fulldimensional fast Fourier transforms, even if the power spectrum is isotropic. However, integration of the angular part can be performed for all of the following equations in a very similar manner.
2.3. Converting the linear power spectrum to the logarithmic power spectrum – the backward conversion
Suppose the statistical power spectrum of ρ, P_{ρ}(k), is known and we want to know the power spectrum of s. We therefore need to solve Eq. (11)for P_{s}(k), (14)We invert the operation in front of P_{s}(k) using (15)to arrive at (16)The two correction terms on the righthandside do not affect modes with k ≠ 0, (17)and there is a degeneracy between the monopole P_{s}(k = 0) and the mean, (18)where we have identified V = (2π)^{u}δ_{D}(0) as the volume of the system. We recommend to set the monopole to zero to fix the mean. Equations (17) and (18)are our backward conversion formulas.
We note that knowledge about the monopole of ρ is crucial for this conversion to work. If the monopole is not supplied, one can estimate it from the mean of ρ as (19)Using the assumption of statistical homogeneity the backward conversion formula can also be applied in real space to get S(x,y) from C_{ρ}(x,y), (20)This relation can (in a different form) also be found in Coles & Jones (1991, Eq. (30) therein).
3. The matter power spectrum
In this section, we use Eqs. (12), (17), and (18)to test the range of validity of a lognormal approximation to the power spectrum of dark matter. In order to apply the formulas on a computer one needs to discretize them correctly, since global prefactors are important in a nonlinear transformation such as the exponential and logarithmic functions. We present a consistent discretization in Appendix B.
The cosmic matter density ρ is typically parametrized as the mean density ρ_{0} and mass density contrast δ according to Eq. (1). The threedimensional isotropic power spectrum of these fluctuations, P_{δ}(k), is usually referred to as the matter power spectrum of the largescale structure. At high redshifts the fluctuations are small, δ ≪ 1. With decreasing redshifts, the magnitude of the fluctuations increases. In linear theory, each Fourier mode of the fluctuations is enhanced by the same linear growth factor D(z), yielding a very simple relation between the matter power spectrum at different redshifts, (21)where P_{δ}(k,z) denotes the power spectrum of δ at redshift z. The functional form of the linear growth factor is slightly different for different cosmologies. We use the cosmological parameters determined by Planck Collaboration XVI (2014). The prefactor of the power spectrum is determined by the σ_{8} normalization^{2} which is the variance of δ convolved with a spherical top hat function with an 8 Mpc /h radius. Its value at redshift zero is determined by Planck Collaboration XVI (2014) to be σ_{8}_{z = 0} = 0.83. Together with the growth factor this determines the linear power spectrum P_{δ}(k) at all redshifts, since in linear theory it retains its shape. However, the linear description of the redshift dependence of the matter power spectrum fails for low redshifts, where the fluctuations can be on the order of 1. This has been successfully treated up to redshift 1 by third order perturbation theory (henceforth 3PT) around the linearly evolved spectrum by Jeong & Komatsu (2006). For redshifts below 1, the nonlinearities in the matter power spectrum can be modeled using the Cosmic emulator (henceforth CosmicEmu) based on Heitmann et al. (2009), Heitmann et al. (2010) and Lawrence et al. (2010).
Using the formalism presented in this paper we investigate whether some of the nonlinearities resolved by third order perturbation theory and the Cosmic emulator arise naturally if linear growth is applied to the logarithmic density contrast instead of the density contrast itself. A similar question has been investigated by Neyrinck et al. (2009). Using data from the Millennium Simulation by Springel et al. (2005), Neyrinck et al. (2009) compared the power spectrum of log ^{(}1 + δ^{)} at different redshifts. They found a remarkable reduction of nonlinearities in the power spectra up to k = 1.0 h Mpc^{1} at all redshifts. They also found a bias factor for large scales, which is not apparent in our figures. We discuss the origin of this factor in Appendix D.4.
Around redshift 7 the 3PT corrections by Jeong & Komatsu (2006) start to become significant. Jeong & Komatsu (2006) find a good agreement between the 3PT spectrum and Nbody simulations for wavevectors up to k = 1.4 h Mpc^{1} and redshifts higher or equal to 1. For redshifts 1 to 0 we use matter spectra calculated using CosmicEmu. According to Heitmann et al. (2009), Heitmann et al. (2010) and Lawrence et al. (2010) these are accurate to 1% up to k = 1.0 h Mpc^{1}. We therefore assume, that they are also reasonably accurate up to k = 1.4 h Mpc^{1}.
We denote the logarithmic density contrast as (22)At high redshifts, where δ ≪ 1, we have s ≈ δ. Therefore, at high redshifts applying the linear growth factor to s has the same effect as applying it to δ. We keep applying the growth factor to s instead of δ throughout the whole redshift spectrum in order to test whether some of the nonlinearities appearing at lower redshifts arise naturally this way. Therefore we apply the forward conversion formula (Eq. (12)) to the linearly evolved spectrum at redshifts 0 to 7 and the backward conversion formulas (Eqs. (17) and (18)) to the 3PT spectra and the CosmicEmu spectra respectively.
Fig. 1
Conversion formalism for redshifts 1 to 7. Left panel: forward converted linear spectra (solid lines) and the corresponding 3PT spectra (dashed lines), which are both divided by the respective linear spectrum for better comparison of the nonlinearities. Right panel: backward converted 3PT spectra (solid lines) and linear spectra (dashed lines), which are both divided by the respective 3PT spectrum. 

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To that end, we calculate the matter power spectrum at several redshifts between 1 and 7 by applying the 3PT code^{3} by Jeong & Komatsu (2006) to the linear power spectrum calculated using CAMB^{4} (see, e.g., Lewis et al. 2000) and between 0 and 1 using the CosmicEmu code^{5}.
The lowest spectral length covered is k = 0.004 h Mpc^{1} for the 3PT code and k = 0.0075 h Mpc^{1} for the CosmicEmu code. Therefore, we let our numerical setup cover the region 0.0075 h Mpc^{1} ≤ k ≤ 1.4 h Mpc^{1}. There are several ways to resolve this spectral range and because of the nonlinear nature of the exponential function the result of the conversion formulas is not independent of the choice. The smoothing onto a grid of a logarithmic function is thoroughly discussed by Wang et al. (2011). We perform the calculation on four different grids to demonstrate this difference. We present the results of one grid here and discuss the differences between the grids in Appendix D.2.
The mean of (1 + δ) is 1, the mean of e^{s}, however, is higher than 1, since the fluctuations are not symmetric. In order to properly compare the resulting spectra we therefore absorb a factor of ⟨e^{s}⟩ into ρ_{0}, i.e., in the following discussion we compare the power spectra of δ and (e^{s}/ ⟨e^{s}⟩ − 1).
3.1. The mildly nonlinear regime
For redshifts higher or equal to 1, the nonlinear corrections (calculated using 3PT) are rather mild. In this regime the model of a linearly evolved log density contrast works rather well, as we depict in Fig. 1. For a more quantitative comparison we depict the forward converted spectra divided by the 3PT spectra and the backward converted spectra divided by the linear spectra in Fig. 2. For redshifts 1 to 7 and k ≤ 1.0 h Mpc^{1} the maximal logdistance between the converted spectra and the 3PT spectra stays below 0.17. The distances are slightly lower for the backward conversion. As one can see in Fig. 2, the distance is strongest around k ≈ 0.2 h Mpc^{1}. For a full list of the logdistances see Appendix D.1. In the region where 1.0 h Mpc^{1}<k< 1.4 h Mpc^{1} the results are susceptible to the choice of gridding. We discuss this in detail in Appendix D.2.
Fig. 2
Conversion formalism for redshifts 1 to 7. Left panel: forward converted linear spectra (solid lines) divided by the corresponding 3PT spectra. Right panel: backward converted 3PT spectra (solid lines) divided by the respective linear spectrum. The dashed line marks 1. 

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3.2. The nonlinear regime
For redshifts smaller than 1, the nonlinear corrections add smallscale power which is comparable to the total linear power. On the grid we chose, the total power of the CosmicEmu spectrum is twice as high as the power of the linear spectrum at redshift 0.8. In this regime the agreement between the converted spectra and the CosmicEmu (or linear spectra, respectively) is much weaker. We depict the nonlinearities generated by the forward conversion and the reduction of nonlinearities in the backward conversion in Fig. 3. A more error focused comparison with the forward converted spectra divided by the CosmicEmu spectra and with the backward converted spectra divided by the linear spectra can be found in Fig. 4. The maximal logdistance for k ≤ 1.0 h Mpc^{1} between the backward converted spectra and the CosmicEmu spectra ranges between 0.17 for z = 1 and 0.8 for z = 0. For the forward converted spectra it ranges from 0.2 at z = 1 to 1.5z = 0. Clearly, a logdistance of 1.5 (corresponding to a factor of 4.5) is not within an acceptable margin of error. Emulating the nonlinear corrections from CosmicEmu by forward conversion breaks down in this regime. The backward conversion performs better than the forward conversion, but a logdistance of 0.8 (corresponding to a factor of 2.2) is far from ideal. However, the backward conversion still reduces the magnitude of nonlinear corrections significantly. See Table D.1 for a detailed comparison of the logdistances.
Fig. 3
Conversion formalism for redshifts 0 to 1. Left panel: forward converted linear spectra (solid lines) and the corresponding CosmicEmu spectra (dashed lines), which are both divided by the respective linear spectrum for better comparison of the nonlinearities. Right panel: backward converted CosmicEmu spectra (solid lines) and linear spectra (dashed lines), which are both divided by the respective CosmicEmu spectrum. 

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Fig. 4
Conversion formalism for redshifts 0 to 1. Left panel: forward converted linear spectra (solid lines) divided by the corresponding CosmicEmu spectra. Right panel: backward converted CosmicEmu spectra (solid lines) divided by the respective linear spectrum. The dashed line marks 1. 

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3.3. Smearing of baryon acoustic oscillations
Another important nonlinear effect is the smearing of baryon acoustic oscillations (BAO). Towards lower redshifts the smallest scale wiggles in the matter power spectrum are erased while the large scale wiggles become increasingly damped as redshift decreases. This can be nicely seen in Fig. 5, where we depict a comparison between 3PT spectra calculated on the basis of the CAMB power spectrum and 3PT spectra calculated on the basis of the “no wiggle” power spectrum by Eisenstein & Hu (1998)^{6} in the left panel. The same comparison but using the forward converted linear spectra instead of the 3PT spectra can be seen in the right panel. It is evident that BAO smearing appears only very slightly in the forward converted power spectra, it is much weaker than the smearing calculated using 3PT. BAO smearing appears to be about 3 to 4 times weaker (see Appendix D.3) in the forward converted spectra compared to the 3PT spectra, which exhibit a smearing in agreement with Nbody simulations.
Fig. 5
BAO smearing. Left panel: 3PT spectra with BAO divided by the 3PT spectra without BAO at several redshifts. Right panel: forward converted linear spectra with BAO divided by the forward converted linear spectra without BAO. We note the smearing of smallscale wiggles towards lower redshifts in the left panel. 

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4. Discussion and conclusions
Starting from the assumption of Gaussian statistics for s we presented a formalism to calculate the power spectrum of s = log (ρ) from the power spectrum of ρ and vice versa. This formalism can for example be used to compare theoretical considerations about logarithmic densities with theoretical or observed power spectra, which are calculated from the linear density. A numerical implementation of these formulas can be found in the NIFTy python package^{7} (Selig et al. 2013). The formalism is also useful to generate lognormal fields with a given power spectrum, as one can simply convert the spectrum, use the resulting spectrum to generate Gaussian random fields, and then exponentiate them (see Appendix A).
We used this formalism to investigate whether the nonlinear corrections to the matter spectrum are reduced for the logarithmic density and whether the nonlinearities can be emulated by applying the growth factor to the logdensity instead of the density. To that end we compared emulated linear (CAMB) and nonlinear (thirdorder perturbation theory and CosmicEmu) spectra with the in and outputs of our formulas. For the mildly nonlinear regime (redshift 1−7) we find that the logtransformed nonlinear spectra agree with the linear spectra rather well (less than 20% difference between them up to k = 1.0 h Mpc^{1}). This enables one to easily generate a lognormal field, which follows the appropriate nonlinear power spectrum, even for position dependent redshifts. We describe this procedure in detail in Appendix D.5. For lower redshifts the agreement decreases but the nonlinearities are still reduced significantly. The smearing of baryon acoustic oscillations can not be emulated by applying the growth factor to the logdensity. There is some smearing due to mode coupling, but it is about 3 to 4 times weaker than in the more exact thirdorder perturbation theory.
We performed the calculation on four different grids leading to different but within the achieved precision comparable results. The differences between the results on different grids indicate that the agreement between our model and the nonlinear spectra from literature decreases if the grid allows scales corresponding to k ≥ 1.4 h Mpc^{1}, since mode coupling to the small scales overestimates the nonlinear corrections. This problem arises since the total power of the matter spectrum diverges as its spectral index is above − 3, which makes some sort of cutoff in power necessary in a nonlinear transformation such as the exponential and logarithmic functions. Here, this cutoff is imposed by the resolution of the grid. Ultimately, one would have to find a physically justifiable way to regularize the integral in Eq. (13).
The “no wiggle” power spectrum was calculated by putting the cosmological parameters from Planck Collaboration XVI (2014) into the code from http://www.mpagarching.mpg.de/~komatsu/CRL/powerspectrum/nowiggle/
Acknowledgments
The authors would like to thank Niels Oppermann, Philipp Wullstein, Sebastian Dorn, and Marco Selig for fruitful discussions and support. We would also like to thank the anonymous referee for the constructive review and useful comments. All numerical calculations were done using the NIFTy python package by Selig et al. (2013).
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Appendix A: Generating lognormal fields from a given power spectrum
We can use the backward conversion (Eqs. (17)and (18)) to generate lognormal random fields that follow a given linear power spectrum. This method has already been presented by Percival et al. (2004, see Sect. 3.2 therein). For illustrative purposes we demonstrate the procedure for an isotropic case, but the same procedure can be applied for an anisotropic power spectrum.
Suppose the power spectrum P_{ρ}(k) is known within some range k_{min}<k<k_{max} and the mean ⟨ρ⟩ is also known. First, we set up a discretized space in which k_{min} corresponds to the minimal nonzero mode and k_{max} is the highest supported mode. We construct the monopole according to Eq. (19)and apply Eqs. (17) and (18)to the power spectrum. Setting P_{s}(k = 0) = 0 in Eq. (18)we end up with a power spectrum P_{s}(k) and a mean m. We can now construct lognormal fields by generating Gaussian random fields from P_{s}(k) and exponentiating the sum of s and m. The resulting field ρ = e^{s + m} follows (in the statistical average) the power spectrum P_{ρ}(k).
We illustrate this in Fig. A.1. Starting with the power spectrum of ρ and ⟨ρ⟩ = 1, we calculate the power spectrum and mean of s. The mean is − 0.76. With these quantities we can draw lognormal fields that follow the original power spectrum. One random field of that kind is plotted in Fig. A.2.
Fig. A.1
Backward conversion applied to a onedimensional power spectrum P_{ρ}(k) (solid line) yields the power spectrum P_{s}(k) (dashed line). 

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Fig. A.2
A onedimensional lognormal random field following the power spectrum P_{ρ}(k) from Fig. A.1. 

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Appendix B: The discretized conversion formula
The discretized conversion formulas are implemented in the NIFTy python package by Selig et al. (2013, version 0.8.4 or higher).
In discretizing the forward and backward conversion formulas from Sects. 2.2 and 2.3 one needs to pay careful attention to volume factors arising from the discretization of the integrals. We define the discrete Fourier transform as (B.1)We note that the definition of the Fourier vector has changed with respect to the main text, = k/ (2π), as this is more common in a numerical setting. The vector x can only take discrete values, (B.2)where the dimension j is discretized into N_{j} pixels with edge length Δx_{j}. Therefore, our discretized space consists of pixels that have the volume (B.3)This defines a conjugate set of discrete values for , (B.4)where Δk_{j} = 1 / (N_{j} Δx_{j}). Therefore, the conjugate space consists of N pixels that have the volume V_{k} = 1 / (NV_{x}). The power spectrum is defined analogously to Eq. (7)by (B.5)where (B.6)Defining ρ(x): = e^{m + s(x)} one can derive^{8} the forward conversion formula as (B.7)The backward conversion formula is (B.8)and for the monopole (B.9)
Appendix C: The conversion for spherical harmonics
The spherical harmonics conversion formulas are implemented in the NIFTy python package by Selig et al. (2013, version 0.8.4 or higher).
We define the spherical harmonics as (C.1)where we will write Ω as a shorthand notation for θ,ϕ with Ω = 0 corresponding to θ = 0, ϕ = 0. In the spherical harmonics basis we define the power spectrum as (C.2)where we assumed statistical homogeneity and isotropy. In this section, δ_{ij} denotes the Kronecker delta and ^{∗} denotes complex conjugation. The covariance matrix in pixel space is related to the power spectrum by (C.3)which in the case of Ω^{′} = 0 is (C.4)Because of statistical homogeneity and isotropy, this stays the same for all angles that are separated by Ω.
Following a similar calculation as in Sects. 2.2 and 2.3 we derive the forward conversion as (C.5)and the backward conversion as (C.6)and (C.7)
Appendix D: Supplements to Sect. 3
Appendix D.1: Logdistances
We calculate the maximal logdistance between two spectra as (D.1)This distance gives a quantitative measure about the goodness of approximating the nonlinear spectra by forward converted spectra and about the reduction of nonlinearities in the backward converted spectra. In Sects. 3.1 and 3.2 we give an overview over the logdistances for k ≤ 1.0 h Mpc. Here, we list all of their values in Table D.1, which also shows the logdistances between the linear and nonlinear spectra. As one can see the converted spectra always reduce the logdistance.
Highest logdistance (for k ≤ 1.0 h Mpc^{1}) between the forward converted spectra and the emulated spectra (3PT and CosmicEmu, respectively) and the backward converted emulated spectra and the linear spectra.
Appendix D.2: The effect of different grids
The calculation in Sect. 3 is performed on four different grids which all cover the same physical volume, but with different resolution. The figures in Sect. 3 show the results of the second grid (grid B). The lowest nonzero mode we want to cover is k = 0.0075 h Mpc^{1} for all grids. The highest mode is different for the three grids, the coarsest one having k_{max} = 1.0 h Mpc^{1}. The minimum spectral length covered by a threedimensional Cartesian box with the origin in the middle is (D.2)where L_{x}, L_{y}, and L_{z} are the total edge lengths of the box. The maximum spectral length is (D.3)where Δx, Δy, and Δz are the edge lengths of one pixel. This leaves us with an infinite number of possible pixelizations. We restrict ourselves to cubic pixels and an equal number of pixels in each dimension leaving us with only two parameters: the number of pixels per dimension N_{pix} and the pixel edge length Δx.
The first grid (grid A) consists of 152^{3}, the second grid (grid B) of 214^{3}, the third grid (grid C) of 522^{3}, and the fourth grid (grid D) of 766^{3} cubic pixels. The pixel edge lengths are chosen in a way that the lowest nonzeros value of k is 0.0075 h Mpc^{1}. We summarize the properties of these grids in Table D.2. The upper limit of the spectral range of grid D is higher than 1.4 h Mpc^{1}. To investigate the effect of the pixel size on the conversion we cut the power spectrum at k = 1.4 h Mpc^{1} setting all higher modes to zero before the conversion. Therefore, any difference in the results of grid B and D originates from the different choice of pixel sizes, and because grid D covers a sphere in Fourier space whereas grid B covers a cube, since no individual component of the wavevector in grid B can have a value above 0.8 h Mpc^{1} and wavevectors with a length above that can only be reached in the corners of the cube.
Grids used for conversion of matter density spectra.
To see the effect of the grid on the conversion we plot a selection of forward converted spectra using all four grids divided by the corresponding emulated spectra in Fig. D.1 and the backward converted spectra divided by the corresponding linear spectra in Fig. D.2. In grid D the power spectrum is only filled up to k = 1.4 h Mpc^{1} before the conversion, higher modes are set to zero. In the backward conversion the power spectra start to differ around k = 0.9 h Mpc^{1}, where the result from grid D starts to overshoot the others. In the forward conversion the differences are much more prominent. For redshift 0 the spectrum from grid C exhibits a clear increase in broadband power on all scales, because at z = 0 the region with 1.4 h Mpc^{1}<k ≤ 3.4 h Mpc^{1} contains more power than the region with k ≤ 1.4 h Mpc^{1}. This additional power couples to all scales in the forward conversion. However, for redshifts greater than 1 the spectra appear to be consistent up to k = 0.8 h Mpc^{1} and grids A, B, and D appear to be consistent at all redshifts. Table D.3 lists the logdistances up to k = 1.0 h Mpc^{1} for grids A, C, and D with respect to grid B. One can see, that the logdistances are comparable with the logdistances of grid B with respect to the emulated and linear spectra listed in Table D.1. We therefore conclude that the calculation is consistent between the investigated grids within the precision of our model. There is however a systematic trend apparent in Fig. D.1 that an increase in total power due to a greater covered krange leads to an increase in broadband power in the forward converted spectra. We therefore expect the validity of our model to break down for higher high dynamic ranges as the total power of the Cosmic matter spectrum diverges, since its spectral index towards high k is above − 3. The problem with a spectral index above − 3 can be seen best in the angle integrated conversion formula Eq. (13).
Logdistances for k ≤ 1.0 h Mpc^{1} between the converted spectra at different grids.
Fig. D.1
Forward converted spectra using different grids at a selection of redshifts. The panels show the ratio between the forward converted spectrum and the emulated spectrum (CosmicEmu for redshifts 0, 0.5, and 1 and 3PT else). The solid line corresponds to grid B (the grid used in Sect. 3), the dashed line to grid A, the dotdashed line to grid C, and the dotted line to grid D. 

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Fig. D.2
Backward converted spectra using different grids at a selection of redshifts. The panels show the ratio between the backward converted emulated spectrum (emulators as in Fig. D.1) and the linear spectrum. The solid line corresponds to grid B (the grid used in Sect. 3), the dashed line to grid A, the dotdashed line to grid C, and the dotted line to grid D. 

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Appendix D.3: Strength of the smearing of BAO
We estimate the strength of the smearing of baryon acoustic oscillations by comparing to a smoothing (with respect to log (k)) of the linear spectrum using a Gaussian kernel, (D.4)where σ_{g} is the smoothing length in terms of efolds. σ_{g} is a dimensionless distance in log (k). The smoothed spectrum is therefore (D.5)We can compare P_{nl}/P_{nl,nw} with P_{sm}(σ_{g}) /P_{lin,nw} in order to find a σ_{g} where the smoothing appears to be similar. The higher σ_{g}, the stronger the smoothing. Here, P_{nl} denotes the nonlinear power spectrum with BAO, P_{nl,nw} the nonlinear power spectrum without BAO, and P_{lin,nw} the linear power spectrum without BAO. The best value for σ_{g} at each redshift is found by visual comparison in the absence of a more rigorous criterion. We list the best fit values for different redshifts for the 3PT spectra as well as the forward converted spectra in Table D.4. The values for the CosmicEmu spectra are missing because the CosmicEmu code did not allow us to calculate nonlinear power spectra without BAO.
Best fit smoothing scales of a Gaussian smoothing on logscale that emulate the smearing of BAO for the 3PT spectra and the forward converted spectra at different redshifts.
Appendix D.4: Largescale bias
Neyrinck et al. (2009) find a bias factor between the power spectra of the density contrast and the logarithmic density, which they fit to exp( − Var [ log (1 + δ) ]) with high accuracy up to z ≈ 1.2. If the density field follows lognormal statistics the correlation functions of the density and logdensity are related by (D.6)which simplifies under the assumption of statistical homogeneity and a zero mean for s to (D.7)where . This prefactor is the square of the expectation value of ρ, (D.8)In Sect. 3 of this work, we compared the spectra of the δ and e^{s}/ ⟨e^{s}⟩ since the density contrast is defined around a mean of 1. In the backward conversion, the mean of the resulting logdensity field was not zero. Equation (18) determined it as (D.9)for all redshifts (to 0.1% precision). However, this prefactor should not appear in the work of Neyrinck et al. (2009), since they compare the power spectra of δ and s = log (1 + δ), where δ = ρ/ρ_{0} − 1. This means that the prefactor in Equation (D.7)is already divided out.
There is an additional bias apart from this factor, which can be seen best in the low redshift panels in the left part of Fig. 4. Here the forward converted power spectrum exceeds the original power spectrum even at the lowest kbin. This is not due to the prefactor presented in the previous paragraph, but simply to mode coupling in the forward conversion. The inverse of this effect is present in the backward conversion, where the backward (i.e., logtransformed) power spectrum undershoots the linear power spectrum at the lowest kbin. This factor is, however, much weaker than what Neyrinck et al. (2009) find. For completeness, we list the factors between the lowest kbins, i.e., P_{backward}(k → 0) /P_{emulated}(k → 0), in Table D.5. In conclusion, the lognormal model offers no insight to the bias factor found by Neyrinck et al. (2009).
Largescale bias factors due to mode coupling.
Appendix D.5: Generating matter densities in spaces spanning in redshift
In Sect. 3 we have established that the power spectra of the exponentiated linear density contrast agree with the emulated spectra to a reasonable accuracy down to redshift 1 and k ≤ 1.0 h Mpc^{1}. Therefore, the logdensity at different redshifts is (in a statistical average) related by a simple global prefactor. This enables us to formulate a local function which translates the density between different redshifts to better accuracy than linear theory. We let G(z;z_{0}) be the growth factor between redshift z_{0} and redshift z and δ(z) the density contrast at a given redshift. Then we have (D.10)where Var [· ] is the variance in one cell.
Using this formula one can easily generate a lognormal field that behaves like the matter density contrast to a good accuracy. One simply takes z_{0} to be sufficiently high so that Var[δ(z_{0})] ≪ 1 and log (1 + δ(z_{0})) ≈ δ(z_{0}). At such a redshift a Gaussian random field generated from the matter power spectrum desribes the statistics of δ(z_{0}) very well. By applying Eq. (D.10)using a position dependent redshift z(x), (D.11)one can now generate a lognormal matter density contrast that follows the appropriate nonlinear matter power spectrum in each position (or redshift slice).
All Tables
Highest logdistance (for k ≤ 1.0 h Mpc^{1}) between the forward converted spectra and the emulated spectra (3PT and CosmicEmu, respectively) and the backward converted emulated spectra and the linear spectra.
Logdistances for k ≤ 1.0 h Mpc^{1} between the converted spectra at different grids.
Best fit smoothing scales of a Gaussian smoothing on logscale that emulate the smearing of BAO for the 3PT spectra and the forward converted spectra at different redshifts.
All Figures
Fig. 1
Conversion formalism for redshifts 1 to 7. Left panel: forward converted linear spectra (solid lines) and the corresponding 3PT spectra (dashed lines), which are both divided by the respective linear spectrum for better comparison of the nonlinearities. Right panel: backward converted 3PT spectra (solid lines) and linear spectra (dashed lines), which are both divided by the respective 3PT spectrum. 

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In the text 
Fig. 2
Conversion formalism for redshifts 1 to 7. Left panel: forward converted linear spectra (solid lines) divided by the corresponding 3PT spectra. Right panel: backward converted 3PT spectra (solid lines) divided by the respective linear spectrum. The dashed line marks 1. 

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In the text 
Fig. 3
Conversion formalism for redshifts 0 to 1. Left panel: forward converted linear spectra (solid lines) and the corresponding CosmicEmu spectra (dashed lines), which are both divided by the respective linear spectrum for better comparison of the nonlinearities. Right panel: backward converted CosmicEmu spectra (solid lines) and linear spectra (dashed lines), which are both divided by the respective CosmicEmu spectrum. 

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In the text 
Fig. 4
Conversion formalism for redshifts 0 to 1. Left panel: forward converted linear spectra (solid lines) divided by the corresponding CosmicEmu spectra. Right panel: backward converted CosmicEmu spectra (solid lines) divided by the respective linear spectrum. The dashed line marks 1. 

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In the text 
Fig. 5
BAO smearing. Left panel: 3PT spectra with BAO divided by the 3PT spectra without BAO at several redshifts. Right panel: forward converted linear spectra with BAO divided by the forward converted linear spectra without BAO. We note the smearing of smallscale wiggles towards lower redshifts in the left panel. 

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In the text 
Fig. A.1
Backward conversion applied to a onedimensional power spectrum P_{ρ}(k) (solid line) yields the power spectrum P_{s}(k) (dashed line). 

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In the text 
Fig. A.2
A onedimensional lognormal random field following the power spectrum P_{ρ}(k) from Fig. A.1. 

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In the text 
Fig. D.1
Forward converted spectra using different grids at a selection of redshifts. The panels show the ratio between the forward converted spectrum and the emulated spectrum (CosmicEmu for redshifts 0, 0.5, and 1 and 3PT else). The solid line corresponds to grid B (the grid used in Sect. 3), the dashed line to grid A, the dotdashed line to grid C, and the dotted line to grid D. 

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In the text 
Fig. D.2
Backward converted spectra using different grids at a selection of redshifts. The panels show the ratio between the backward converted emulated spectrum (emulators as in Fig. D.1) and the linear spectrum. The solid line corresponds to grid B (the grid used in Sect. 3), the dashed line to grid A, the dotdashed line to grid C, and the dotted line to grid D. 

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In the text 
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