Constraints on primordial magnetic fields from the optical depth of the cosmic microwave background

# Constraints on primordial magnetic fields from the optical depth of the cosmic microwave background

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###### Abstract

Damping of magnetic fields via ambipolar diffusion and decay of magnetohydrodynamical (MHD) turbulence in the post decoupling era heats the intergalactic medium (IGM). Delayed recombination of hydrogen atoms in the IGM yields an optical depth to scattering of the cosmic microwave background (CMB). The optical depth generated at does not affect the “reionization bump” of the CMB polarization power spectrum at low multipoles, but affects the temperature and polarization power spectra at high multipoles. Writing the present-day energy density of fields smoothed over the damping scale at the decoupling epoch as , we constrain as a function of the spectral index, . Using the Planck 2013 likelihood code that uses the Planck temperature and lensing data together with the WMAP 9-year polarization data, we find the 95% upper bounds of , 0.39, and 0.18 nG for , , and , respectively. For these spectral indices, the optical depth is dominated by dissipation of the decaying MHD turbulence that occurs shortly after the decoupling epoch. Our limits are stronger than the previous limits ignoring the effects of the fields on ionization history. Inverse Compton scattering of CMB photons off electrons in the heated IGM distorts the thermal spectrum of CMB. Our limits on imply that the -type distortion from dissipation of fields in the post decoupling era should be smaller than , , and , respectively.

a]Kerstin E. Kunze, b,c]Eiichiro Komatsu Prepared for submission to JCAP

Constraints on primordial magnetic fields from the optical depth of the cosmic microwave background

• Departamento de Física Fundamental and IUFFyM, Universidad de Salamanca, Plaza de la Merced s/n, 37008 Salamanca, Spain

• Max-Planck-Institut für Astrophysik, Karl-Schwarzschild-Str. 1, 85748 Garching, Germany

• Kavli Institute for the Physics and Mathematics of the Universe (WPI), Todai Institutes for Advanced Study, The University of Tokyo, 5-1-5 Kashiwanoha, Kashiwa, Chiba 277-8583, Japan

E-mail: kkunze@usal.es

## 1 Introduction

Damping of magnetic fields affects the thermal and ionization history of the universe. The damping processes before the decoupling epoch can be approximately modeled by damping of three magnetic modes. Of these, damping of the fast magnetosonic waves proceeds in a similar way as the Silk damping of density perturbations, resulting in a damping scale on the order of the Silk scale. Slow magnetosonic and Alfvén waves can avoid damping up to smaller scales, resulting in a larger damping wave number. The value at the decoupling epoch is given by [1, 2]

 kd,dec=299.66cosθ(B01 nG)−1Mpc−1, (1.1)

for the best-fit CDM model of the “Planck 2013+WP” data [3]. Here, is the angle between the wave vector and the field direction which will be set to zero in this paper.

We assume that the magnetic field is a non-helical and Gaussian random field with its two-point function in Fourier space given by

 ⟨B∗i(→k)Bj(→q)⟩=(2π)3δ(→k−→q)PB(k)(δij−kikjk2), (1.2)

where the power spectrum, , is assumed to be a power law, , with the amplitude, , and the spectral index, . This can be expressed in terms of the ensemble average of the present-day magnetic energy density by

 ⟨ρB,0⟩=∫d3k(2π)3PB,0(k)e−2(kkc)2, (1.3)

where is a Gaussian smoothing scale. The power-law magnetic power spectrum then gives

 PB,0(k)=4π2k3c2(nB+3)/2Γ(nB+32)(kkc)nB⟨ρB,0⟩. (1.4)

For convenience, we define a smoothed magnetic field strength at the present epoch, , as , where is a wavenumber corresponding to . In this paper, we shall set to the maximal wave number determined by the damping scale at the decoupling epoch, , given by equation (1.1). For simplicity we shall write throughout the rest of the paper.

Primordial magnetic fields present before the decoupling epoch can generate scalar, vector, and tensor modes of CMB temperature and polarization anisotropies [4, 5, 6, 7, 8]. In general, there are two different types; namely, the compensated magnetic mode which is similar to an isocurvature mode, and the passive mode due to the presence of anisotropic stress of the magnetic field before neutrino decoupling. The latter is just like a curvature mode with its amplitude determined by the magnetic anisotropic stress and the time of generation of the primordial magnetic field. These can be important contributions to the CMB anisotropies, depending on the magnetic field parameters. On small angular scales, the scalar compensated mode as well as the vector mode for nG fields with positive spectral indices, , can dominate over the primary CMB anisotropies. On large angular scales, the tensor compensated mode for a few nG fields with a nearly scale invariant spectrum, , can dominate [9]. However, here we shall ignore these contributions and derive constraints focusing only on the effect of dissipation of fields in the post decoupling era. Since we only consider , the former contributions can be ignored. The limit we obtain for is smaller than nG, making the latter contributions sub-dominant. In any case, including these contributions in the analysis would make the constraints on stronger.

After the decoupling epoch, magnetic fields are damped by ambipolar diffusion and decaying MHD turbulence [10]. This leads to a change in the ionization and thermal history, hence the visibility function of CMB anisotropies. In ref. [11], we have calculated the thermal and ionization history of the IGM including dissipation of fields. Ionization gives an optical depth to Thomson scattering of the CMB. By writing the total optical depth as , the additional contribution from dissipation of magnetic fields is given by111This formula is a minor update of the formula we gave in ref. [11]. We now use the Planck 13+WP best fit cosmological parameters. Following ref. [9, 12], we calculate the photoionization rates at the photon temperature instead of the electron temperature in the modified version of Recfast++, and include the collisional ionization. Finally, we have also corrected a numerical error in the amplitude of the ambipolar diffusion heating rate. We are grateful to J. Chluba for helping us implement these updates.

 Δτ(B0,nB) = 0.0241(B0nG)1.547(−nB)−0.0370 (1.5) × e−5.2815×10−12(−nB)23.8731+5.4×10−3(B0nG)3.3706−7.1×10−3(−nB)1.948(B0nG)2.0713

for .

In general, there are two important contributions to the total optical depth out to the decoupling epoch: the contribution due to reionization, , and that generated at high redshifts close to decoupling, . Hence . Whereas determines the CMB polarization angular power spectrum at low multipoles (“reionization bump”), the total optical depth out to decoupling determines the overall suppression of the temperature power spectrum at high multipoles as . As the contribution to the optical depth from dissipation of fields comes from high redshifts, , it has little effect on and hence the CMB polarization power spectrum at low multipoles. Therefore, the change in the amplitude of the temperature angular power spectrum induced by the magnetic field dissipation is determined by , and the temperature data at high multipoles will be the key to measure this effect. In this paper, we shall use the Planck 2013 temperature data [13, 14] (including the lensing data [15]) and the Planck 13 polarization likelihood [14] derived from the WMAP 9-year polarization data [16, 17] to constrain for some representative values of . In particular, the lensing data play an important role in isolating the optical depth in the temperature data.

The rest of the paper is organized as follows. In section 2, we calculate the CMB temperature and polarization power spectra with a modified thermal and reionization history due to the dissipation of the magnetic field in the post decoupling era. In section 3, we obtain constraints on the magnetic field strength for some representative values of . We conclude in section 4.

## 2 CMB anisotropies with dissipation of magnetic fields in the post-decoupling era

Dissipation of magnetic fields in the post decoupling era takes place by two processes; namely, ambipolar diffusion and decaying MHD turbulence [10]. These processes affect the evolution of the electron temperature, , as

 ˙Te=−2˙aaTe+xe1+xe8ργσT3mec(Tγ−Te)+xeΓ1.5kBne, (2.1)

where the dissipation rate, , includes the contribution from ambipolar diffusion, , and decaying MHD turbulence, . The other variables are: the scale factor, the photon temperature, the Thomson scattering cross section, the ionization fraction, the electron number density, the photon energy density, the electron rest mass, the speed of light, and the Boltzmann constant.

Ambipolar diffusion is due to different velocities of the neutral and the ionized matter components in the presence of a magnetic field. As this velocity difference is caused by the action of the Lorentz force on the ionized component, the dissipation rate of ambipolar diffusion is determined by the Lorentz term as [10]

 Γin=ρn16π2γρ2bρi|(→∇×→B)×→B|2, (2.2)

where , , and are the energy densities of neutral hydrogen, ionized hydrogen, and the total baryons, respectively, and is the coupling between the ionized and neutral component given by with  cm s [18]. Equation (2.2) is evaluated for the average Lorentz force using the two point function of the magnetic field (cf., eq. (1.2)). The final expression depends on the magnetic field strength as well as on its spectral index, and can be found in [11].

Dissipation of the magnetic field due to decaying MHD turbulence rests on the fact that turbulence is no longer suppressed in the plasma after the decoupling epoch. On scales below the magnetic Jeans scale, the magnetic energy on large scales is transferred to small scales and dissipates. The dissipation rate of this highly non linear process is estimated by numerical simulations of MHD turbulence in flat space using the fact that there exists an appropriate rescaling of variables in flat space to match those in an expanding, flat Friedmann-Robertson-Walker background [19, 20, 21, 22, 23, 24]. In the matter-dominated era, the estimated dissipation rate of a non-helical magnetic field is given by [10]

 Γdecay=B208π3m2[ln(1+tdti)]m[ln(1+tdti)+ln[(1+zi1+z)32]]m+1H(t)(1+z)4, (2.3)

where is the present-day field value assuming a flux freezing; is related to the magnetic spectral index as ; is the physical decay time scale for turbulence given by with the magnetic Jeans wavenumber of Mpc [10]; and and are the redshift and time at which dissipation of the magnetic field due to decaying MHD turbulence becomes important.

Ref. [10] calculated the evolution of the matter temperature, , and the ionization fraction, , with the effect of damping of magnetic fields in the post decoupling era. In ref. [11], we revisited these calculations using a modified version of Recfast++ [25, 26, 27, 28, 29, 30, 31]. We found that ambipolar diffusion contributes at , and the effect decreases as decreases. The amplitude is proportional to . On the other hand, the effect of decaying MHD turbulence increases as decreases, is proportional to , and dominates over ambipolar diffusion up to intermediate redshifts.

In figure 1 we show the evolution of , , the visibility function of CMB (), and the optical depth to scattering of CMB (), as a function of redshift. For each choice of parameters, we show the case including the standard implementation of instantaneous reionization (denoted as “s r”) and not including it (denoted as “no s r”). We use the CLASS code [32, 33, 34, 35] to compute these quantities. The standard implementation of CLASS is the same as in the CAMB code [36, 37], which uses a tanh fitting formula for the ionization fraction centered at the reionization redshift. The case not including the standard reionization is shown only for comparison. Dissipation of the decaying turbulence heats the IGM since shortly after the decoupling epoch, delaying recombination of hydrogen atoms in the IGM. At low redshifts, , the temperature of the completely reionized universe falls as decreases because ambipolar diffusion cannot act on ionized plasma. In a complete treatment of the late time thermal and ionization history one should also include contributions from stellar feedback which ionizes and can efficiently heat the IGM up to temperatures of  K at . Since our main conclusions are not based on the temperature but on the ionization fraction, the error in the temperature evolution at has no consequences. Decay of MHD turbulence increases the total optical depth to scattering of CMB shortly after the decoupling epoch, and this changes the power spectra of the temperature and polarization anisotropies, as discussed below.

We use the CLASS code with its standard implementation of instantaneous reionization at late times to calculate the power spectra, and show the effects of dissipation of fields in figure 2 for a magnetic field with nG and spectral indices of , , and . It is well known that the optical depth to scattering of CMB suppresses the temperature and polarization power spectra by at multipoles higher than that corresponding to the horizon size at the epoch of the scattering. In addition to the suppression due to the standard late-time reionization, the optical depth due to dissipation of fields, , creates an additional suppression of the power spectra by (see figure 2). Also, as the peak of the visibility function of CMB shifts slightly toward a lower redshift than the standard decoupling redshift, the angular diameter distance to the decoupling epoch is slightly reduced, shifting the locations of the acoustic peaks of the temperature and polarization power spectra to lower multipoles. This effect is more pronounced for polarization, and is clearly visible in the top right panel of figure 2.

Not only does an additional optical depth suppress the power spectra at multipoles higher than that corresponding to the horizon size at the epoch of the scattering, but also creates an additional polarization at multipoles corresponding to the horizon size at the epoch of the scattering. The amplitudes of the first and second peaks in the -mode polarization power spectrum at and are enhanced due to regeneration of polarization by additional scattering of CMB between the decoupling and the reionization epochs. This can be seen in the top right panel of figure 2. While the polarization power spectrum at higher multipoles is significantly influenced by the change in the optical depth, that at lower multipoles is not. The “reionization bump” in the polarization power spectrum at is not affected by dissipation of the fields, as ionization at is totally dominated by that of the late-time reionization. Similar features are observed in the temperature-polarization cross power spectrum (cf. lower panel of figure 2). This phenomenology is similar to the effect of heating due to annihilation of dark matter particles [38, 39, 40, 3].

The top left panel of figure 2 shows that the low- temperature power spectrum increases with increasing magnetic spectral index. We find that this is due to an enhanced Doppler term (in Newtonian gauge). For our choice of parameters this is most noticeable for the largest spectral index, . In the left panel of figure 3, we show the contributions from the Sachs-Wolfe term, the integrated Sachs-Wolfe term, the Doppler term, and the polarization term to the total angular power spectrum. The right panel shows only the Doppler term, which increases as increases at . This explains what we find in the top left panel of figure 2.

## 3 Parameter estimation

To estimate the magnetic field parameters along with the cosmological parameters, we use Markov chains Monte Carlo as implemented in montepython [41]. Specifically, we fix the magnetic spectral index, , and vary the field strength, , along with the six standard CDM parameters, i.e., the Hubble constant, ; the physical baryon density, ; the physical cold dark matter density, ; the amplitude of the scalar power spectrum at , ; the tilt of the power spectrum, ; and the optical depth from the late-time reionization, .

We use the Planck 2013 temperature data [13, 14] (including the lensing data [15]) and the likelihood of the WMAP 9-year polarization data [16, 17] derived by the Planck collaboration [14]. The lensing data are essential for breaking degeneracy between and . This degeneracy arises because the optical depth constraint from the temperature data is degenerate with . (The temperature data effectively measure .) In our study the key element is that the magnetic field dissipation significantly changes the optical depth close to decoupling and so changes the total optical depth to decoupling but does not change the optical depth to reionization. The former is determined by the temperature anisotropy data and the latter by the polarization data. The combination of the two data sets together with the lensing data allows to constrain the magnetic field parameters.

We summarize the constraints on and the cosmological parameters in table 1, and show the marginalized posterior distributions of in figure 4. We chose , , and as representative cases. We find no evidence for dissipation of the magnetic fields in the data. The 95% CL upper bounds on the field strength are , 0.39, and 0.18 nG for , , and , respectively.222The corresponding smoothing scales are much smaller than 1 Mpc. The largest one is of order 13 kpc for  nG, and 4 kpc for nG (cf. equation (1.1)).

These limits are significantly stronger than those from the magnetic scalar- and vector-mode contributions to the angular power spectra of the CMB. For example, the Planck collaboration used the Planck 2013 temperature data, the WMAP 9-year polarization data, and the high- temperature data of ACT and SPT to find  nG (95% CL) for a smoothing scale of 1 Mpc from the magnetic scalar and vector modes, while ignoring the effects on the ionization history of the universe. Our limits on , which is smoothed over the magnetic damping scale at decoupling, become stronger if we scale them to a Mpc scale, as changing the smoothing scale, , to a different smoothing scale, , leads to a rescaling of the magnetic field amplitude by a factor of .

The only limit in the literature that is stronger than ours is  nG for a smoothing scale of 0.1 kpc [42], which was derived from the change in the ionization history before the decoupling epoch, due to the effect of clumping in the baryon density perturbations induced by a primordial magnetic field. Rescaling our limits to 0.1 kpc makes their limit much stronger than ours.

In figure 5 the two-dimensional marginalized posterior probability density distributions ( versus the cosmological parameters) are shown, for , , and . Most of the cosmological parameters are determined independently of ; however, the scalar spectral tilt, , is weakly correlated with because suppresses the power spectrum at high multipoles by , which can be partly compensated by increasing .

## 4 Conclusions

Dissipation of the magnetic fields in the post-decoupling era heats the IGM and delays recombination of hydrogen atoms. This effect can be detected as the extra optical depth to scattering of CMB photons. A qualitatively new effect is that it affects only the total optical depth to decoupling, which is determined by the temperature data together with the lensing data, but not the optical depth to reionization inferred from the low- polarization data (). Using the 2013 Planck data including the CMB lensing data, together with the likelihood of the low- polarization data from WMAP as derived by the Planck collaboration, we find no evidence for the effect of dissipation of (non-helical) magnetic fields in the CMB data. The 95% CL upper bounds are , 0.39, and 0.18 nG for , , and , respectively. These limits are stronger than the previous limits that did not use the effect of fields on ionization history of the universe.

Inverse Compton scattering of CMB photons by hot electrons in the IGM heated by dissipating magnetic fields in the post decoupling era leads to a -type spectral distortion [43]. For negative magnetic spectral indices, the Compton parameter is well approximated by (see footnote 1 for the update from ref. [11])

 y(nB,B0) = 1.2194×10−5(B0nG)1.7263(−nB)0.3602 (4.1) −1.2155×10−5(B0nG)1.7260(−nB)0.3619e9.3978×10−9(−nB)10.9842.

For the upper limits on the magnetic field amplitudes derived in this paper, the resulting -type distortions are , , and for , , and , respectively. These limits are well below the contribution from the thermal Sunyaev-Zel’dovich effect in galaxy clusters and groups, [44], and thus are negligible.

We expect that this new method would yield much improved limits, once the full Planck data sets including high- polarization are used, as they provide significantly better measurement of the CMB lensing (which fixes thus breaking degeneracy between and ), and potentially measure the extra polarization at generated by dissipation of decaying MHD turbulence.

## 5 Acknowledgements

We would like to thank J. Chluba for very useful discussions. KEK would like to thank the Max-Planck-Institute for Astrophysics and the Perimeter Institute for Theoretical Physics for hospitality where part of this work was done. This research was supported in part by Perimeter Institute for Theoretical Physics. Research at Perimeter Institute is supported by the Government of Canada through Industry Canada and by the Province of Ontario through the Ministry of Economic Development & Innovation. KEK acknowledges financial support by Spanish Science Ministry grants FIS2012-30926 and CSD2007-00042. We acknowledge the use of the Legacy Archive for Microwave Background Data Analysis (LAMBDA). Support for LAMBDA is provided by the NASA Office of Space Science.

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