Anatomy of chiral magnetic effect in and out of equilibrium

Anatomy of chiral magnetic effect in and out of equilibrium

Dmitri Kharzeev Department of Physics and Astronomy, Stony Brook University, Stony Brook, New York 11794-3800, USA Department of Physics, Brookhaven National Laboratory, Upton, NY 11973, USA RIKEN-BNL Research Center, Brookhaven National Laboratory, Upton, New York 11973-5000, USA    Mikhail Stephanov Physics Department, University of Illinois at Chicago, Chicago, Illinois 60607, USA    Ho-Ung Yee Physics Department, University of Illinois at Chicago, Chicago, Illinois 60607, USA RIKEN-BNL Research Center, Brookhaven National Laboratory, Upton, New York 11973-5000, USA
Abstract

We identify a new contribution to the chiral magnetic conductivity at finite frequencies – the magnetization current. This allows to quantitatively reproduce the known field-theoretic time-dependent (AC) chiral magnetic response in terms of kinetic theory. We evaluate the corresponding AC chiral magnetic conductivity in two flavor QCD plasma at weak coupling. The magnetization current results from the spin response of chiral quasiparticles to magnetic field, and is thus proportional to the quasiparticle’s -factor. In condensed matter systems, where the chiral quasi-particles are emergent and the -factor can significantly differ from 2, this opens the possibility to tune the AC chiral magnetic response.

pacs:
12.38.Mh,72.10.Bg,75.45.+j
preprint: RBRC-1212

I Introduction and summary

The Chiral Magnetic Effect (CME) Fukushima:2008xe () (see Kharzeev:2013ffa (); Kharzeev:2012ph (); Miransky:2015ava (); Kharzeev:2015znc (); Landsteiner:2016led () for reviews and additional references) is the generation of electric current along an external magnetic field induced by the imbalance in the densities of right- and left-handed chiral fermions. It has been observed recently in Dirac Li:2014bha (); Xiong:2015 () and Weyl Huang:2015 (); Zhang:2015 () semimetals. An evidence for CME in the quark-gluon plasma has been previously reported by high-energy heavy ion experiments at RHIC Abelev:2009ac (); Abelev:2009ad (); Adamczyk:2015eqo () and LHC Adam:2015vje ().

In the limit of a constant external magnetic field, the CME conductivity is completely fixed by the chiral anomaly:

(1)

where is the chiral chemical potential describing the amount of imbalance between the densities of right- and left-handed fermions in the system. Because it is topologically protected, the zero frequency CME conductivity is universal and is not modified by interactions (even though the magnitude of magnetic field can be of course renormalized). As a result, the CME conductivity is reproduced in approaches that assume very different properties of the system, including perturbation theory (weak coupling) Fukushima:2008xe (); Kharzeev:2009pj (), holographic correspondence (strong coupling) Yee:2009vw (); Rebhan:2009vc (); Gynther:2010ed (), hydrodynamics Son:2009tf (); Kharzeev:2011ds (), and kinetic theory Son:2012wh (); Stephanov:2012ki (); Chen:2012ca (); Son:2012zy (); Basar:2013qia (); Chen:2014cla (); Monteiro:2015mea ().

However the frequency dependence of the CME conductivity in an oscillating magnetic field presents the following puzzle Kharzeev:2009pj (): the real part of the conductivity drops from to as soon as the frequency deviates from . The computation in Kharzeev:2009pj () has been performed using leading order perturbation theory, and thus assumed the absence of interactions between the fermions. Taking account of these interactions through the damping of fermion propagators smoothens out the discontinuity in Satow:2014lva (), as conjectured in Kharzeev:2009pj (). In the collisionless limit of Kharzeev:2009pj (), this perturbative field-theoretic result has to be reproduced by the Chiral Kinetic Theory (CKT) without the collision term – and here there appears to be a problem, as we will now explain.

Indeed, kinetic theory operates with the single particle distributions, and so the field-theoretic result of Kharzeev:2009pj () may be interpreted in terms of the particle energy shift due to the interaction of chiral particle’s magnetic moment with magnetic field , . In equilibrium, this energy shift aligns with to lower the energy, which in turn aligns the momentum of chiral particles along . The asymmetry between the left- and right-handed particles then results in the electric current – however, as will be shown below, this alignment is responsible only for of the result (1). We will see that the rest results from a more kinematic effect including the Berry curvature of the monopole in momentum space Volovik:2003fe (), that modifies both the phase space measure and the particle velocity. In fact, without Berry curvature, the kinematic modification of particle velocity due to the interaction with magnetic field yields a contribution to the current equal to of (1), and cancels exactly the contribution arising from the particle’s energy shift - there is thus no CME in equilibrium without the Berry curvature. Since Berry curvature in momentum space is a quasi-classical description of chiral anomaly, this explains why there is no CME in a system of chirally imbalanced fermions in the absence of anomaly Vilenkin:1980fu (); Vilenkin:1980ft ().

When an external magnetic field oscillates with frequency that exceeds the inverse relaxation time , , the system is driven out of equilibrium, and the contribution to CME conductivity from the energy shift in equilibrium distributions should disappear. Since the leading order perturbative result of Kharzeev:2009pj () corresponds to , this means that as soon as deviates from zero, the CME conductivity should only contain the contribution from the kinematic effects including Berry curvature that does not require equilibrium and hence survives at finite frequency. Based on this, we might expect that at small non-zero the CME conductivity should become – in sharp contrast to computed in Kharzeev:2009pj ().

What is the origin of this discrepancy between the field-theoretic and kinetic theory results? It appears that in the kinetic theory description we miss a contribution to the CME conductivity that at finite frequency is negative and given by , and that vanishes in equilibrium, when .

In this paper we identify this missing contribution and show that it is the magnetization current resulting from magnetization density of chiral particles:

(2)

At frequencies the magnetization current contributes an additional to the chiral magnetic conductivity , whereas at zero frequency this contribution vanishes.

Since in chiral materials the Lorentz invariance is in general lost, the identification of individual contributions to the chiral magnetic conductivity at finite frequency may make it possible to manipulate them separately.

Ii CME in static equilibrium

We start our discussion with a dissection of chiral magnetic conductivity in static equilibrium. Throughout the paper, we shall assume that the chirality relaxation time is long enough (in particular, much longer than the typical relaxation time) that it makes sense to consider the chirally imbalanced system as being close to equilibrium.

For brevity, we will consider a weakly interacting theory of single chiral (Weyl) fermion species of right-handed chirality; the generalization to a massless Dirac fermion (as well as to QCD in chiral limit) is straightforward. In this theory, the equilibrium CME current is given by where is a chemical potential for the chiral charge of the Weyl fermion.

In weakly coupled regime, a natural description of the system is in terms of a kinetic theory of quasi-particles described by the Boltzmann equation with collisions. Collision terms that cause the system to relax to the thermal equilibrium set a characteristic relaxation time scale which, due to weak coupling, is much longer than the thermal quasi-particle scale, where is the system’s temperature. If the external background (such as the magnetic field ) changes with a rate slower than , we expect the system to stay in local thermal equilibrium; the hydrodynamic description of the system then applies. On the other hand, if an external field changes with a rate faster than , the collision terms become sub-leading and the Boltzmann equation reduces to the kinetic theory of non-interacting quasi-particles at leading order. Therefore, serves as a crossover scale between hydrodynamic regime and the free streaming (collisionless) kinetic theory. In this section we will focus on CME in the hydrodynamic regime.

Quantization of a single right-handed Weyl field gives “particles” of helicity and U(1) chiral charge , as well as “anti-particles” carrying and . We will call them fermions and anti-fermions in the following, while the term “quasi-particles” will be used to refer to both. The helicity defines the spin of a quasi-particle along its momentum direction as . Since the magnetic moment is given by (with the factor ), we see that the fermion and anti-fermion with a given momentum carry the same magnetic moment . In the presence of magnetic field , their energy is shifted by the same amount from the relativistic massless spectrum . In equilibrium, this energy shift should give rise to a tendency of aligning with to lower the energy, which in turn aligns the momentum of quasi-particles along : this has long been a qualitative explanation of CME in weakly coupled theory.

We will be more quantitative on this. The equilibrium thermal distributions of fermions () and anti-fermions () in the magnetic field become

(3)

where is the Fermi-Dirac distribution with a chemical potential and temperature , that we have expanded to linear order in . The U(1) charge current in kinetic theory (in leading order gradient expansion) is easy to understand intuitively: , where and is the quasi-particle velocity which is to leading order in (we will come back to accounting the correction to velocity shortly). Then the net current resulting from the shift of distributions in (3) is

(4)

where we have used an identity

(5)

that holds independently of temperature . We see that the shift of thermal equilibrium distribution from the magnetic moment interaction (3) explains only of the expected value of CME in equilibrium.

To identify the remaining , we need a more careful description of kinetic theory of chiral fermions: the chiral kinetic theory. A novel element in chiral kinetic theory is the inclusion of quantum effect originating from chiral spinors in first order of , which appears as a Berry curvature of monopole shape in momentum space: . This Berry curvature has been shown to be sufficient to describe the chiral anomaly in the framework of kinetic theory of quasi-particles Son:2012wh (); Stephanov:2012ki (); Chen:2012ca (); Son:2012zy (); Basar:2013qia (); Chen:2014cla (); Monteiro:2015mea (). We will now show that this Berry curvature plays a crucial role in explaining the rest of the equilibrium CME conductivity.

The Berry curvature modifies the charge current in the following way: it affects the phase space measure , and also changes the quasi-particle velocity :

To linear order in , the contribution to the net current arising from this modification of phase space and velocity (that is independent of the modification of the thermal equilibrium distribution considered above) can be obtained by using as

(6)

where we use the identity that is related to the identity (5) via integration by parts. Because this term in the current arises from the modification of quasiparticle velocity, we will call (6) the kinematic contribution to CME; it is responsible for of the equilibrium CME conductivity.

If we had not included the Berry curvature, and simply used with (obtained by putting ), it is easy to check that we would get the kinematic contribution of that would cancel (4) resulting in the zero total CME in equilibrium. In other words, the change in the velocity due to the energy shift from magnetic moment interaction with magnetic field precisely cancels the contribution from the shift of thermal equilibrium distribution due to the same energy shift in the equilibrium CME. We see that the net amount of the equilibrium CME, , originates solely from the Berry curvature.

The dissection of into and described above is important both conceptually and practically when we consider out-of-equilibrium CME in free streaming regime discussed in the next section. In this regime, the thermal relaxation governed by the time scale cannot follow the fast change of the system induced by the time dependence of the background field. The contribution to CME from the shift of thermal equilibrium distribution is expected to be lost, while the kinematic contribution that does not rely on relaxation dynamics should persist. We may thus naively expect that about of the equilibrium CME (carried by ) will survive in out-of equilibrium conditions. Interestingly, in the next section, we will see that the story of CME in out-of equilibrium is more subtle.

Iii Out-of equilibrium CME

One way of driving the system out-of equilibrium is to apply a magnetic field oscillating in time with frequency . When the system reaches a stationary phase, the CME current oscillates with the same frequency and we can define a chiral magnetic conductivity by in frequency space. In the hydrodynamic regime , thermal relaxation dynamics is able to sustain instantaneous thermal equilibrium, and the chiral magnetic conductivity should approach the equilibrium value . In the free-streaming regime on the other hand, the system is unable to follow the rapidly oscillating magnetic field, and the distribution functions cannot deviate much from . We would expect that only the kinematic contribution of CME, , manifests itself and that in the free streaming regime.

A first hint of what should be truly happening in free streaming regime can be seen in the diagrammatic 1-loop computation of in Ref.Kharzeev:2009pj (), as well as in the Hard Thermal Loop (HTL) computation of Ref.Son:2012zy (); Satow:2014lva (); Manuel:2013zaa (). The real part of at agrees with the equilibrium value as expected, while it drops discontinuously to for an infinitesimally non-zero . A careful inspection shows that this behavior of arises from the structure

(7)

which is a good approximation to the full in the kinetic HTL regime . The presence of is an artifact of non-interacting limit, which is replaced by the effective relaxation rate that smoothens the discontinuity at Satow:2014lva (). The important fact for us is that this result indicates in the free streaming regime after this replacement. As we mentioned in the Introduction, this is in puzzling contradiction to our expectation of based on the dissection of equilibrium CME into and . Since both and follow from the structure of chiral kinetic theory, the only possible solution should be an existence of yet another contribution to CME that vanishes in hydrodynamic regime (i.e. in equilibrium) and approaches in the free-streaming regime. We will now show that such a contribution indeed exists.

The charge current we presented before, is the leading classical term in the expansion in powers of . Since the Berry curvature in momentum space is the first quantum correction in this parameter, we have to consider the first quantum corrections to the expression for . One such correction is a magnetization current arising from quantum spins of quasi-particles Chen:2014cla (): where the magnetization density is given by the sum of magnetic moments of quasi-particles (recall that fermion and anti-fermion with a given momentum carry the same magnetic moment),

(8)

In fact, one can show that the current is responsible for the kinematic contribution of of the equilibrium chiral vortical effect (CVE) in the presence of non-zero fluid vorticity, and the rest of equilibrium CVE arises from the shift of thermal equilibrium distribution in the presence of vorticity Chen:2014cla (): this closely parallels the dissection of equilibrium CME we discuss before. It turns out that this quantum current also gives rise to the additional contribution to out-of equilibrium CME, as we will now demonstrate.

The key element is the Bianchi identity, the well-known Faraday’s Law of induction, between a time-dependent magnetic field and a space-dependent electric field, which in the frequency space becomes . Note that this is an identity in terms of vector potential : the time-dependent magnetic field is a space-dependent electric field . The electric field gives a local acceleration to quasi-particles , and the free streaming Boltzmann equation in frequency space becomes

(9)

The solution of this equation to linear order in with a retarded boundary condition is with . The should be replaced in the interacting theory by that appears in the collision term of the Boltzmann equation, that we neglect in free streaming regime. The spin magnetization from this distribution is (see 8)

(10)

This gives the magnetization current (2)

(11)

that contributes an additional to the chiral magnetic conductivity in free-streaming regime : . Together with , this explains the total CME current of in the free streaming regime. Note that the physics of is independent of the Berry curvature.

Table 1: The dissection of CME in the hydrodynamic () and the free-streaming () regimes. The numbers are in units of the equilibrium CME conductivity.

Iv Dependence on the g-factor

The anatomy of CME in and out-of equilibrium presented above depends on the -factor (taken to be for relativistic chiral fermions), and it is easy to generalize our results to an arbitrary value of -factor. This discussion should be important in Dirac/Weyl semi-metals where the emergent pseudo-chiral fermions are expected to have a dynamically determined -factor different from . It also helps us to disentangle the physics of Berry curvature and the physics of spin magnetic moment (-factor). The magnetic moment of a quasi-particle of momentum is , and therefore the contribution from the shift of thermal distribution in equilibrium is modified by a factor of , which becomes . It is easy to check that the effect of the Berry curvature together with the new energy shift gives

which results in the kinematic contribution to equilibrium CME as . As expected, the total equilibrium CME, , is robust and does not depend on the value of -factor.

In the free streaming regime , only the kinematic contribution of survives. On the other hand, the spin magnetization changes by a factor of , therefore the magnetization current contribution will change by the same factor and become . The total CME in the free streaming regime is then .

It is interesting to consider what the results would look like in the absence Berry curvature (which can be seen by keeping only the terms with the -factor). The equilibrium CME is absent in this case, while the CME in free-streaming regime is . Interestingly, the existence of CME in free streaming regime does not necessarily require the Berry curvature, but its value would be smaller by from the one with the Berry curvature. The importance of distinguishing the effects of the Berry curvature and of the magnetic moment has been also emphasized in the context of gyrotropic effect Moore1 (); Moore2 (); Pesin (). We emphasize again that the equilibrium CME in hydrodynamic regime, , is a consequence of the Berry curvature, independent of the physics of spin magnetic moment (-factor).

Table 2: The dissection of CME with an arbitrary -factor. The terms with the -factor originate from the physics of spin magnetic moment, and the others from the physics of Berry curvature.

V Interpolating hydrodynamic regime and free streaming regime

In interacting systems, such as QCD and Dirac/Weyl semi-metals in weakly coupled regime, the transition between the hydrodynamic regime and the free streaming regime should be well approximated by a function

(12)

with a single effective parameter with a dimension of time. One way to fix this parameter is to consider a small frequency expansion, with , where is one of the parity-odd transport coefficients in second order hydrodynamics, Kharzeev:2011ds (). In two-flavor QCD, it has been computed in leading-log accuracy of coupling constant by re-summing leading pinch singularities Jimenez-Alba:2015bia (), , which gives (with )

(13)

We also mention that the imaginary part of is proportional to the parity-odd spectral density Jimenez-Alba:2015bia (); Mamo:2015xkw () that appears in the thermal fluctuation-dissipation relation of charge current . As can be seen from (12) the is proportional to the -factor – this provides an intuitive explanation of why , though it arises from the same triangle diagram, is sensitive to the microscopic details of dynamics that are not constrained by the chiral anomaly.

Vi Towards a full quantum description of AC chiral magnetic conductivity in QCD

To describe the AC CME conductivity , we have to keep in mind that the kinetic theory is valid only in the classical regime of quasi-particles, , where characterizes the typical energy-momentum of thermal quasi-particles. For the probing scale is smaller than the Compton length of quasi-particles, and the response function is governed by quantum dynamics. This quantum response is dominated by a sum of one-particle responses of quasi-particles without collisions (since the scale of collisions is well separated from , see (13)), and it is reliably captured by a 1-loop diagrammatic computation Kharzeev:2009pj ().

This suggests a smooth interpolation of the previous kinetic theory result (12) in with a 1-loop diagrammatic result in . In FIG. 1, we plot the emerging global picture of in two-flavor perturbative QCD with (neglecting the log factor) and . For comparison, we also show a result in the AdS/CFT correspondence for strongly coupled regime. One can see that at large frequency the pQCD and AdS/CFT results for the real part of conductivity approach each other, whereas at small frequency these results significantly differ signaling the difference in the relaxation mechanisms in these approaches. At zero frequency, the CME conductivity is completely fixed by the chiral anomaly and is universal. The imaginary part of AC conductivity is seen to exhibit different behavior both at small and large frequencies.

Figure 1: The real (blue) and imaginary (red) parts of in two-flavor pQCD with and (solid lines). The dotted curves are the results in the AdS/CFT correspondence Yee:2009vw ().

Vii Discussion

We have identified the new contribution to chiral magnetic conductivity – the magnetization current (11) that allows to quantitatively reproduce the field-theoretic AC response in terms of kinetic theory. The magnetization current results from the spin response of chiral quasiparticles to magnetic field, and is thus proportional to the quasiparticle’s -factor, see Table II.

The Lorentz-invariance of Dirac and Weyl actions fixes the value of -factor to , and the field-theoretic result automatically takes account of the corresponding magnetization current contribution. However, in Dirac/Weyl semimetals, the chiral quasiparticles are emergent, and the value of -factor can significantly differ from – for example, in that possesses 3D Dirac quasiparticles with a finite mass of about meV the value of -factor is Wolos () due to a strong spin-orbit interaction. Moreover, left- and right-handed chiral quasiparticles may have different properties in so-called asymmetric Weyl semimetals, leading to essential modification of CME Kharzeev:2016mvi ().

Therefore, the identification of individual contributions to CME conductivity presented above opens the possibility to tune the chiral magnetic response at finite frequencies by choosing the appropriate chiral materials.

Viii Acknowledgment

We thank Qiang Li, Larry McLerran, Dam Son and Naoki Yamamoto for useful comments. This work is partially supported by the U.S. Department of Energy, Office of Science, Office of Nuclear Physics, within the framework of the Beam Energy Scan Theory (BEST) Topical Collaboration, and grant No. DE-FG0201ER41195.

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