Electromagnetic signatures of the chiral anomaly in Weyl semimetals

# Electromagnetic signatures of the chiral anomaly in Weyl semimetals

Edwin Barnes    J. J. Heremans    Djordje Minic Department of Physics, Virginia Tech, Blacksburg, VA 24061, U.S.A.
July 12, 2019
###### Abstract

Weyl semimetals are predicted to realize the three-dimensional axial anomaly first discussed in particle physics. The anomaly leads to unusual transport phenomena such as the chiral magnetic effect in which an applied magnetic field induces a current parallel to the field. Here we investigate diagnostics of the axial anomaly based on the fundamental equations of axion electrodynamics. We find that materials with Weyl nodes of opposite chirality and finite energy separation immersed in a uniform magnetic field exhibit an anomaly-induced oscillatory magnetic field with a period set by the chemical potential difference of the nodes. In the case where a chemical potential imbalance is created by applying parallel electric and magnetic fields, we find a suppression of the magnetic field component parallel to the electric field inside the material for rectangular samples, suggesting that the chiral magnetic current opposes this imbalance. For cylindrical geometries, we instead find an enhancement of this magnetic field component along with an anomaly-induced azimuthal component. We propose experiments to detect such magnetic signatures of the axial anomaly.

###### pacs:

Dirac/Weyl semimetals are topological states of matter in which the 3D bulk contains Dirac or Weyl points protected by crystalline symmetries and near which the low-energy quasiparticles are linearly dispersing massless Dirac/Weyl fermions Herring (1937); Abrikosov and Beneslavskiĭ (1970); Wan et al. (2011); Burkov and Balents (2011); Young et al. (2012); Zyuzin et al. (2012). While Dirac semimetals were theorized early on Herring (1937); Abrikosov and Beneslavskiĭ (1970), Weyl semimetals were predicted only recently, with pyrochlore iridates such as YIrO as examples Wan et al. (2011). The prediction that Weyl semimetals host exotic topological surface states distinct from those in other materials spurred extensive experimental efforts to confirm the existence of both Dirac and Weyl semimetal phases, leading to Dirac semimetal discoveries such as NaBi and CdAs Wang et al. (2013); Liu et al. (2014a); Borisenko et al. (2014); Liu et al. (2014b); Neupane et al. (2014), and recent Weyl semimetal discoveries such as TaAs and NbAs Huang et al. (2015); Weng et al. (2015); Lv et al. (2015, 2015); Xu et al. (2015, 2015).

Theoretical works have shown that Dirac semimetals lie at the intersection of several types of topological states reachable by breaking symmetries including inversion, time-reversal, or crystal symmetries Wan et al. (2011); Burkov and Balents (2011); Young et al. (2012); Zyuzin et al. (2012); Wang et al. (2013); Weng et al. (2015); Huang et al. (2015). For example, breaking crystal symmetries can cause Weyl nodes in the bulk to couple and open a band gap, which can produce a topological insulator Wang et al. (2013). The breaking of either time-reversal or inversion symmetry can result in a stable Weyl semimetal state which hosts topological Fermi arc states on the material’s surface Wan et al. (2011); Burkov and Balents (2011); Hosur et al. (2012); Wang et al. (2013); Xu et al. (2015); Weng et al. (2015); Huang et al. (2015).

Weyl semimetals are also expected to show unusual phenomena associated with the three-dimensional axial anomaly Zyuzin and Burkov (2012); Chen et al. (2013); Khaidukov et al. (2013); Goswami et al. (2013). Notable among these is the chiral magnetic effect (CME) in which the application of an external magnetic field produces a current Son and Yamamoto (2012); Son and Spivak (2013); Burkov (2014). This effect has also been studied in the contexts of quark-gluon plasmas Fukushima et al. (2008); Nielsen and Ninomiya (1983) and topological insulators Fu and Kane (2007); Teo et al. (2008); Qi et al. (2008); Hasan and Kane (2010); Li et al. (2010); Kim et al. (2013). Transport measurements in Weyl semimetals revealed a negative longitudinal magnetoresistance as a diagnostic for the CME He et al. (2014); Liang et al. (2015); Zhang et al. (2016); Li et al. (2016a). Debate exists whether this transport signature necessarily implies the CME Goswami et al. (2015), and in this Letter we thus develop a diagnostic based on magnetic properties, which finds a parallel in the development of the London penetration depth in superconductors.

The approach is based on self-consistent solutions to Maxwell’s equations in the presence of anomalous chiral currents. Even for currents derived in the limit of linear response, the electromagnetic fields should be obtained self-consistently as becomes clear when starting with the fundamental equations of axion electrodynamics—the relevant effective field theoretic description when the axial anomaly is present. We obtain such solutions for systems in which the chiral chemical potential is either intrinsic or induced by parallel electric and magnetic fields. In both cases, we find that the solutions exhibit detectable signatures due to the presence of the axial anomaly.

The defining characteristic of axion electrodynamics is captured by the axionic term in the action Wilczek (1987) (in addition to the canonical term),

 Sθ=α4π2∫d3xdtθ→E⋅→B, (1)

where is the electric field, and is the fine structure constant. The parameter , when dependent on space and time, is called the axion field in the particle physics context. The relevant equations of axion electrodynamics are well known Goswami et al. (2013); Sikivie (1984); Huang and Sikivie (1985); Wilczek (1987); Carroll et al. (1990)

 ∇⋅→E=ρ−κ∇θ⋅→B,∇×→E=−∂→B∂t, (2)

together with

 ∇⋅→B=0,∇×→B=∂→E∂t+→j+κ(∂θ∂t→B+∇θ×→E). (3)

Note that when the axion profile is linear in time, , one obtains for stationary fields that with constant , a result known as the Beltrami equation and which is well known 111We thank Roman Buniy and Tom Kephart for discussions about this connection. in the context of plasma physics Beltrami (1889); Buniy and Kephart (2014); Gorbar et al. (2013); Khaidukov et al. (2013).

We proceed with a brief review of the CME as a physical consequence of the chiral anomaly Fukushima et al. (2008). Consider the minimal coupling of the carriers of such as chiral fermions to an external gauge field. First we rewrite the axion term in a covariant way Then we perform a rotation in the minimal coupling of fermions to the gauge field in order to obtain In particular if we concentrate on the th (temporal) component we get where the chiral chemical potential is given as The energy spectrum of the free Dirac equation in the presence of a chiral chemical potential is for the massless modes (assuming 1D) where represents the spin in the direction and stand for the right and left chirality. If the chiral chemical potential is positive, a net chirality is created, thus lifting the degeneracy between the R and L modes. lifts the degeneracy in spin, depending on the charge of the particle. Therefore particles with the right-handed helicity will move opposite to the antiparticles (holes) with the right-handed helicity, thus creating . This is the CME Fukushima et al. (2008). The physics underlying this reasoning harks back to the original papers on chiral anomalies Adler (1969); Bell and Jackiw (1969). The total current is given as the volume integral, where the current density is given as the expectation value, and where the fermion field can be written in terms of the left- and right-handed components , so that, Here and , where are the canonical Pauli matrices.

As pointed out in Fukushima et al. (2008), one path to the CME in the context of quark-gluon plasmas uses the argument based on energy balance as presented originally in Nielsen and Ninomiya (1983). One considers a situation with and in the presence of a chiral chemical potential and relates the work performed by in to the energy penalty related to the chirality change (given essentially by the volume integral over ), i.e. Therefore is proportional to (even in the limit) which is the defining expression for the CME.

The final equation (in SI units, with constants recovered to facilitate evaluation), , does not depend on covariance and thus it can be realized in many-body systems, such as Weyl semimetals. In this context, should be interpreted as the energy separation of bulk Weyl nodes, Zyuzin and Burkov (2012); Chen et al. (2013). In the case of Weyl semimetals, one must take care to show that nonlinearities in the dispersion do not remove the anomaly by solving a quantum kinetic equation. This approach has been used to show that the chiral magnetic current is not an equilibrium current, but still holds at arbitrarily low frequencies Vazifeh and Franz (2013); Chen et al. (2013); Goswami et al. (2013). A second important difference in the Weyl semimetal context is that the axion field also depends on the Weyl node momentum separation: , so that the last term in Eq. (3) gives rise to an anomalous Hall effect Zyuzin and Burkov (2012). We thus have the well-known result Zyuzin and Burkov (2012); Vazifeh and Franz (2013); Chen et al. (2013); Goswami et al. (2013) (in SI units, with )

 →∇×→B=μ0→j=−μ0e22π2ℏ2Δε→B+μ0e22π2ℏ2Δ→p×→E. (4)

While our main focus here is on Weyl semimetals, future work may include generalization of our results to other quasi-relativistic materials and to high energy systems such as quark-gluon plasmas.

As a first example of the consequences of Eq. (4), we consider a semi-infinite slab of Weyl semimetal occupying . Suppose that and is constant, and that ; the solution to Eq. (4) is with . Incidentally, this solution is a special case of the more general solution in plasma physics known as the Arnold-Beltrami-Childress flow Arnold and Khesin (1998). In the context of Weyl semimetals, we see that a consequence of the chiral anomaly is that inside the slab, forms a standing wave with wavelength .

In the case of time-dependent fields where and and for constant , solutions to Eqs. (2) and (3) can be obtained by requiring that both and satisfy Beltrami equations: and with . Note that here we have chosen the minus sign in front of the square root to ensure that in the limit, the wave vector of the magnetic field goes to zero faster than the frequency, , as is necessary to ensure the existence of the CME as a non-equilibrium transport phenomenon Chen et al. (2013); Chang and Yang (2015); Ma and Pesin (2015); Zhong et al. (2016). Such Beltrami-type solutions describing the pure CME are only valid if and if the last term in Eq. (4) can be neglected. Since for such solutions , the latter condition requires , which can be satisfied if we take . We must also ensure that is below the threshold for optical absorption: Chang and Yang (2015); Ma and Pesin (2015); Zhong et al. (2016), which in turn gives a constraint on the Weyl node momentum and energy separations: . We can then obtain Beltrami-type solutions within this frequency window by starting from static solutions such as the above semi-infinite slab solution and taking . (The time-dependent solutions of axion electrodynamics have been considered in Fujita and Oshikawa (2016).)

Detectable signatures of axion electrodynamics can be obtained by solving the Beltrami equation in systems with finite dimensions. Consider a long cylinder of Weyl semimetal with radius and axis along immersed in a constant magnetic field, . We work in cylindrical coordinates () and require to be independent of and . The Beltrami equation reduces to

 1rddr(rdBzdr)+ζ2Bz=0,Bϕ=−1ζdBzdr, (5)

and . These equations are easily solved to yield the field inside the cylinder: , . Outside the cylinder, satisfies the ordinary Maxwell equations with a current source . Using that and employing Stokes’ theorem, we obtain the full solution inside and outside:

 Bϕ = B0[J1(ζr)J0(ζR)Θ(R−r)+RJ1(ζR)rJ0(ζR)Θ(r−R)], Bz = B0[J0(ζr)J0(ζR)Θ(R−r)+Θ(r−R)]. (6)

This solution is shown in Fig. 1. The maximal value of occurs at the center of the cylinder, where . Outside the cylinder, the chiral anomaly gives rise to a which depends on and which varies quasi-periodically with the cylinder size at fixed .

Although the CME has not yet been observed in Weyl semimetals where the energy separation between Weyl nodes persists in the absence of externally applied fields, experimental observations in a Dirac semimetal in which the degeneracy of Dirac nodes is lifted through the application of non-orthogonal and have been reported Zhang et al. (2016); Li et al. (2016b, a); Xiong et al. (2015, 2015); Wang et al. (2016) following theoretical predictions Gorbar et al. (2013). In this case, an anomalous current parallel to is still generated Son and Spivak (2013); Burkov (2014), with a magnitude depending on : Unlike the pure CME relation, , the above relation is not captured by axion electrodynamics and does not require time-dependent fields Zhong et al. (2016). However, combining this relation with Ampere’s law, we still obtain a self-consistent equation for the local in the material (SI units):

 ∇×→B=μ0→j=μ0σa(→E⋅→B)→B. (7)

To illustrate consequences of Eq. (7), consider the case with constant and applied along the -direction, , , with the semimetal occupying the semi-infinite space , and with boundary conditions , , . We look for solutions of the form , in which case Eq. (7) reduces to:

 B′x=μ0σaE0B2y,B′y=−μ0σaE0BxBy. (8)

These two equations together imply We can then parameterize the two components in terms of a new function, , for which Eq. (8) implies This equation is readily solved: with the constant of integration chosen to respect . We obtain for inside the material:

 →B=B0tanh(z/Λ)^x+B0sech(z/Λ)^y. (9)

Thus decays exponentially over a characteristic length into the bulk, while grows from to over a similar distance. In the bulk thus becomes orthogonal to , in turn implying that exists only near the surface. Maxwell’s equations would thus seem to oppose the separation of Weyl nodes due to the chiral anomaly.

A similar effect persists even in the presence of an additional Ohmic current (conductivity ): With , Eq. (8) becomes

 B′x=μ0σaE0B2y+μ0σ0E0,B′y=−μ0σaE0BxBy. (10)

Writing , Eqs. (10) become

 d|→B|dz=μ0σ0E0cosφ,φ′cscφ=−μ0σ0E0|→B|(σaσ0|→B|2+1). (11)

Unlike the previous case lacking the Ohmic term, here we note that not only the direction but also the magnitude of varies with . The second equation in (11) can be integrated to yield Combining this with the first equation in (11) and writing , with , yields

 h′′(ξ)+β2[h′(ξ)]2−2β(1+β)2h(ξ)=2(1+β)2, (12)

where . We want to find solutions to (12) that obey the boundary conditions (since ) and , where is the angle of the relative to the -axis at . Given a solution to Eq. (12) for the magnitude of , its orientation follows from Before looking for solutions to Eq. (12) in the presence of both the Ohmic and anomalous currents, it is instructive to first consider the solution that arises in the absence of the anomalous current. Setting in Eq. (10), we obtain We see that the Ohmic current produces a nonzero that grows linearly with distance into the bulk, while remains constant.

We have found that both the Ohmic and anomalous currents generate a component of perpendicular to which grows with distance into the bulk of the material. In the case of the anomalous current however, this growth saturates, and the component of parallel to is simultaneously suppressed over the length scale . When both currents are nonzero, it is necessary to solve Eq. (12) numerically; the results are shown in Fig. 2 for various values of . It is evident from the figure that always decays when the anomalous current is present, albeit over longer and longer distances as is increased.

We also present a solution to Eq. (7) for the case of a long cylinder (radius ) in applied fields and . Writing where again , this equation reduces to

 r2ff′′+rff′−r2(f′)2−1=0, (13)

and , . Eq. (13) can be solved exactly: , where is one integration constant, while the other has been chosen to ensure that , are nonsingular at . Since everywhere outside the cylinder, continuity of requires , implying . The magnetic field inside and outside is then

 Bϕ = 2B0Λrr2+k2Θ(R−r)+B0(2Λ−k)rΘ(r−R), Bz = 2B0Λkr2+k2Θ(R−r)+B0Θ(r−R). (14)

This solution is valid for and assumes that is sufficiently small that screening of the electric field is negligible. As for the pure CME (Eq. (6)), the axial anomaly produces a maximal at and a nonzero outside the cylinder with a -dependent magnitude.

The characteristic length can be evaluated using Son and Spivak (2013); Burkov (2014); Zhang et al. (2016); Li et al. (2016b, a); Xiong et al. (2015)

 σa=le4τa4π4ℏ4g(EF) (15)

where is the number of Weyl node pairs, is the density of states at the Fermi level and is the relaxation time for charge pumping between Weyl node pairs. Characteristic values for the Weyl semimetal TaAs Zhang et al. (2016) are and , yielding (for ) . These values yield 9.6 cm, for = 1 V/m and = 1 T as typical experimental values of applied and . A of this magnitude would lead to detectable effects in magnetometry measurements performed in SQUID or VSM systems with planar gradiometer geometries to access spatial variations of . As an additional diagnostic the magnetometer results can be compared on samples of different sizes, above and below . An increase in and would result in a proportional decrease in the characteristic length , allowing a measure of tuning to sample size and yet a further diagnostic. Magnetometry hence functions for Weyl fermion materials as an alternative to magnetoresistance measurements, in parallel to the case of superconducting materials. can vary widely for the different materials hosting Weyl fermions currently described in the literature, due to differences in and . In Dirac materials, , where and are the spin- and valley degeneracies resp., and is the velocity constant characterizing the Dirac dispersion. Equation (15) then shows that a low (hence low carrier density), high and long lead to shorter and more readily observable effects in magnetometry. A longer is expected to arise from higher carrier mobility Li et al. (2016b); Xiong et al. (2015, 2015). Currently TaAs forms a promising candidate, while estimates of can be much longer and would not be conducive to ready observations, at least currently, in CdAs microwires Li et al. (2016b), or in Zr Te Li et al. (2016a). However, strides are being made to lower carrier densities and further increase mobilities in many Weyl fermion materials Xiong et al. (2015); Liang et al. (2015); Wang et al. (2016); Shekhar et al. (2015), which will lead to much reduced .

In conclusion, we have presented a diagnostic procedure for the chiral magnetic effect, additional to negative magnetoresistance and motivated by the fundamental equations of axion electrodynamics. The procedure is based on the penetration of magnetic fields over characteristic length scales in Weyl semimetals.

Acknowledgements: We would like to thank R. Buniy, T. Kephart, G. Sharma and E. N. Economou for interesting conversations and helpful comments. The work of D.M. was supported in part by the U.S. Department of Energy under contract DE-FG02-13ER41917. The work of J.J.H. was supported by the U.S. Department of Energy, Office of Basic Energy Sciences, Division of Materials Sciences and Engineering under award DOE DE-FG02-08ER46532.

## References

• Herring (1937) C. Herring, Phys. Rev. 52, 365 (1937).
• Abrikosov and Beneslavskiĭ (1970) A. A. Abrikosov and S. D. Beneslavskiĭ, Zh. Eksp. Teor. Fiz. 32, 699 (1970).
• Wan et al. (2011) X. Wan, A. M. Turner, A. Vishwanath,  and S. Y. Savrasov, Phys. Rev. B 83, 205101 (2011).
• Burkov and Balents (2011) A. A. Burkov and L. Balents, Phys. Rev. Lett. 107, 127205 (2011).
• Young et al. (2012) S. M. Young, S. Zaheer, J. C. Y. Teo, C. L. Kane, E. J. Mele,  and A. M. Rappe, Phys. Rev. Lett. 108, 140405 (2012).
• Zyuzin et al. (2012) A. A. Zyuzin, S. Wu,  and A. A. Burkov, Phys. Rev. B 85, 165110 (2012).
• Wang et al. (2013) Z. Wang, H. Weng, Q. Wu, X. Dai,  and Z. Fang, Phys. Rev. B 88, 125427 (2013).
• Liu et al. (2014a) Z. K. Liu, B. Zhou, Y. Zhang, Z. J. Wang, H. M. Weng, D. Prabhakaran, S.-K. Mo, Z. X. Shen, Z. Fang, X. Dai, Z. Hussain,  and Y. L. Chen, Science 343, 864 (2014a).
• Borisenko et al. (2014) S. Borisenko, Q. Gibson, D. Evtushinsky, V. Zabolotnyy, B. Büchner,  and R. J. Cava, Phys. Rev. Lett. 113, 027603 (2014).
• Liu et al. (2014b) Z. K. Liu, J. Jiang, B. Zhou, Z. J. Wang, Y. Zhang, H. M. Weng, D. Prabhakaran, S.-K. Mo, H. Peng, P. Dudin, T. Kim, M. Hoesch, Z. Fang, X. Dai, Z. X. Shen, D. L. Feng, Z. Hussain,  and Y. L. Chen, Nat. Mater. 13, 677 (2014b).
• Neupane et al. (2014) M. Neupane, S.-Y. Xu, R. Sankar, N. Alidoust, G. Bian, C. Liu, I. Belopolski, T.-R. Chang, H.-T. Jeng, H. Lin, A. Bansil, F. Chou,  and M. Z. Hasan, Nat. Commun. 5, 3786 (2014).
• Huang et al. (2015) S.-M. Huang, S.-Y. Xu, I. Belopolski, C.-C. Lee, G. Chang, B. Wang, N. Alidoust, G. Bian, M. Neupane, A. Bansil, H. Lin,  and M. Zahid Hasan, Nat. Commun. 6, 7373 (2015).
• Weng et al. (2015) H. Weng, C. Fang, Z. Fang, B. A. Bernevig,  and X. Dai, Phys. Rev. X 5, 011029 (2015).
• Lv et al. (2015) B. Q. Lv, H. M. Weng, B. B. Fu, X. P. Wang, H. Miao, J. Ma, P. Richard, X. C. Huang, L. X. Zhao, G. F. Chen, Z. Fang, X. Dai, T. Qian,  and H. Ding, Phys. Rev. X 5, 031013 (2015).
• Lv et al. (2015) B. Q. Lv, N. Xu, H. M. Weng, J. Z. Ma, P. Richard, X. C. Huang, L. X. Zhao, G. F. Chen, C. Matt, F. Bisti, V. Strokov, J. Mesot, Z. Fang, X. Dai, T. Qian, M. Shi,  and H. Ding, Nat. Phys. 11, 724 (2015).
• Xu et al. (2015) S.-Y. Xu, I. Belopolski, N. Alidoust, M. Neupane, G. Bian, C. Zhang, R. Sankar, G. Chang, Z. Yuan, C.-C. Lee, S.-M. Huang, H. Zheng, J. Ma, D. S. Sanchez, B. Wang, A. Bansil, F. Chou, P. P. Shibayev, H. Lin, S. Jia,  and M. Z. Hasan, Science 349, 613 (2015).
• Xu et al. (2015) S.-Y. Xu, N. Alidoust, I. Belopolski, C. Zhang, G. Bian, T.-R. Chang, H. Zheng, V. Strokov, D. S. Sanchez, G. Chang, Z. Yuan, D. Mou, Y. Wu, L. Huang, C.-C. Lee, S.-M. Huang, B. Wang, A. Bansil, H.-T. Jeng, T. Neupert, A. Kaminski, H. Lin, S. Jia,  and M. Zahid Hasan, Nat. Phys. 11, 748 (2015).
• Hosur et al. (2012) P. Hosur, S. A. Parameswaran,  and A. Vishwanath, Phys. Rev. Lett. 108, 046602 (2012).
• Zyuzin and Burkov (2012) A. A. Zyuzin and A. A. Burkov, Phys. Rev. B 86, 115133 (2012).
• Chen et al. (2013) Y. Chen, S. Wu,  and A. A. Burkov, Phys. Rev. B 88, 125105 (2013).
• Khaidukov et al. (2013) Z. V. Khaidukov, V. P. Kirilin, A. V. Sadofyev,  and V. I. Zakharov, ArXiv e-prints  (2013), arXiv:1307.0138 [hep-th] .
• Goswami et al. (2013) P. Goswami,  and S. Tewari, Phys. Rev. B 88, 245107 (2013).
• Son and Yamamoto (2012) D. T. Son and N. Yamamoto, Phys. Rev. Lett. 109, 181602 (2012).
• Son and Spivak (2013) D. T. Son and B. Z. Spivak, Phys. Rev. B 88, 104412 (2013).
• Burkov (2014) A. A. Burkov, Phys. Rev. Lett. 113, 247203 (2014).
• Fukushima et al. (2008) K. Fukushima, D. E. Kharzeev,  and H. J. Warringa, Phys. Rev. D 78, 074033 (2008).
• Nielsen and Ninomiya (1983) H. B. Nielsen and M. Ninomiya, Phys. Lett. B 130, 389 (1983).
• Fu and Kane (2007) L. Fu and C. L. Kane, Phys. Rev. B 76, 045302 (2007).
• Teo et al. (2008) J. C. Y. Teo, L. Fu,  and C. L. Kane, Phys. Rev. B 78, 045426 (2008).
• Qi et al. (2008) X.-L. Qi, T. L. Hughes,  and S.-C. Zhang, Phys. Rev. B 78, 195424 (2008).
• Hasan and Kane (2010) M. Z. Hasan and C. L. Kane, Rev. Mod. Phys. 82, 3045 (2010).
• Li et al. (2010) R. Li, J. Wang, X.-L. Qi,  and S.-C. Zhang, Nat. Phys. 6, 284 (2010).
• Kim et al. (2013) H.-J. Kim, K.-S. Kim, J.-F. Wang, M. Sasaki, N. Satoh, A. Ohnishi, M. Kitaura, M. Yang,  and L. Li, Phys. Rev. Lett. 111, 246603 (2013).
• He et al. (2014) L. P. He, X. C. Hong, J. K. Dong, J. Pan, Z. Zhang, J. Zhang,  and S. Y. Li, Phys. Rev. Lett. 113, 246402 (2014).
• Liang et al. (2015) T. Liang, Q. Gibson, M. N. Ali, M. Liu, R. J. Cava,  and N. P. Ong, Nat. Mater. 14, 280 (2015).
• Zhang et al. (2016) C.-L. Zhang, S.-Y. Xu, I. Belopolski, Z. Yuan, Z. Lin, B. Tong, G. Bian, N. Alidoust, C.-C. Lee, S.-M. Huang, T.-R. Chang, G. Chang, C.-H. Hsu, H.-T. Jeng, M. Neupane, D. S. Sanchez, H. Zheng, J. Wang, H. Lin, C. Zhang, H.-Z. Lu, S.-Q. Shen, T. Neupert, M. Z. Hasan,  and S. Jia, Nat. Commun. 7, 10735 (2016).
• Li et al. (2016a) Q. Li, D. E. Kharzeev, C. Zhang, Y. Huang, I. Pletikosic, A. V. Fedorov, R. D. Zhong, J. A. Schneeloch, G. D. Gu,  and T. Valla, Nat. Phys. 12, 550 (2016a).
• Goswami et al. (2015) P. Goswami, J. H. Pixley,  and S. Das Sarma, Phys. Rev. B 92, 075205 (2015).
• Wilczek (1987) F. Wilczek, Phys. Rev. Lett. 58, 1799 (1987).
• Sikivie (1984) P. Sikivie, Physics Letters B 137, 353 (1984).
• Huang and Sikivie (1985) M. C. Huang and P. Sikivie, Phys. Rev. D 32, 1560 (1985).
• Carroll et al. (1990) S. M. Carroll, G. B. Field and R. Jackiw, Phys. Rev. D 41, 1231 (1990).
• Beltrami (1889) E. Beltrami, Rendiconti del Reale Instituto Lombardo, Series II, Vol. 22  (1889).
• Buniy and Kephart (2014) R. V. Buniy and T. W. Kephart, Annals Phys. 344, 179 (2014).
• Gorbar et al. (2013) E. V. Gorbar, V. A. Miransky,  and I. A. Shovkovy, Phys. Rev. B 88, 165105 (2013).
• Bell and Jackiw (1969) J. S. Bell and R. Jackiw, Nuovo Cim. A 60, 47 (1969).
• Vazifeh and Franz (2013) M. M. Vazifeh and M. Franz, Phys. Rev. Lett. 111, 027201 (2013).
• Arnold and Khesin (1998) V. Arnold and B. Khesin, Springer-Verlag  (1998).
• Chang and Yang (2015) M.-C. Chang and M.-F. Yang, Phys. Rev. B 91, 115203 (2015).
• Ma and Pesin (2015) J. Ma and D. A. Pesin, Phys. Rev. B 92, 235205 (2015).
• Zhong et al. (2016) S. Zhong, J. E. Moore,  and I. Souza, Phys. Rev. Lett. 116, 077201 (2016).
• Fujita and Oshikawa (2016) H. Fujita and M. Oshikawa, ArXiv e-prints  (2016), arXiv:1602.00687 [cond-mat.str-el] .
• Li et al. (2016b) H. Li, H. He, H.-Z. Lu, H. Zhang, H. Liu, R. Ma, Z. Fan, S.-Q. Shen,  and J. Wang, Nat. Commun. 7, 10301 (2016b).
• Xiong et al. (2015) J. Xiong, S. K. Kushwaha, T. Liang, J. W. Krizan, M. Hirschberger, W. Wang, R. J. Cava,  and N. P. Ong, Science 350, 413 (2015).
• Xiong et al. (2015) J. Xiong, S. K. Kushwaha, T. Liang, J. W. Krizan, W. Wang, R. J. Cava,  and N. P. Ong, ArXiv e-prints  (2015), arXiv:1503.08179 [cond-mat.str-el] .
• Wang et al. (2016) Z. Wang, Y. Zheng, Z. Shen, Y. Lu, H. Fang, F. Sheng, Y. Zhou, X. Yang, Y. Li, C. Feng,  and Z.-A. Xu, Phys. Rev. B 93, 121112 (2016).
• Shekhar et al. (2015) C. Shekhar, A. K. Nayak, Y. Sun, M. Schmidt, M. Nicklas, I. Leermakers, U. Zeitler, Y. Skourski, J. Wosnitza, Z. Liu, Y. Chen, W. Schnelle, H. Borrmann, Y. Grin, C. Felser,  and B. Yan, Nat. Phys. 11, 645 (2015).
You are adding the first comment!
How to quickly get a good reply:
• Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
• Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
• Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters