## Abstract

Time-reversal invariant superconductors in three dimensions may contain nodal lines in the Brillouin zone, which behave as Wilson loops of 3D momentum-space Chern-Simons theory of the Berry connection. Here we study the conditions of realizing linked nodal lines (Wilson loops), which yield a topological contribution to the thermal magnetoelectric coefficient that is given by the Chern-Simons action. We find the essential conditions are the existence of torus or higher genus Fermi surfaces and spiral spin textures. We construct such a model with two torus Fermi surfaces, where a generic spin-dependent interaction leads to double-helix-like linked nodal lines as the superconductivity is developed.

Original language | English (US) |
---|---|

Article number | 147001 |

Journal | Physical review letters |

Volume | 119 |

Issue number | 14 |

DOIs | |

State | Published - Oct 2 2017 |

Externally published | Yes |

## All Science Journal Classification (ASJC) codes

- Physics and Astronomy(all)

## Access to Document

## Other files and links

## Fingerprint

Dive into the research topics of 'Double Helix Nodal Line Superconductor'. Together they form a unique fingerprint.## Cite this

- APA
- Author
- BIBTEX
- Harvard
- Standard
- RIS
- Vancouver

*Physical review letters*,

*119*(14), [147001]. https://doi.org/10.1103/PhysRevLett.119.147001

**Double Helix Nodal Line Superconductor**. In: Physical review letters. 2017 ; Vol. 119, No. 14.

}

*Physical review letters*, vol. 119, no. 14, 147001. https://doi.org/10.1103/PhysRevLett.119.147001

**Double Helix Nodal Line Superconductor.** / Sun, Xiao Qi; Lian, Biao; Zhang, Shou Cheng.

Research output: Contribution to journal › Article › peer-review

TY - JOUR

T1 - Double Helix Nodal Line Superconductor

AU - Sun, Xiao Qi

AU - Lian, Biao

AU - Zhang, Shou Cheng

N1 - Funding Information: Sun Xiao-Qi Lian Biao Zhang Shou-Cheng Department of Physics, McCullough Building, Stanford University , Stanford, California 94305-4045, USA 2 October 2017 6 October 2017 119 14 147001 11 April 2017 © 2017 American Physical Society 2017 American Physical Society Time-reversal invariant superconductors in three dimensions may contain nodal lines in the Brillouin zone, which behave as Wilson loops of 3D momentum-space Chern-Simons theory of the Berry connection. Here we study the conditions of realizing linked nodal lines (Wilson loops), which yield a topological contribution to the thermal magnetoelectric coefficient that is given by the Chern-Simons action. We find the essential conditions are the existence of torus or higher genus Fermi surfaces and spiral spin textures. We construct such a model with two torus Fermi surfaces, where a generic spin-dependent interaction leads to double-helix-like linked nodal lines as the superconductivity is developed. National Science Foundation http://dx.doi.org/10.13039/100000001 NSF http://sws.geonames.org/6252001/ NSF DMR-1305677 The nodal-line superconductor is an intriguing class of three dimensional (3D) unconventional superconductor that respects time-reversal symmetry. Unlike usual superconductors which are fully gapped, a nodal-line superconductor contains closed gapless nodal lines in the Brillouin zone (BZ), which are protected by time-reversal symmetry. In nature, such superconductors widely occur in cuprates [1–4] , iron-based superconductors [5,6] , and noncentrosymmetric superconductors [7,8] . As 1D loops, the nodal lines in the 3D BZ can form nontrivial links [9–12] , where the linking numbers are topologically invariant and give a classification of nodal-line superconductors [9] . Physically, change of linking numbers of nodal lines has been shown to yield a topological shift in the coefficient of thermal magnetoelectric effect, which is also known as the theta angle [9,13,14] . This is because the theta angle is theoretically given by the action of the Chern-Simons (CS) theory of Berry connection in the 3D BZ [13] , while the nodal lines behave exactly as Wilson loops [9] and linking numbers contribute topologically [15,16] . On the surface of the superconductor, linked nodal lines lead to topologically protected kissing Majorana flat bands which are bounded by the projected nodal lines [17–21] . However, superconductors with linked nodal lines have not been discovered. In this Letter, we investigate the physical conditions for realizing linked nodal-line superconductors, and we show the key ingredients for linked nodal lines to occur are torus or higher genus Fermi surfaces and certain spiral spin textures. In particular, we construct a double helix nodal-line superconductor lattice model, which contains two pairs of linked nodal lines resembling the DNA double helix structure [22,23] under the standard BCS mean field theory. Our theory gives a guidance on the search for linked nodal-line superconductors in nature. Though nodal lines could occur in centrosymmetric TRI materials such as cuprates, they appear more commonly in noncentrosymmetric TRI superconductors, where the electron bands are generically nondegenerate due to spin-orbital couplings (SOCs) [8,24] . Here we restrict ourselves to the noncentrosymmetric TRI superconductors, which allows us to consider a larger variety of Hamiltonians. Nodal lines are protected by the time-reversal symmetry. Given an electron band of dispersion ε ( k ) where k is the lattice momentum, the time-reversal symmetry restricts its pairing amplitude Δ ( k ) to be real in a TRI basis [25] . Therefore, the system is gapless when the two conditions ε ( k ) = Δ ( k ) = 0 are satisfied, which gives rise to one-dimensional nodal lines in the BZ. Note that the nodal lines are restricted on the Fermi surface of the band given by ε ( k ) = 0 , so the Fermi surface topology will limit the possible configurations of nodal lines. It is easy to see that a spherical Fermi surface does not support linked nodal lines. While if the Fermi surface is a torus, one is able to draw two nodal lines linked with each other along the toroidal direction of the torus, which resembles a closed DNA double helix. An integer Gauss linking number [15,16,26] n L can be defined for such two nodal lines, which is equal to the total number of coils of the double helix (up to a sign). However, one must note the linking number n L reverses sign under time-reversal transformation, so a double helix cannot be TRI by itself. Instead, the superconductor must contain minimally two double helices which are time reversal partners of each other, and this requires at least two torus Fermi surfaces forming a time reversal pair. Figure 1(a) shows such a configuration of two double helices with linking number n L = ± 1 , respectively, where the two torus Fermi surfaces are cylinders periodic in the k z direction. For Fermi surfaces with a higher genus (number of holes) N g ≥ 2 , it is possible to draw two such double helices on a single TRI Fermi surface, and Fig. 1(d) shows such an example. In nature, Fermi surfaces with a high genus are quite common in metals. 1 10.1103/PhysRevLett.119.147001.f1 FIG. 1. Examples of Fermi surfaces compatible with TRI linked nodal lines. (a)–(c) shows how such linked nodal lines may occur on torus Fermi surfaces. (d) shows a possible configuration of linked nodal lines on a genus two Fermi surface. Given a suitable topology of Fermi surfaces, we still need a nontrivial electron-electron interaction to achieve linked nodal lines in the superconductor. Here we take the example of Fig. 1(a) where two cylindrical torus Fermi surfaces are centered at ( k x , k y ) = ( ± Q x , 0 ) , and investigate how the double-helix linked nodal lines of linking number n L = ± 1 can be realized. The Cooper channel interaction of the superconductor is generically given by H I = ∑ k , k ′ ( V k k ′ / 2 N ) c k † c - k † c - k ′ c k ′ , where c k and c k † are the electron annihilation and creation operators at momentum k near the Fermi surfaces, V k k ′ are the interaction coefficients, and N is the number of unit cells. In the presence of time-reversal symmetry, the pairing amplitude Δ k = ⟨ ∑ k ′ V k k ′ c - k ′ c k ′ ⟩ / N is real. The mean-field free energy of the superconductor is then F ( Δ k ) = ∑ k , k ′ ( Δ k / 2 E k ) V k k ′ ( Δ k ′ / 2 E k ′ ) / 2 N , where E k = ( ε k 2 + Δ k 2 ) 1 / 2 is the Bogoliubov–de Gennes quasiparticle spectrum. Therefore, Δ k and Δ k ′ tend to have the same (opposite) sign for V k k ′ < 0 ( V k k ′ > 0 ). By definition of nodal lines, Δ k on a Fermi surface will take opposite signs on the two sides of a nodal line. For the double helix nodal lines shown in Fig. 1(a) , one finds Δ k Δ k ′ ≤ 0 when k - k ′ = ( 0 , 0 , π ) , or when k and k ′ lie in the same plane of constant k z and opposite to each other on the same cylindrical Fermi surface. This motivates us to write down the following interaction for k and k ′ on the same Fermi surface: V k k ′ = - ( η 1 k x ˜ k x ′ ˜ + η 2 k y k y ′ ) cos ( k z - k z ′ ) , (1) where we have defined k x ˜ = k x ∓ Q x for momentum k near ( k x , k y ) = ( ± Q x , 0 ) , respectively. The interaction at the other momentums can be obtained via the relation V k k ′ = - V k , - k ′ = - V - k , k ′ . We expect the double helix nodal lines with linking number ± 1 to be favored when such a term dominates in the electron-electron interaction near Fermi surfaces. Such a k -dependent interaction can be realized from a spin-dependent Heisenberg interaction together with a spiral Fermi-surface spin texture due to SOC. To illustrate this idea, we can start from two spin-degenerate cylindrical Fermi surfaces at ( k x , k y ) = ( ± Q x , 0 ) , and add a SOC as follows: H soc ( k ) = g ( k ) · σ = λ ( k y σ x - k x ˜ σ y ) + λ z ( sin k z σ x ± cos k z σ y ) , (2) where σ x , y , z are the Pauli matrices for spins, the ± signs correspond to k near ( k x , k y ) = ( ± Q x , 0 ) , respectively, and we keep only the leading order expansion in k x ˜ and k y . Because of the SOC, the Fermi surfaces split into two inner cylinders and two outer ones centered at ( k x , k y ) = ( ± Q x , 0 ) . In particular, the λ z term leads to a spiral spin texture on each Fermi surface that rotates along the k z direction. For a generic spin-dependent interaction H I = V ( r 1 - r 2 ) ρ ( r 1 ) ρ ( r 2 ) + J ( r 1 - r 2 ) S ( r 1 ) · S ( r 2 ) , where ρ ( r ) and S ( r ) are the local electron density and spin operators. The projection onto the spin texture will naturally yield an interaction as shown in Eq. (1) , as we will show later. We also want to mention a different way to understand the linked nodal lines induced by SOC as follows. Generically, the TRI pairing amplitude of the two bands split by SOC is a matrix in the natural electron spin s z = ± 1 / 2 basis as follows [27] : Δ s s ′ ( k ) = { [ ψ ( k ) + d ( k ) · σ ] i σ y } s s ′ , (3) where ψ ( k ) = ψ ( - k ) gives a singlet pairing while d ( k ) = - d ( - k ) corresponds to a triplet pairing, both of which are real functions of k . For a system with a SOC given by H soc = g ( k ) · σ , it is shown [28] that the most favorable pairing amplitude satisfies d ( k ) = ξ ( k ) g ( k ) , where ξ ( k ) is a scalar function. This yields a pairing amplitude Δ ( k ) = ψ ( k ) ∓ ξ ( k ) | g ( k ) | on the two outer ( - sign) and inner ( + sign) cylindrical Fermi surfaces. In the simplest case when both ψ ( k ) = ψ and ξ ( k ) = ξ are constants, nodal lines will occur at the intersections between the outer cylindrical Fermi surfaces and the constant | g ( k ) | surfaces defined by Δ ( k ) = ψ - ξ | g ( k ) | = 0 . Figure 2(a) shows the intersection nodes A , B and A ′ , B ′ in the k z = 0 plane, where the white circles are the outer cylindrical Fermi surfaces, and the yellow loops are constant | g ( k ) | = ψ / ξ > 0 surfaces, which are centered at Λ and Λ ′ where | g ( k ) | = 0 . The light (dark) color represents the regions where | g ( k ) | is large (small), and the arrows show the spin textures in the BZ. As k z increases from 0 to 2 π , the Λ point moves along a spiral trajectory ( Q x + ( λ z / λ ) cos k z , - ( λ z / λ ) sin k z , k z ), and similarly for Λ ′ , so the gapless nodes A , B (and A ′ , B ′ ) will undergo a 2 π rotation with respect to k z , yielding a double helix nodal-line structure. We note that in order to have intersection nodes, the value of ψ / ξ must be within a certain range, which is determined by interactions. Similarly, nodal lines may also occur on the inner Fermi surfaces at intersections where | g ( k ) | = - ψ / ξ (if ψ / ξ < 0 ), which also form double helices. 2 10.1103/PhysRevLett.119.147001.f2 FIG. 2. The arrows show the spin textures of the lower electron band in the k z = 0 plane for λ = - 0.02 t , λ z = 0.005 t , and the brightness is proportional to the SOC strength | g ( k ) | (brighter color for larger | g ( k ) | ). In particular, | g ( k ) | = 0 at Λ and Λ ′ points. The nodal lines occur at A , B and A ′ , B ′ points which are intersections between the Fermi surfaces as given by the white circles and the constant | g ( k ) | = ψ / ξ contours (yellow circles). Now we rewrite the above model in a 3D lattice, and demonstrate the above interaction and SOC indeed give rise to double-helix linked nodal lines. We assume the following single-electron Hamiltonian with SOC: H 0 ( k ) = t ′ cos 2 k x - t cos k y + λ 1 σ x sin k y + λ 2 σ y sin 2 k x + λ 3 σ x sin k z + λ 4 σ y sin k x cos k z - μ , (4) where t and t ′ are positive, and λ i ( 1 ≤ i ≤ 4 ) are SOC parameters which are TRI but inversion asymmetric. When the SOC is zero, the electron kinetic energy has its minima at ( k x , k y ) = ( ± π / 2 , 0 ) . For chemical potential μ satisfying - t ′ - t < μ < - | t - t ′ | , the Fermi surfaces are two spin-degenerate cylindrical tori centered at the minima. When the SOC is turned on, the Fermi surfaces split into two inner tori and two outer tori, and acquire spin textures. For convenience, we fix λ 1 = 2 λ 2 = λ and λ 3 = λ 4 = λ z . The SOC reduces to the form of Eq. (2) in the vicinity of ( k x , k y ) = ( ± π / 2 , 0 ) . In principle, the Hamiltonian could contain other hopping or SOC terms, but we will keep them zero since they do not qualitatively change the physics [29] . In the following discussion, we will fix the single-particle parameters at t ′ = 0.25 t , λ = - 0.2 t , λ z = 0.4 t . For simplicity, we will also fix the chemical potential at μ = - 1.6 t slightly above the band minimum, so that the two inner torus Fermi surfaces shrink to zero [29] , with only the two outer torus Fermi surfaces left. We then add an electron-electron interaction to the system as follows [30] : H int = 1 N ∑ q V ( q ) ρ q ρ - q + 1 N ∑ q J ( q ) S q · S - q , (5) where ρ q = ∑ k s c k + q , s † c k , s and S q = 1 2 ∑ k s s ′ c k + q , s † σ s s ′ c k , s ′ are the electron density and spin operators at momentum q . Such an interaction may generically arise from the phonon exchange and the electron itinerant magnetism. Explicitly, we assume the interaction potentials take the form V ( q ) = V 0 + V x cos 2 k x + V y cos k y and J ( q ) = J x cos 2 k x + J y cos k y , where V 0 , V x , V y , J x , and J y are constants. With the spin textures known, one can readily project the interaction onto the two cylindrical Fermi surfaces. Using a k · p expansion, one can show the Cooper channel interaction potential V k k ′ for k and k ′ on the same Fermi surface is given by [29] V k k ′ = η 0 - ( η 1 k x ˜ k x ′ ˜ + η 2 k y k y ′ ) cos [ ϕ ( k ) - ϕ ( k ′ ) ] - η 3 ( k x ˜ 2 + k x ′ ˜ 2 ) - η 4 ( k y 2 + k y ′ 2 ) , (6) where we have kept terms up to the second order in k x ˜ and k y . Here ϕ ( k ) is the angle of the spin direction at k in the k x - k y plane, η 1 = - ( 4 V x + J x ) , η 2 = - ( V y + J y / 4 ) , η 3 = 2 V x - 3 J x / 2 , η 4 = V y / 2 - 3 J y / 8 , η 0 = V 0 + η 3 / 2 + 2 η 4 , and we have k x ˜ = k x ∓ π / 2 for momentum near ( k x , k y ) = ( ± π / 2 , 0 ) , respectively. Compared with Eq. (1) , the above interaction contains a few other less important terms and has the spin angle ϕ ( k ) in place of k z . However, since the spin angle ϕ ( k ) increases (decreases) by 2 π as k z goes from - π to π on the two Fermi surfaces, the above interaction still satisfies the condition for double helix nodal lines. Based on this interaction near Fermi surfaces, we solve numerically the linearized gap equation that determines the mean-field superconductivity critical temperature T c [30] : - χ Ψ ( k ) = 1 2 N ε c ∑ k ′ V k k ′ Ψ ( k ′ ) , (7) where ε c is the interaction cutoff energy (e.g., Debye energy), k is summed within the energy shell [ - ε c , ε c ] near the Fermi surface, while Ψ ( k ) ∝ Δ ( k ) is an eigenvector of V k k ′ , and λ is the eigenvalue. For χ > 0 , the critical temperature is given by k B T c = 1.14 ε c e - 1 / χ . For χ ≤ 0 , the eigenvector Ψ ( k ) is not a pairing instability. The most favorable pairing function Δ ( k ) is proportional to the eigenvector Ψ ( k ) with the largest positive eigenvalue χ . Figure 3(a) shows a phase diagram with respect to J x = J y = J and V 0 , where we have fixed V x = V y = V < 0 . Different phases are distinguished by the topology of their nodal lines, and are labeled using different Greek letters. Both the α phase and the α ′ phase are double-helix nodal-line phases with different double helix helicities. The typical nodal-line shapes of the α and α ′ phases are shown in Figs. 3(b) and 3(c) , respectively, where θ = arg ( k x ˜ + i k y ) is the poloidal angle of the torus Fermi surface. Figure 3(e) shows the double-helix nodal lines of the α phase in the 3D BZ. We note that the physical picture in Fig. 2 only predicts the double-helix helicity of phase α , which is valid for small λ z / λ [29] . In the case we calculated in Fig. 3 where λ z / λ is large, both phases α and α ′ arise, which is because the projected interaction in Eq. (6) in this case does not give a double-helix helicity preference. The β phase has two unlinked nodal loops as shown in Fig. 3(d) , while the γ phase is fully gapped without any nodal lines. The phase diagram shows that ferromagnetic spin interactions J < 0 tend to favor double-helix nodal lines, which makes η 1 and η 2 positive as required in our argument. We note that ferromagnetic electron interactions are quite common for metals. 3 10.1103/PhysRevLett.119.147001.f3 FIG. 3. (a) Phase diagram for fixed V < 0 , where the horizontal and vertical axes are J and V 0 , respectively. Both α and α ′ phases are double-helix linked nodal line phases, except that their helicities are opposite. The β phase contains two unlinked nodal lines on each Fermi surface. The γ phase is the conventional fully gapped phase. Panels (b)–(d) show the nodal-line configuration on the Fermi surface at k x = π / 2 for points A , B , and C in the phase diagram, respectively, where θ = arg ( k x ˜ + i k y ) is the poloidal angle of the torus Fermi surface. (e) The 3D plot of the spin texture (arrows) and nodal lines (blue and red lines) on the Fermi surfaces at point A of the phase diagram. We have seen that the realization of linked nodal lines requires torus or higher genus Fermi surfaces, and strongly varying spin textures along the toroidal direction of the Fermi surfaces. These conditions put a limitation on the crystalline symmetry of candidate materials. In general, a lower crystalline symmetry is preferred. In particular, in the double helix nodal line configuration in Fig. 1(a) , the only allowed point-group symmetry (up to a translation) is either a twofold rotation C 2 x about the x axis or a mirror reflection M x from x to - x . In other configurations as shown Figs. 1(b)–1(d) , a few other symmetry operations such as the threefold rotation C 3 z are allowed. For instance, the configuration of Fig. 1(c) is allowed for materials with a hexagonal 3 R structure, which is common in transition metal dichalcogenides [31] . We therefore suggest to search for (double-helix) linked nodal-line superconductors in layered metallic materials with strong SOCs and low crystalline symmetries, such as lithium-inserted metal oxide, transition metal dichalcogenides, and transition metal halides, etc. [32] , where torus Fermi surfaces and strongly varying spin textures are more likely to occur. The detection of linked nodal lines is also essential in experiments. A few techniques such as corner junction [2,33] , angular-resolved thermal transport measurement [34,35] , and angular-resolved photoemission spectroscopy (ARPES) [6] have been used to reveal the nodal structure of superconductors, which will, however, be more complicated for linked nodal lines. Instead, we suggest a possibly easier way to reveal linked nodal lines through probing the surface states on the surface cuts of different directions using ARPES. As we mentioned at the beginning, nodal line superconductors exhibit topologically protected zero energy Majorana flat bands, which are bounded by the projection of nodal lines on the surface [17–19] . If two nodal lines are linked, their projections will necessarily cross each other on any surface cuts. Therefore, the corresponding surface Majorana flat bands always kiss each other as shown in Fig. 4 , no matter which surface cut one takes. 4 10.1103/PhysRevLett.119.147001.f4 FIG. 4. (a) Sketch of a typical example of double-helix nodal lines in the BZ. (b)–(d) Illustration of the zero-energy surface Majorana flat bands (colored in green) on surface cuts along the Γ - Z , Γ - X , and Γ - M directions, which are bounded by the projection of nodal lines. In conclusion, we have demonstrated the possibility of realizing linked nodal lines in noncentrosymmetric superconductors with torus or higher genus Fermi surfaces and strongly k -dependent spin textures, and studied an explicit lattice model that realizes a double-helix nodal-line superconductor. These results may serve as a preliminary guidance on searching for and detecting linked nodal-line superconductors in nature. We are grateful to Peizhe Tang for helpful discussions. This work is supported by the NSF Grant No. DMR-1305677. [1] 1 C.-R. Hu , Phys. Rev. Lett. 72 , 1526 ( 1994 ). PRLTAO 0031-9007 10.1103/PhysRevLett.72.1526 [2] 2 D. A. Wollman , D. J. Van Harlingen , W. C. Lee , D. M. Ginsberg , and A. J. Leggett , Phys. Rev. Lett. 71 , 2134 ( 1993 ). PRLTAO 0031-9007 10.1103/PhysRevLett.71.2134 [3] 3 D. A. Wollman , D. J. Van Harlingen , J. Giapintzakis , and D. M. Ginsberg , Phys. Rev. Lett. 74 , 797 ( 1995 ). PRLTAO 0031-9007 10.1103/PhysRevLett.74.797 [4] 4 J. R. Kirtley , C. C. Tsuei , J. Z. Sun , C. C. Chi , Lock See Yu-Jahnes , A. Gupta , M. Rupp , and M. B. Ketchen , Nature (London) 373 , 225 ( 1995 ). NATUAS 0028-0836 10.1038/373225a0 [5] 5 K. Okazaki , Y. Ota , Y. Kotani , W. Malaeb , Y. Ishida , T. Shimojima , T. Kiss , S. Watanabe , C.-T. Chen , K. Kihou , Science 337 , 1314 ( 2012 ). SCIEAS 0036-8075 10.1126/science.1222793 [6] 6 Y. Zhang , Z. Ye , Q. Ge , F. Chen , J. Jiang , M. Xu , B. Xie , and D. Feng , Nat. Phys. 8 , 371 ( 2012 ). NPAHAX 1745-2473 10.1038/nphys2248 [7] 7 E. Bauer , G. Hilscher , H. Michor , C. Paul , E. W. Scheidt , A. Gribanov , Y. Seropegin , H. Noël , M. Sigrist , and P. Rogl , Phys. Rev. Lett. 92 , 027003 ( 2004 ). PRLTAO 0031-9007 10.1103/PhysRevLett.92.027003 [8] 8 S. Yip , Annu. Rev. Condens. Matter Phys. 5 , 15 ( 2014 ). ARCMCX 1947-5454 10.1146/annurev-conmatphys-031113-133912 [9] 9 B. Lian , C. Vafa , F. Vafa , and S.-C. Zhang , Phys. Rev. B 95 , 094512 ( 2017 ). PRBMDO 2469-9950 10.1103/PhysRevB.95.094512 [10] 10 W. Chen , H.-Z. Lu , and J.-M. Hou , Phys. Rev. B 96 , 041102 ( 2017 ). PRBMDO 2469-9950 10.1103/PhysRevB.96.041102 [11] 11 Z. Yan , R. Bi , H. Shen , L. Lu , S.-C. Zhang , and Z. Wang , Phys. Rev. B 96 , 041103 ( 2017 ). PRBMDO 2469-9950 10.1103/PhysRevB.96.041103 [12] 12 M. Ezawa , Phys. Rev. B 96 , 041202 ( 2017 ). PRBMDO 2469-9950 10.1103/PhysRevB.96.041202 [13] 13 Z. Wang , X.-L. Qi , and S.-C. Zhang , Phys. Rev. B 84 , 014527 ( 2011 ). PRBMDO 1098-0121 10.1103/PhysRevB.84.014527 [14] 14 S. Ryu , J. E. Moore , and A. W. W. Ludwig , Phys. Rev. B 85 , 045104 ( 2012 ). PRBMDO 1098-0121 10.1103/PhysRevB.85.045104 [15] 15 A. M. Polyakov , Mod. Phys. Lett. A 03 , 325 ( 1988 ). MPLAEQ 0217-7323 10.1142/S0217732388000398 [16] 16 E. Witten , Commun. Math. Phys. 121 , 351 ( 1989 ). CMPHAY 0010-3616 10.1007/BF01217730 [17] 17 A. P. Schnyder and S. Ryu , Phys. Rev. B 84 , 060504 ( 2011 ). PRBMDO 1098-0121 10.1103/PhysRevB.84.060504 [18] 18 A. P. Schnyder , P. M. R. Brydon , and C. Timm , Phys. Rev. B 85 , 024522 ( 2012 ). PRBMDO 1098-0121 10.1103/PhysRevB.85.024522 [19] 19 A. P. Schnyder and P. M. R. Brydon , J. Phys. Condens. Matter 27 , 243201 ( 2015 ). JCOMEL 0953-8984 10.1088/0953-8984/27/24/243201 [20] 20 M. Sato , Y. Tanaka , K. Yada , and T. Yokoyama , Phys. Rev. B 83 , 224511 ( 2011 ). PRBMDO 1098-0121 10.1103/PhysRevB.83.224511 [21] 21 Y. Tanaka , M. Sato , and N. Nagaosa , J. Phys. Soc. Jpn. 81 , 011013 ( 2012 ). JUPSAU 0031-9015 10.1143/JPSJ.81.011013 [22] 22 J. D. Watson and F. H. Crick , Nature (London) 171 , 737 ( 1953 ). NATUAS 0028-0836 10.1038/171737a0 [23] 23 J. Watson , The Double Helix ( Hachette , UK, 2012 ). [24] 24 P. W. Anderson , Phys. Rev. B 30 , 4000 ( 1984 ). PRBMDO 0163-1829 10.1103/PhysRevB.30.4000 [25] 25 X.-L. Qi , T. L. Hughes , S. Raghu , and S.-C. Zhang , Phys. Rev. Lett. 102 , 187001 ( 2009 ). PRLTAO 0031-9007 10.1103/PhysRevLett.102.187001 [26] 26 C. F. Gauss , Werke , ( Königliche Gesellschaft der Wissenschaften , Göttingen, 1833 ), Vol. 5 , p. 605 . [27] 27 M. Sigrist and K. Ueda , Rev. Mod. Phys. 63 , 239 ( 1991 ). RMPHAT 0034-6861 10.1103/RevModPhys.63.239 [28] 28 P. A. Frigeri , D. F. Agterberg , A. Koga , and M. Sigrist , Phys. Rev. Lett. 92 , 097001 ( 2004 ). PRLTAO 0031-9007 10.1103/PhysRevLett.92.097001 [29] 29 See Supplemental Material at http://link.aps.org/supplemental/10.1103/PhysRevLett.119.147001 for technical details on (i) the Fermi surface of single particle Hamiltonian, (ii) the projected interaction on the Fermi surface, (iii) the phase diagram for small λ z / λ , (iv) the double helix-nodal line phase at zero temperature, (v) and the stability of the double helix nodal-line phase under symmetry allowed perturbations. [30] 30 M. Sigrist , AIP Conf. Proc. 789 , 165 ( 2005 ). APCPCS 0094-243X 10.1063/1.2080350 [31] 31 M. Chhowalla , H. S. Shin , G. Eda , L.-J. Li , K. P. Loh , and H. Zhang , Nat. Chem. 5 , 263 ( 2013 ). NCAHBB 1755-4330 10.1038/nchem.1589 [32] 32 P. Miró , M. Audiffred , and T. Heine , Chem. Soc. Rev. 43 , 6537 ( 2014 ). CSRVBR 0306-0012 10.1039/C4CS00102H [33] 33 D. Van Harlingen , Rev. Mod. Phys. 67 , 515 ( 1995 ). RMPHAT 0034-6861 10.1103/RevModPhys.67.515 [34] 34 M. J. Graf , S. K. Yip , J. A. Sauls , and D. Rainer , Phys. Rev. B 53 , 15147 ( 1996 ). PRBMDO 0163-1829 10.1103/PhysRevB.53.15147 [35] 35 Y. Matsuda , K. Izawa , and I. Vekhter , J. Phys. Condens. Matter 18 , R705 ( 2006 ). JCOMEL 0953-8984 10.1088/0953-8984/18/44/R01 Publisher Copyright: © 2017 American Physical Society.

PY - 2017/10/2

Y1 - 2017/10/2

N2 - Time-reversal invariant superconductors in three dimensions may contain nodal lines in the Brillouin zone, which behave as Wilson loops of 3D momentum-space Chern-Simons theory of the Berry connection. Here we study the conditions of realizing linked nodal lines (Wilson loops), which yield a topological contribution to the thermal magnetoelectric coefficient that is given by the Chern-Simons action. We find the essential conditions are the existence of torus or higher genus Fermi surfaces and spiral spin textures. We construct such a model with two torus Fermi surfaces, where a generic spin-dependent interaction leads to double-helix-like linked nodal lines as the superconductivity is developed.

AB - Time-reversal invariant superconductors in three dimensions may contain nodal lines in the Brillouin zone, which behave as Wilson loops of 3D momentum-space Chern-Simons theory of the Berry connection. Here we study the conditions of realizing linked nodal lines (Wilson loops), which yield a topological contribution to the thermal magnetoelectric coefficient that is given by the Chern-Simons action. We find the essential conditions are the existence of torus or higher genus Fermi surfaces and spiral spin textures. We construct such a model with two torus Fermi surfaces, where a generic spin-dependent interaction leads to double-helix-like linked nodal lines as the superconductivity is developed.

UR - http://www.scopus.com/inward/record.url?scp=85030775009&partnerID=8YFLogxK

UR - http://www.scopus.com/inward/citedby.url?scp=85030775009&partnerID=8YFLogxK

U2 - 10.1103/PhysRevLett.119.147001

DO - 10.1103/PhysRevLett.119.147001

M3 - Article

C2 - 29053291

AN - SCOPUS:85030775009

VL - 119

JO - Physical Review Letters

JF - Physical Review Letters

SN - 0031-9007

IS - 14

M1 - 147001

ER -