Abstract
Carbon, the basic building block of our universe, enjoys a vast number of allotropic structures. Owing to its bonding characteristic, most carbon allotropes possess the motif of hexagonal rings. Here, with firstprinciples calculations, we discover a new metastable threedimensional carbon allotrope entirely composed of pentagon rings. The unique structure of this Pentagon Carbon leads to extraordinary electronic properties, making it a cornucopia of emergent topological fermions. Under lattice strain, Pentagon Carbon exhibits topological phase transitions, generating a series of novel quasiparticles, from isospin1 triplet fermions to triply degenerate fermions and further to Hopflink Weylloop fermions. Its Landau level spectrum also exhibits distinct features, including a huge number of almost degenerate chiral Landau bands, implying pronounced magnetotransport signals. Our work not only discovers a remarkable carbon allotrope with highly rare structural motifs, it also reveals a fascinating hierarchical particle genesis with novel topological fermions beyond the Dirac and Weyl paradigm.
Introduction
Most stable carbon allotropes, including the prominent members such as graphite, diamond, carbon nanotube^{1} and graphene^{2}, possess a motif of hexagonal rings due to the dominating sp^{2} and sp^{3} bonding character^{3}. In contrast, the motif of pentagonal rings, although can appear in molecules such as fullerene^{4}, is very rare in threedimensional (3D) allotropes. This is partly due to the unfavourable bonding angles that may easily cause structural instability^{5}, and also because the pentagonal motif does not readily fit into the 3D space group symmetry^{6}. It seems unlikely to have a stable 3D carbon allotrope dominated by pentagonal carbon rings.
Meanwhile, the research on topological metals and semimetals (TMs) has been attracting tremendous interest^{7,8,9,10,11,12,13,14}. In these materials, topologically protected quasiparticles emerge at protected bandcrossing points around Fermi Level, giving rise to condensed matter realizations of many peculiar fermions with a variety of distinct electronic properties. For example, in Dirac and Weyl semimetals, the quasiparticles near the protected linear bandcrossing points are direct analogues of the Dirac and Weyl fermions in relativistic quantum field theory, providing unique opportunities to study interesting highenergy physics phenomena such as chiral anomaly and gravitational anomaly in a tabletop experiment^{15,16,17,18}. The emergent topological fermions can be classified by the degeneracy of the bandcrossing point, which dictates the number of internal degrees of freedom of the fermion. Dirac and Weyl fermions are associated with crossing points with fourfold and twofold degeneracies^{19,20}. Importantly, the breaking of Lorentz symmetry at lattice scale makes it possible to have TMs that can host new types of fermions with different degeneracies beyond the Dirac and Weyl fermions^{21}, ^{22}, ^{23}. These new fermions are now actively searched for, and if realized, they are believed to host a wealth of exotic physical properties unprecedented in highenergy physics.
The search for TMs has been focused on compounds involving heavy elements^{7,24,25}, hoping that the strong spin–orbit coupling could help to achieve a nontrivial band structure. On the other hand, light elements such as carbon may offer a distinct alternative. For example, graphene is wellknown with twodimensional (2D) Dirac fermions^{26}. With negligible spin–orbit coupling, the real spin in carbon materials can be considered as a dumb degree of freedom^{27}. Then the fundamental time reversal operation () here satisfies , contrasting with for the spinful case. Thus in terms of topological classifications, the nontrivial phases in carbon would be fundamentally distinct from those in spin–orbitcoupled systems. Indeed, previous studies have identified a few TM carbon allotropes with Weyl points^{28,29}, nodal loops^{27,29,30,31,32} and even Weyl surfaces^{28}. Motivated by these observations, one may naturally wonder: is it possible to also realize new types of topological fermions in carbon allotropes?
In this work, based on firstprinciples calculations, we propose a new 3D carbon allotrope, named as 3D Pentagon Carbon (3DC5), which is entirely composed of pentagonal carbon rings. With nicely interlaced structures, the structure shows good stability comparable to other metastable carbon allotropes. We characterize its phononic, mechanical and electronic properties. At the equilibrium state, Pentagon Carbon is a narrowgap semiconductor. A semiconductor–metal quantum phase transition can be driven by an applied strain. Remarkably, at the critical transition point, three bands cross at a single Fermi point in the energymomentum space, making the emergent lowenergy fermions a novel type of isospin1 triplet fermions. Beyond the transition, the single Fermi point splits into two triply degenerate bandcrossing points along the fourfold screwrotational axis. The material is turned into a novel TM possessing another type of triply degenerate fermions. When further breaking the screwrotational symmetry, the triply degenerate fermion points will transform into two interconnected Hopflink Weyl loops protected by the remaining mirror symmetry. We show that, for each case, the Landau level (LL) spectrum exhibits distinct features tied to the topological fermions, suggesting pronounced anomalies in magnetotransport experiment. In addition, we discuss a possible reaction pathway for the experimental synthesis of Pentagon Carbon.
Results
Lattice structure and stability
The structure of 3D Pentagon Carbon is shown in Fig. 1a , which can be viewed as formed by interlinking two orthogonal arrays of pentagonring nanoribbons and stacking them along the zdirection (Fig. 1b). After linking, the two nanoribbons share one (greencolored) atom. Hence in the Pentagon Carbon lattice, there are two kinds of carbon atoms, that is, the sp^{2}hybridized (red and bluecolored) atoms forming the backbones of the pentagonring nanoribbons and the sp^{3}hybridized (greencolored) atoms forming the linkage between ribbons.
The structure has the nonsymmorphic space group symmetry (No. 141, I4_{1}/amd). Here an important symmetry element is the screw rotation , which is a fourfold rotation along z followed by a factional lattice translation of , where c is the lattice parameter in the z direction. The detailed structural properties are presented in Table 1 and are compared with several other (meta) stable 3D carbon allotropes. One observes that the cohesive energy of Pentagon Carbon, although slightly higher than graphite and diamond, is less than T6 (ref. 33) and BccC8 (ref. 34) and is comparable with Carbon Kagome Lattice (CKL)^{35,36} structure. Due to its porous structure, the mass density of Pentagon Carbon is low (∼2.18 g cm^{−3}) comparable with that of graphite. This is also correlated with its relatively low bulk modulus ∼257 GPa compared with other allotropes (except for graphite), suggesting that external strain can be more easily applied. The phonon spectrum of Pentagon Carbon is also investigated, which shows no soft mode, confirming its dynamical stability (more analysis of lattice structure and stability can be found in Supplementary Fig. 1 and Note 1).
Electronic structure and quantum phase transition
Remarkably, Pentagon Carbon is also a material hosting a series of novel topological fermions beyond the usual Dirac and Weyl fermions. The band structure in Fig. 2a shows that, in equilibrium state, it is a narrowgap semiconductor with a small energy gap ∼21.4 meV. The electronic structure shows strong anisotropy between inplane (xy) and outofplane (z) directions in accordance with the crystal structural anisotropy. Focusing on the Γ point, there are two valence bands (heavyhole and lighthole) and a single conduction band at low energy, with the conduction band and the lighthole valence band almost crossing linearly. Note that the degeneracy of the two valence bands at Γ is dictated by symmetry: the two states belong to a 2D irreducible representation E_{g} of the D_{4h} group at Γ. In comparison, the conduction band belongs to the onedimensional (1D) A_{1u} representation. Another salient feature is that the two valence bands are degenerate along the Γ–Z path (k_{z}axis). This is because that there is remaining C_{4v} little group symmetry along this screw axis, such that the 2D representation does not split according to the compatibility relation. From the analysis of wavefunction and projected density of states (PDOS), we find that the lowenergy states are mainly from the π orbitals of the sp^{2} atoms (Fig. 2f, Supplementary Fig. 2).
Since the semiconducting gap is small, a slight perturbation may close the gap and drive a semiconductortometal phase transition (a tightbinding model analysis is given in Supplementary Figs 3,4 and Note 2). In Fig. 2b–d, we show band structures for three applied uniaxial strains ɛ=1, −0.1 and −1% along the z direction. One observes that indeed a semiconductor–metal phase transition is induced. A tensile strain drives the system to a semiconductor with wider gap, whereas a compressive strain drives the system towards a metal. Of particular interest is the change of band ordering at the Γ point. The A_{1u} singlet state and the E_{g} doublet switch their positions in energy across the transition. Due to their different symmetry character, A_{1u} and E_{g} states cannot hybridize in the transition. Hence at the critical strain, we must have the three bands crossing at a single point, where the conduction and the lighthole bands have linear dispersion in the k_{x}–k_{y} plane; and all three bands have quadratic dispersion along the screw axis. The 3D band structures in Fig. 2i,j clearly show the anisotropic feature around the triplet point.
Passing the critical point, the band ordering is inverted at Γ. However, the corresponding states at Z on the Brillouin zone boundary still have the original ordering. This band topology means that the two bands must cross each other between Γ and Z. Further, because the two bands still belong to different representations along the screw axis, they must cross in a linear manner with two triply degenerate bandcrossing points (one on each side of Γ), as confirmed in Fig. 2d. Therefore, the metallic phase represents a novel TM phase with a pair of triply degenerate bandcrossing points near the Fermi level. In such sense, the quantum phase transition may also be regarded as a topological phase transition from a trivial semiconductor phase to a TM phase.
We can define a Z_{2} invariant to characterize this TM phase and the phase transition. Let Δ and Δ_{z} be the values of the energy difference between A band and E band at Γ point and at Z point, respectively. Then a Z_{2} invariant can be defined as . corresponds to the trivial case where a bandcrossing point does not need to occur, while is the topologically nontrivial case where a triply degenerate crossing point must exist between Γ and Z. The topological phase transition from a trivial semiconductor phase to TM phase (as shown in Fig. 2) is thus characterized by changing from +1 to −1. The topological character is manifest in the sense that as long as the Z_{2} invariant is well defined (that is, symmetry is preserved) and does not change, the existence of the triply degenerate crossing point and the linear band dispersion along k_{z} near the point are guaranteed and insensitive to system parameters and perturbations.
Emergent fermions and k·p model
Nontrivial bandcrossing points are fascinating objects because the fermionic quasiparticles around these points necessarily have a multicomponent structure, distinct from the usual Schrodinger fermions. The essential physics of these emergent fermions are characterized by the lowenergy effective k·p model expanded around the crossing point.
Around the Γ point, we can construct the k·p model based on the three basis states of A_{1u} and E_{g}. Constrained by the D_{4h} symmetry group and the time reversal symmetry for a spinless system (as spin–orbit coupling is negligible for carbon), one obtains the k·p model up to kquadratic order as
where the coefficients A, B_{1}, B_{2}, C, D_{1}, D_{2}, and Δ can be determined by fitting the density functional theory (DFT) result. At transition point, Δ=0, the three bands cross at a single point, as illustrated in Fig. 3a. Then we can further simplify the model by keeping only the klinear terms:
where , and
are three of the eight GellMann matrices corresponding to spin1 (ref. 37). This describes an isospin1 triplet fermion moving in the xy plane. The fermion is helical, with a welldefined helicity of ±1 and 0 corresponding to the eigenvalues of the helicity operator k·λ/k. The two branches with helicity ±1 are massless while the remaining one with helicity 0 has a flat dispersion, and these are constrained by the presence of an emergent ‘chiral symmetry’ operation with . The finite mass term for breaks this symmetry, generating a mass for both ±1 branches and gapping the spectrum.
Passing the critical point, the isospin1 triplet fermion point split into two triply degenerate points located at k_{z}=τK_{c}, as shown in Fig. 3b, where τ=± is an index labelling the two crossing points and (note that we must have Δ<0 and B_{1}>0 to reproduce the band structure). The emergent triply degenerate fermions around each crossing point are described by the linearized model obtained from equation (1) as
where the wave vector q is measured from the crossing point. One notes that in the direction perpendicular to the screw axis, that is, in the q_{x}–q_{y} plane, the dispersion is the same as that for the isospin1 triplet fermion in equation (2). One finds that the triply degenerate fermions basically inherit the structure of the triplet fermions but acquire one more degree of freedom, that is, the motion along the z direction. In the meantime, they lose the welldefined helicity.
The two kinds of fermionic quasiparticles, the isospin1 triplet fermions and the triply degenerate fermions, are new types of emergent fermions. Unlike the Dirac and Weyl fermions studied before, these new fermions do not have direct analogues in the relativistic quantum field theory. The isospin1 triplet fermion point is not topologically protected: it marks the critical point in the quantum phase transition. In contrast, the two triply degenerate fermion points are protected by the nontrivial band topology and the fourfold screw axis. These features are schematically illustrated in Fig. 3a,b.
When further breaking the screwrotational symmetry, the double degeneracy of the E band will be lifted; hence the triply degenerate fermion point will disappear. However, note that the original A and E bands have different eigenvalues under the mirror operations M_{xz} and M_{yz}. Hence crossings between each split E band and A band in the mirrorinvariant k_{x}–k_{z} and k_{y}–k_{z} planes will be protected if the respective mirror symmetry remains. For example, by an additional uniaxial strain along x direction or along diagonal directions in the x–y plane, we find that, interestingly, the resulting band crossings form two orthogonal concatenated Weyl loops, which has the topology of a Hopf link. As shown in Fig. 3c, for an additional tensile strain along the x direction, one Weyl loop is centred at the Γ point lying in the k_{x}–k_{z} plane, while the other loop is in the k_{y}–k_{z} plane and crosses the first Brillouin zone boundary. Around each point on the loop, the energy dispersion along two transverse directions is of the Weyllike linear type as shown in Fig. 3d. It needs to be emphasized that the band crossing forms the Weylloop fermion, not Weyl fermion, because the inversion symmetry is still preserved. It is particularly interesting that the two Weyl loops form an interconnected Hopflink pattern, and these two loops are protected by the M_{xz} and M_{yz} mirror symmetries, respectively. It should also be noted that there is no symmetry to pin these Weyl loops at a constant energy, and, indeed, the energy varies along each loop.
Landau level spectrum
Topological character of the band structure can manifest when subjecting to a magnetic field^{38,39,40}. For a 3D system, the electron motion in the plane perpendicular to the field is quantized into LLs. The dispersion along the field connects the levels to form dispersive Landau bands. For example, at each Weyl point, there is a gapless chiral Landau band, such that an additional parallel electric field will drive charge creation or depletion depending on the chirality. Since Weyl points appear in pairs of opposite chirality, the process leads to charge pumping between the Weyl points. This nonconservation of chiral charge at a single Weyl point is the wellknown chiral anomaly^{14,18,40}. Experimentally, it manifests as a negative magnetoresistance, which has recently been demonstrated in Weyl semimetals^{15,16}.
For Pentagon Carbon, considering a magnetic field along the screw axis such that the screw rotational symmetry is preserved. Focusing on the lowenergy physics around the Γ point where the quantum phase transition occurs, we find that the LL spectrum exhibits drastic difference across the transition. As illustrated in Fig. 4a, one observes that in the semiconductor phase, the LL spectrum shows a spectral gap, typical for a semiconducting state. Remarkably, in the TM phase, there appear two chiral Landau bands crossing the spectral gap and crossing the location of the original triply degenerate fermion points (Fig. 4b). This is like that of a Weyl point; however, there is a marked difference: the chiral band here is in fact with a huge number of Landau bands nearly degenerate onto a single curve^{21}. This behaviour is due to the small values of the inplane quadratic terms such as B_{2} and B_{3}. If one artificially increases these parameters, there will be a visible splitting between the almost degenerate Landau bands. Similar to chiral anomaly, a parallel Efield would pump charges from one triply degenerate point to the other. Due to the large number of the bands, it is expected to generate pronounced signals in magnetotransport experiment.
When further breaking the screwrotational symmetry, the triply degenerate fermion points disappear, giving rise to interconnected Hopflink Weyl loops. In the LL spectrum, we see that the main effect of the symmetry breaking is to split the chiral Landau bands, as indicated in Fig. 4c. These interesting LL features reflect the evolution of the bandcrossing points and will be useful for probing the quantum phase transition and the emergent topological fermions.
Discussion
Our work discovers a new metastable 3D carbon allotrope—the Pentagon Carbon, which exhibits a beautiful lattice structure entirely composed of pentagonal rings—a highly rare lattice motif for 3D crystals. Originating from this unique structure, there appear interesting quantum phase transitions and the associated novel emergent fermions. Remarkably, we reveal a fascinating transformation from isospin1 triplet fermion point to triply degenerate fermion point and finally to interconnected Hopflink Weyl loops.
Nontrivial bandcrossing point is also predicted in a few recent works. Particularly, Bradlyn et al.^{21} classified all possible degeneracy points at highsymmetry kpoints for the 230 space groups in spin–orbitcoupled systems, and tripledegenerate points have also been found in a few materials with strong spin–orbit coupling^{22,41,42}. The triply degenerate points here are distinct from those previous examples in the following aspects: first, due to the negligible SOC, Pentagon Carbon is essentially a spinless system, and, as we mentioned at the beginning, spinful and spinless systems belong to different symmetry/topological classes (For example, the time reversal operation has distinct properties between the two cases. And rotations for spinful systems will also operate on the spin degree of freedom, requiring a double group representation, distinct from spinless systems.); second, while the degeneracy points in ref. 21 are at highsymmetry points, here they are on symmetry lines (Γ–Z). Hence, without altering the symmetry, the latter is free to move along the symmetry line by applying a strain with observable physical consequences, whereas the former is pinned at the highsymmetry kpoints. A work by Heikkila and Volovik discussed possible triply degenerate points in Bernal graphite^{27}, where each point connects four Dirac bandcrossing lines with each line protected by a Z_{2} invariant N_{1}=±1. In contrast, the triply degenerate points in Pentagon Carbon are on a singleband degeneracy line along k_{z}axis (as in Fig. 3b); it is not a Dirac line because the dispersion is quadratic along the transverse directions, so the corresponding Z_{2} invariant, as defined in ref. 27, is trivial (N_{1}=0). The protection of the band degeneracy line and triply degenerate point here has a qualitatively different physical origin, which is originated from the fourfold screwrotational symmetry and band ordering topology, not present in Bernal graphite. We note that the different configurations of degeneracy lines in Bernal graphite and Pentagon Carbon precisely reflect their distinct symmetries: the arrangement of four Dirac lines with Z_{2} indices (−1,+1,+1,+1) observed in Bernal graphite is allowed by its threefold rotational symmetry, but it is not compatible with the fourfold screwrotation in Pentagon Carbon.
Here, we focus on the effect of uniaxial strain in driving the phase transition. Other types of lattice deformation can also produce a similar effect, as long as the fourfold screwrotational symmetry is preserved. For example, isotropic lattice strain or hydrostatic pressure can drive the phase transition with qualitatively similar features: the critical value is −1% for isotropic strain and 4.75 GPa for hydrostatic pressure. We also mention that like other carbon allotropes, Pentagon Carbon has excellent mechanical property. From firstprinciples calculation, it shows a linear elastic regime up to ±10% strain (Supplementary Fig. 5). Hence the straininduced phase transitions discussed here should be readily achievable.
To guide experiment, we simulate Xray diffraction peaks of Pentagon Carbon and contrast them with those of representative carbon allotropes (Supplementary Fig. 6). We also suggest a possible reaction route for the chemical synthesis. Molecules with pentagonal rings can be synthesized, for example, in cyclopentadiene with different substitutes. Starting from 1,4dibromocyclopentadiene, the cyclopentadiene building units can be linked into a 1D ribbon through Yamamoto polymerization. The 1D ribbons could be functionalized with bromides and boronic acids which are connected into the 3D framework through Suzuki coupling (the details are described in Supplementary Fig. 7). Each step in this process is either already achieved or have a high chance to be achieved because of the existence of similar reactions. Given its energetic and dynamic stabilities and in view of the rapid progress in experimental techniques which have realized a number of carbon structures in recent decade^{34,43}, we expect that Pentagon Carbon could also be realized in the near future.
Methods
Computational methods
We performed firstprinciples calculations within the DFT formalism as implemented in VASP code^{44,45}. The potential of the core electrons and the exchangecorrelation interaction between the valence electrons are described, respectively, by the projector augmented wave^{46} approach and the generalized gradient approximation in the Perdew–Burke–Ernzerhof^{47} implementation. The kinetic energy cutoff of 500 eV is employed. The atomic positions were optimized using the conjugate gradient method. The energy and force convergence criteria are set to be 10^{−5} eV and 10^{−2} eV Å^{−1}, respectively. The band structure and projected density of states (PDOS) were calculated using the primitive cell. The Brillouin zone was sampled with a 7 × 7 × 7 Monkhorst–Pack special kpoint grid for geometrical optimization. Phonon spectra are calculated using forceconstants method, and the dynamical matrices are computed using the finite differences method in a 2 × 2 × 2 supercell to eliminate errors in the low frequency modes (calculation with 3 × 3 × 3 supercell is also carried out for verification). The force constants and phonon spectra were obtained using the Phonopy package^{48}. Calculation with the Heyd–Scuseria–Ernzerhof (HSE06) hybrid functional^{49} is also performed to verify the band structure. The values of the band gap and the critical transition strain become larger compared with Perdew–Burke–Ernzerhof results (the HSE06 gap is about 471 meV and the critical strain is about −2%), but the qualitative features of the bands and phase transitions remain the same (Supplementary Fig. 8 and Note 3). The effect of van der Waals interaction is also tested and is found to be weak, for example, by including the van der Waals interaction, the cohesive energy is decreased from −8.79 to −8.89 eV and the lattice constants are decreased by about 0.2% (Supplementary Fig. 9).
Data availability
The data that support the findings of this study are available from the corresponding authors upon reasonable request.
Additional information
How to cite this article: Zhong, C. et al. Threedimensional Pentagon Carbon with a genesis of emergent fermions. Nat. Commun. 8, 15641 doi: 10.1038/ncomms15641 (2017).
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Acknowledgements
We thank the helpful discussions with ManFung Cheung, D.L. Deng, Shuai Yuan, Weiyu Xie and Damien J. West. This work was supported by the National Natural Science Foundation of China (Nos. 51376005 and 11474243). S.Z. acknowledges the support by US DOE under Grant No. DESC0002623. Z.M.Y. and S.A.Y. are supported by the Singapore MOE Academic Research Fund Tier 1 (SUTDT12015004) and Tier 2 (MOE2015T22144).
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Y.C. proposed the Pentagon Carbon. Y.C., S.A.Y. and S.Z. conceived the original ideas. C.Z., Y.C., Z.M.Y. and S.A.Y. conducted the calculations. Y.C. and S.A.Y. wrote the manuscript. All authors discussed the results and commented on the manuscript at all stages.
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Zhong, C., Chen, Y., Yu, ZM. et al. Threedimensional Pentagon Carbon with a genesis of emergent fermions. Nat Commun 8, 15641 (2017). https://doi.org/10.1038/ncomms15641
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