Abstract
We present a scanning tunneling microscopy (STM) and abinitio study of the anisotropic superconductivity of 2HNbSe_{2} in the chargedensitywave (CDW) phase. Differentialconductance spectra show a clear doublepeak structure, which is well reproduced by density functional theory simulations enabling full k and realspace resolution of the superconducting gap. The hollowcentered (HC) and chalcogencentered (CC) CDW patterns observed in the experiment are mapped onto separate van der Waals layers with different electronic properties. We identify the CC layer as the highgap region responsible for the main STM peak. Remarkably, this region belongs to the same Fermi surface sheet that is broken by the CDW gap opening. Simulations reveal a highly anisotropic distribution of the superconducting gap within single Fermi sheets, setting aside the proposed scenario of a twogap superconductivity. Our results point to a spatially localized competition between superconductivity and CDW involving the HC regions of the crystal.
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Introduction
Collective phenomena such as superconductivity and charge or spindensity modulations have been found to coexist in many materials, the interplay among these correlations being discussed in terms of their competition or mutual enhancement^{1,2,3,4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22}. The layered transitionmetal dichalcogenide 2HNbSe_{2} is a prominent example undergoing a transition into a chargeordered phase at T ≤33 K, and into the superconducting phase at T_{c} ≤ 7.2 K. Both orderings are driven by electronphonon coupling^{23,24,25,26,27,28,29,30,31} with a strong momentum dependence^{14,17,20,32}. The superconducting gap turns out to have an anisotropic distribution over the Fermi surface (FS), whereby NbSe_{2} has been interpreted either as a multigap or a highly anisotropic superconductor^{32,33,34,35,36}.
A clear understanding of the structure of the superconducting gap is indeed presently missing, and is one of the key unsolved questions about NbSe_{2}. Knowing whether superconducting anisotropy favors the stability of the superconducting state (like, e.g., in MgB_{2}) is interesting on itself. More importantly, accessing the momentumdependent structure of the superconducting gap in the CDW phase would allow one to unveil the link between superconducting condensation and CDW ordering in this material, resolving the longstanding debate on their competition.
In this paper, we present clear evidence of anisotropic superconductivity in NbSe_{2} by measuring the tunneling density of states (DOS) with unprecedented resolution combined with stateoftheart firstprinciples simulations of the superconducting state based on density functional theory for superconductors (SCDFT). We emphasize that, unlike conventional approaches to superconductivity^{37,38,39}, SCDFT does not rely on any empirical parameter, which allows us to elucidate the strength and distribution of the superconducting gap.
Results
STM spectroscopy
An atomically resolved constantcurrent STM image is shown in Fig. 1a. Besides the atomic corrugation of the terminating Se layer, the image reveals the modulation of the local DOS imposed by the CDW. As the CDW is incommensurate with the atomic lattice, (periodicity \(\vert{{{{{{\bf{q}}}}}}}_{\tiny{{{{\mbox{CDW}}}}}}\vert\lesssim 2\pi /\left(3a\right)\), where a is the inplane lattice constant), different local patterns appear across the surface. The area in the orange rectangle shows a triangular pattern as a result of the maximum of the CDW being centered on a hollow site (hollowcentered, HC pattern). This continuously transforms into the chalcogencentered (CC) pattern highlighted in the blue rectangle. Differentialconductance (dI/dV) spectra in different regions of the CDW are shown in Fig. 1b (for more spectra, see Supplementary Notes 4–6). All spectra exhibit a fully gapped region flanked by a broad peak distribution in the range 2.1 mV < Δ/e < 3.1 mV, with peculiar intensity variations, which can only be resolved by employing a superconducting tip.
Simulations  structural and normalstate properties
The CDW instability is captured by density functional theory (DFT) calculations in the undistorted cell (Ω_{1}), where it manifests itself in imaginary phonon frequencies occurring over a broad range of momenta centered at q_{CDW}^{40}. As discussed in^{23,28,29}, the CDW can not be viewed as a purely electronic Peierls’ instability driven by FS nesting, but is instead a structural phase transition assisted by the enhancement of the electronphonon coupling (EPC) at the characteristic wave vector. Additionally, the CDW transition temperature can be accurately reproduced in DFT calculations by including anharmonic effects in the lattice dynamics^{41}. In this paper we carry out a DFT study of the superconducting state in the CDW phase, providing a firstprinciples interpretation of the STM data.
We approximated the incommensurate CDW vector by \({{{{{{\bf{q}}}}}}}_{\tiny{{{{\mbox{CDW}}}}}}=\left(1/3,0,0\right)2\pi /a\), performing simulations within a superstructure unit cell (Ω_{3×3}) 3 × 3 × 1 times Ω_{1}. The CDW reconstruction was obtained by relaxing the lattice along the phonon instabilities until all the modes were stable in a 2 × 2 × 4 qgrid of the Ω_{3×3} cell.
We found that the CDW formation induces smallamplitude atomic displacements reducing the minimum Nb–Se distance by ~1.0%. Remarkably, the dynamically stable reconstruction that we predict has a unit cell with two crystallographically inequivalent NbSe_{2} layers, L_{1} and L_{2}. These are shown in Fig. 2c,d and correspond, respectively, to the HC and CC patterns observed in experiment. We note that the obtained structures closely resemble those suggested in refs. ^{17,18,42}. The calculated CDW stabilization energy is of 3.7 meV per formula unit.
The CDW distortion is expected to induce relatively small changes of the electronic structure. Figure 2a,b compares the computed band structure and electronic DOS in the presence of the CDW and in the undistorted system. The two DOSs differ mainly by a broad dip developing in the CDW state slightly above the Fermi level, such that the reduction in the DOS at the Fermi level (N_{F}) induced by the CDW is relatively small (about 10%). Due to the large size of the supercell used in the calculations (54 atoms), the BZ folding makes the band structure in the CDW state hard to interpret. We thus employed a technique of band unfolding^{43,44} from the supercell BZ to the larger BZ of the Ω_{1} unit cell. As one can see, the CDW and undistorted bands largely overlap. A closer inspection, however, reveals band gap openings at several points of the BZ path, especially along the MK line, as well as energy shifts at the K point throughout the entire valenceband width.
The CDW effect on the electronic structure can be seen more clearly by considering a horizontal cut through the BZ. Fig. 3a shows the CDW reconstruction of the FS at k_{z} = 0 obtained from the unfolding procedure. The unperturbed FS sheets (blue curves) are included for direct comparison. A doublewalled cylindrical sheet of Nb 4d bands and a pocket of Se 4p character are centered at the Γ point. A second pair of Nb 4dderived FS cylinders is located at the K point. This last double sheet appears to be significantly broader and blurred, indicating a stronger effect of the CDW distortion. Missing segments of the FS crossing the MK line, signal the openings of the CDW gap, which occur in excellent agreement with the ARPES measurements of refs. ^{32,45}.
As already mentioned, the complexity of the CDW state is increased by the fact that the two structural layers undergo different reconstructions. To account for this aspect, we considered projections of the FS quasiparticle states onto the layers. Selected cuts of the unfolded projected FS are shown in Fig. 4. Most of the states (displayed in white) are found to span the entire crystal, yet a significant fraction is strongly localized on one layer. L_{1} states are highlighted in red on the left panel of the figure, while L_{2} states are shown in blue on the right. We observe significant differences: (i) On the k_{z} = 0 plane, the FS of L_{2} develops ring structures, unlike L_{1}. (ii) At \({{{{{{\bf{k}}}}}}}_{z}\simeq \frac{2}{3}\frac{\pi }{c}\) the inner Kcentered sheet is mainly composed by L_{2} states, whereas it has a stronger L_{1} character on the ΓKM plane. (iii) By projecting the Fermipocket resolved DOS onto the layers,
where \({P}_{n{{{{{\bf{k}}}}}}}^{i}\) is a projection operator with i = L_{1}, L_{2}, and D refers to Γ or Kcentered sheets, we found that, remarkably, \({N}_{{{{{{\rm{F}}}}}}}^{{{{{{{\rm{L}}}}}}}_{1}{{{{{\boldsymbol{\Gamma }}}}}}}\) and \({N}_{{{{{{\rm{F}}}}}}}^{{{{{{{\rm{L}}}}}}}_{1}{{{{{\bf{K}}}}}}}\) are equally affected by the CDW (being reduced by 20%), whereas the DOS of L_{2} stays almost constant. The calculated values of \({N}_{{{{{{\rm{F}}}}}}}^{iD}\) are listed in Table 1.
The CDW modulation can strongly affect the lattice dynamics and, in turn, influence phonondriven superconductivity in complex ways. In principle, the CDW can coexist with and even enhance superconductivity. This latter scenario, in particular, has been put forth by recent experimental findings^{2,3,4,5,6,7,11,14,15,16,19,21,22,32}. As a first step to clarify the CDW effect on the superconducting properties of NbSe_{2}, we simulated the lattice dynamics in the CDW phase. We point out that this is a computationally demanding task because of the large size of the crystallographic unit cell and the accuracy required in simulating the small CDW distortion.
We found that the phonon DOSs in the CDW and undistorted structure have a very similar shape. The unstable phonon mode, appearing with imaginary frequency in the latter, has, in fact, low spectral weight. Nevertheless, the CDW transition significantly alters the EPC: since the EPC strength, \({\left{g}_{n{{{{{\bf{k}}}}}}n^{\prime} {{{{{\bf{k}}}}}}^{\prime} }^{\nu }\right}^{2}\), is inversely proportional to the phonon frequency^{37,46,47}, a dynamical instability of the lattice shows up in a divergence of the coupling. The calculated α^{2}F(ω) for the dynamically stable 3 × 3 × 1 CDW structure (shown in Supplementary Note 1) gives a total EPC of λ = 1.4, placing NbSe_{2} in the strongcoupling regime.
To assess the momentum anisotropy of the EPC, we calculated the kresolved EPC parameters
The values obtained for the unfolded k_{z} = 0 plane of the BZ are presented in Fig. 3b, where one can observe a complex pattern of hot spots (light) and weakcoupling (dark) regions. For a quantitative analysis, we examined the EPC contributions to Γ and Kcentered sheets arising from the two structural layers,
and the corresponding DOSindependent parameters, \({V}^{iD}={\lambda }^{iD}/{N}_{{{{{{\rm{F}}}}}}}^{iD}\). The computed values of λ^{iD} and V^{iD} are collected in Table 1. Since V^{iD} varies from a minimum of 0.30 (\({V}^{{{{{{{\rm{L}}}}}}}_{1}{{{{{\boldsymbol{\Gamma }}}}}}}\)) to a maximum of 0.39 (\({V}^{{{{{{{\rm{L}}}}}}}_{2}{{{{{\bf{K}}}}}}}\)), we deduce that the layers contribute almost equally to the intrinsic coupling of the various FS pockets. λ^{iD} is then determined essentially by the value of the DOS at the Fermi level. We also note that the FS Kcylinder and the layer L_{2} can be identified as the regions with higher Fermi DOS and EPC in momentum and real space, respectively.
Simulation of the superconducting state
We simulated the superconducting state from first principles using SCDFT^{48,49,50} with the stateoftheart SPG functional^{51}. The implementation of the method allowed us to make fully anisotropic calculations of the superconducting gap in both reciprocal and real space^{52}. The kdependent SCDFT gap equation was solved on a mesh of random k points more densely distributed around the FS for higher accuracy (computational details are provided in Supplementary Note 2 and refs. ^{47,53}). The estimated T_{c} of 10.2 K, is to be compared with an experimental value \({T}_{{{{{{\rm{c}}}}}}}^{\exp }=\) 7.2 K. Given the usual accuracy of SCDFT calculations (within ~20% of T_{c}), this error is likely to be ascribed to (i) the neglect of anharmonic corrections to the lattice dynamics, that are enhanced close to the CDW transition^{41}, or (ii) limits on the precision in computing phonon properties and dielectric screening imposed by the large size of the CDW cell (see Supplementary Note 2 for an extended discussion). Nevertheless, our prediction is fairly accurate compared to that from conventional Eliashberg theory in the μ^{*} approximation^{39,54}. This, in fact, gives T_{c} ≃ 16 K under the usual assumption μ^{* }= 0.11, while an exceedingly high value of the Coulomb pseudopotential (μ^{*} = 0.28) is required to reproduce the experimental result. The improved SCDFT estimation of T_{c} comes from including Coulomb interactions fully ab initio, thus retaining the energy dependence of the screened electronelectron interaction matrix elements \(V\left({\varepsilon }_{n{{{{{\bf{k}}}}}}},{\varepsilon }_{n{{{{{\bf{k}}}}}}^{\prime} }\right)\). In fact, our simulations show that the electronic states at the Fermi level are poorly screened, that is \(\mu ={N}_{{{{{{\rm{F}}}}}}}V\left(0,0\right)\) is large. Moreover, because of a different orbital character, these states weakly interact with those far from the Fermi level, yielding a weak reduction of the Coulomb pseudopotential (high μ^{*})^{55}.
The computed superconducting state turns out to be extremely complex. Unlike MgB_{2}, which has sheetdependent anisotropy, the superconducting gap in momentum space of NbSe_{2}, Δ_{nk}, varies considerably in magnitude both between sheets and within a single sheet. We also note that whereas anisotropic effects in MgB_{2} enhance T_{c}^{56,57,58}, that of NbSe_{2} stays almost constant if anisotropy is washed out. Nevertheless, the degree of gap anisotropy is of essential importance for understanding thermodynamic and spectroscopic properties^{27,32,34,36,45,59,60,61}. Figure 3d shows the histograms of gap values
over the full BZ (green) and the k_{z} = 0 cut of the FS (red). The total distribution reveals a spread of gap values with the main peak at 2.3 meV and several smaller structures at lower values of Δ. While mid and lowenergy features of the curve are well reproduced by the k_{z} = 0 slice of the CDW BZ, the source of the peak can be identified with a hot spot in Δ_{nk} at 2/3 of the ML line. The obtained average gap value is of \(\bar{{{\Delta }}}\) = 1.85 meV, corresponding to \(2\bar{{{\Delta }}}/{k}_{{{{{{\rm{B}}}}}}}{T}_{{{{{{\rm{c}}}}}}}\) = 4.3, which is in excellent agreement with experiments^{59}. Our overestimation of T_{c} naturally leads to an overestimation of the gap. However, multiplying Δ by the factor \({T}_{{{{{{\rm{c}}}}}}}^{\exp }/{T}_{{{{{{\rm{c}}}}}}}\), the estimated gap is rescaled in between 0.7 and 1.7 meV, which is close to the range seen in Fig. 1b and provided by ARPES measurements^{33}. Figure 3c shows the unfolded gap structure on constantk_{z} slices of the BZ. We see a complex pattern of superconducting gaps that, like for other anisotropic superconductors^{62,63,64}, mirrors the structure of the EPC (compare the k_{z} = 0 slice with Fig. 3b). In the k_{z} = 0 plane, a highgap region can be identified with the inner FS sheet of Nb character around the Γ point, while the Fermi arcs at K have, on average, a much smaller superconducting gap. This observation agrees with the inverse correlation between superconducting and CDW gap suggested by ARPES measurements^{32}. Nevertheless, as already mentioned, the FS Kcylinder largely contributes to the superconducting condensation energy due to the overall higher DOS (Table 1) and a significant increase in the gap at large k_{z} (see the slice at \({{{{{{\bf{k}}}}}}}_{z}=\frac{2}{3}\frac{\pi }{c}\)).
Discussion
For a direct comparison with the experiment, we simulated STM images of bulk NbSe_{2} by a superconducting Nb tip using the SCDFT gap. Specifically, the superconducting DOS of the sample was computed locally at the tip position from the realspace projection of Eq. (4) (see Supplementary Note 3 for an extended discussion). Figure 5a shows the computational differentialconductance spectra of layer L_{1}, L_{2} and the full bulk, compared to the experimental spectrum averaged over the sample surface. The tunneling conductance calculated at the points corresponding to the experimental positions in Fig. 1a is also included. The related histograms of gap values are presented in Fig. 5b. Additionally, Fig. 5c provides a realspace image of the superconducting gap from a side view (bottom) and through horizontal cuts on the Nb planes of L_{1} and L_{2} (top). Simulations show a strong variation of the tunneling conductance with the scanning position, especially between the layers. Due to the higher DOS at the Fermi level, L_{2} has, in fact, a much larger average gap (see the highenergy peak in the distribution of gap values). Moreover, a doublepeak structure is clearly visible in the differential conductance computed for L_{2}, whereas it almost disappears for L_{1}. Changes in the experimental spectra as a function of the tip position are much less pronounced, and two distinct peaks are always observed (see Fig. 1 and Supplementary Note 4). However, in comparing simulated and experimental spectra, one should consider that the actual CDW is slightly incommensurate, and that the structural patterns on L_{1} and L_{2} exist, in fact, on the same surface, smoothly transforming into each other^{42}. This causes an additional degree of hybridization between the electronic states of the two layers, which is not accounted for in the simulations, as it would require using a prohibitively large cell. Additionally, simulations are done in the bulk, thus in absence of surface effects which may influence the gap anisotropy. Nevertheless, by comparing the black and green curves in Fig. 5, we see that the shape of the measured dI/dV tunneling spectrum is, overall, quite well reproduced, especially concerning the positions of the two peaks and the shoulderlike feature at ≈ 3 meV.
We mention that in a recent letter Heil and coworkers^{65} used abinitio Migdal–Eliashberg theory to simulate the superconducting properties and tunneling characteristics of NbS_{2}. While the tunneling spectra show strong similarities with those we predict and measure for NbSe_{2}, in the case of NbS_{2} they are found to originate from a clear twogap structure. If, on the one hand, these results demonstrate the importance of abinitio methods for the interpretation of tunneling data, they also show that similar dichalcogenides can hide significantly different superconducting properties. It would be of interest to address this aspect by a detailed comparative abinitio study.
To summarize, we presented highresolution STM measurements of the differential conductance of NbSe_{2} and an ab initio fully anisotropic description of the CDW and superconducting state. The agreement between measured and computed superconducting properties appears to be good. From our analysis emerge the following key aspects: (i) Contrary to the textbook case of MgB_{2}, the gap anisotropy does not influence the stability of the superconducting state, that is perturbations affecting the gap anisotropy are not expected to reduce T_{c}. (ii) The gap distribution on the FS shows rapid variations with k within each sheet. However, a highgap structure can be clearly identified as responsible for the main STM coherence peak. Specifically, the peak originates from the same FS sheet that is broken by the occurrence of the CDW, i.e., the FS cylinder centered at the K point. (iii) HC regions of the crystal undergo a strong reduction of the Fermi DOS by the CDW, leading to a lower EPC compared to CC regions (whose Fermi DOS is almost unaffected).
Overall, our simulations indicate that superconducting and CDW orderings in NbSe_{2} compete in HC regions, whereas superconductivity is not suppressed in CC regions. We rule out, however, a twogap scenario, providing evidence of strong superconducting gap anisotropy.
Methods
Crystal synthesis and characterization
Bulk crystals of NbSe_{2} were grown by chemical vapor transport^{32} and cleaved under ultrahigh vacuum. Scanning tunneling microscopy and spectroscopy measurements were performed at 1.1 K with superconducting tips fabricated by indenting a clean NbTi wire into a Nb(111) crystal until the tip’s energy gap reached the bulk value (2Δ_{tip} ≈ 3.1 meV). Since the probed signal is a convolution of the DOS of substrate and tip, all the measured spectral features of the sample are shifted by the tip’s energy gap. Additionally, the differentialconductance signal is weighted by the energydependent tunneling probability.
Theoretical calculations
We calculated normalstate properties within DFT^{66,67} using the local density approximation^{68}. Atomic core states were treated in the normconserving pseudopotential approach as implemented in the Quantum Espresso code^{69}. Phonon frequencies and EPC were computed by means of density functional perturbation theory^{70} with an electronic temperature of 270 meV^{40}. Further computational details are given in Supplementary Note 2.
Data availability
The data that support the findings of this study are available from the corresponding author upon reasonable request.
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Acknowledgements
The authors acknowledge financial support by the European Research Council Advanced Grant FACT (ERC2017AdG788890), the CarESS project, Deutsche Forschungsgemeinschaft through grant CRC 183 (project C03), and the European Research Council through the consolidator grant “NanoSpin”.
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K.R. provided the samples. E.L. and K.J.F. performed the STM characterization and related analysis. A.S and C.P. performed abinitio simulations and their analysis. A.S., C.P., E.L., K.R., K.J.F., and E.K.U.G. contributed to the discussion and writing of the manuscript.
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Sanna, A., Pellegrini, C., Liebhaber, E. et al. Realspace anisotropy of the superconducting gap in the chargedensity wave material 2HNbSe_{2}. npj Quantum Mater. 7, 6 (2022). https://doi.org/10.1038/s41535021004128
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DOI: https://doi.org/10.1038/s41535021004128
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