Abstract
The properties of cuprate high-temperature superconductors are largely shaped by competing phases whose nature is often a mystery. Chiefly among them is the pseudogap phase, which sets in at a doping p* that is material-dependent. What determines p* is currently an open question. Here we show that the pseudogap cannot open on an electron-like Fermi surface, and can only exist below the doping p FS at which the large Fermi surface goes from hole-like to electron-like, so that p* ≤ p FS. We derive this result from high-magnetic-field transport measurements in La1.6−x Nd0.4Sr x CuO4 under pressure, which reveal a large and unexpected shift of p* with pressure, driven by a corresponding shift in p FS. This necessary condition for pseudogap formation, imposed by details of the Fermi surface, is a strong constraint for theories of the pseudogap phase. Our finding that p* can be tuned with a modest pressure opens a new route for experimental studies of the pseudogap.
Similar content being viewed by others
Introduction
A central puzzle of cuprate superconductors1, the pseudogap is a partial gap that opens in their spectral function, detected most directly by angle-resolved photoemission spectroscopy (ARPES). It opens below a temperature T* that decreases monotonically with increasing hole concentration (doping) p. For example, T* = 130 ± 20 K in La2-x Sr x CuO4 (LSCO) at p = 0.152 and T* = 75 ± 5 K in La1.6−x Nd0.4Sr x CuO4 (Nd-LSCO) at p = 0.203. Transport properties like the electrical resistivity ρ(T) and the Nernst coefficient ν(T) are affected by the opening of the pseudogap and so may be used to detect T*, as previously reported in refs. 4,5 and ref. 6, respectively.
In Fig. 1a, we show the temperature-doping phase diagram of LSCO, Nd-LSCO and La1.8-x Eu0.2Sr x CuO4 (Eu-LSCO). We see that all three materials have the same T* up to p ~0.17, irrespective of their different crystal structures6. Indeed, Nernst data6 show, for example, that T* = 120 ± 10 K at p = 0.15 in both LSCO and Nd-LSCO, whose structure in that part of the phase diagram is orthorhombic, and T* = 115 ± 10 K at p = 0.16 in Eu-LSCO, whose structure in that part of the phase diagram is tetragonal (LTT) (Supplementary Fig. 1). In Nd-LSCO and Eu-LSCO, T* decreases linearly all the way from p ~0.08 to p ~0.23 (blue line in Fig. 1a). On its trajectory, the T* line goes unperturbed through the LTT transition at p ~0.14 for Eu-LSCO (short green line) and at p ~0.19 for Nd-LSCO (short red line). Clearly, the pseudogap mechanism does not care about the crystal structure (Note that it is also robust against disorder7).
The critical doping p* at which the pseudogap phase comes to an end, however, is material-specific. In LSCO, the linear decrease in T* vs p comes to an end at p* = 0.18 ± 0.018,9. In Nd-LSCO, resistivity measurements4,5 at p = 0.20 and above show that the T* line only comes to an end at p* = 0.23 ± 0.01. Why does T* not continue to track the dashed blue line in Fig. 1 beyond p = 0.17 for LSCO, or beyond p = 0.23 for Nd-LSCO? In Fig. 1e, we plot p* for the three single-layer cuprates LSCO, Nd-LSCO and Bi220110, as a function of p FS, the doping at which the Fermi surface undergoes a change from hole-like to electron-like as determined by ARPES measurements2,3,11,12. Within error bars, we observe that p* = p FS, in other words, it appears that what limits p* is the constraint that the pseudogap cannot open on an electron-like Fermi surface.
In the following, we examine whether this connection is accidental or not, by independently probing how p* and p FS evolve under the effect of hydrostatic pressure in Nd-LSCO. With a maximal T c of only 20 K, this cuprate provides a window into the pseudogap phase near its end point at p*, free of superconductivity, down to the T = 0 limit, achieved by applying a magnetic field of 30 T (or greater), whose sole effect is to suppress superconductivity and reveal the underlying normal state (ref. 5). Our measurements reveal a large and unexpected downward shift of p* with pressure, which we find to be driven by a corresponding change in p FS, so that the relation p* ≤ p FS is obeyed. This fundamental property has direct and fundamental implications for the mechanism of pseudogap formation.
Results
Determination of p* and p FS
Our study is based on transport signatures of p* and p FS. We begin with p*. When p < p*, the electrical resistivity ρ(T), Nernst coefficient and Hall coefficient R H(T) all exhibit large upturns at low temperature4,5,6,9—signatures of the pseudogap phase, attributed to a drop in carrier density n from n = 1 + p above p* to n = p below p*5,9,13. In Nd-LSCO at p = 0.20, ARPES sees a gap opening at T* = 75 K (ref. 3), precisely the temperature below which the resistivity exhibits an upward deviation from its high-T linear behaviour4,5. By contrast, at p = 0.24 the three transport coefficients show no trace of any upturn at low T 4,5,6,, with the resistivity remaining linear down to T → 0 (Fig. 2a), consistent with the absence of a gap in ARPES data3.
In Fig. 3, we reproduce published data5 for ρ(T) (Fig. 3a) and R H(T) (Fig. 3c) in Nd-LSCO at different dopings. The upturns decrease as p approaches p* from below. We determine p* as the doping where the upturns in ρ(T) and R H(T) vanish, giving p* = 0.23 ± 0.01 (Fig. 4). (Note that at that doping ρ(T) displays a slight upturn while R H(T) remains flat. This difference comes possibly from the fact that ρ(T) is sensitive to the total carrier density while R H(T) is balanced by electron- and hole-like contributions, as in the reconstructed Fermi surface just below p* for an anti ferromagnetic scenario14. See discussion in ref. 5).
We now turn to p FS. In a single-layer cuprate, the Fermi surface changes topology from hole-like at p < p FS (Fig. 1c) to electron-like at p > p FS (Fig. 1d). (p FS is the doping at which the van Hove singularity in the density of states crosses the Fermi level.) ARPES studies show that the Fermi surface is hole-like in LSCO at p = 0.1711 and Nd-LSCO at p = 0.203, while it is electron-like at p = 0.202 and p = 0.243, respectively, so that p FS = 0.19 ± 0.01 in LSCO and p FS = 0.22 ± 0.01 in Nd-LSCO.
Changes under hydrostatic pressure
We now examine the effect of pressure on p FS and p*. Pressure is known to change the crystal structure of Nd-LSCO from LTT at ambient pressure to HTT at P > 4.2 GPa15. Our band–structure calculations based on a standard tight-binding model (see 'Methods' section and Supplementary Fig. 2) show that this causes a decrease in the ratio |t’/t|, where t and t’ are nearest- and next-nearest-neighbour hopping parameters. It is a property of this model that the Fermi surface goes from hole-like to electron-like with decreasing |t’/t| (at fixedp), consistent with fits to ARPES data on LSCO2,11. Pressure applied to Nd-LSCO is therefore expected to reduce p FS (Fig. 5c). Although the maximum pressure in our experiment is 2.0 GPa, it still reduces the CuO6 octahedron tilt angle of the LTT structure significantly towards the HTT phase15, which decreases |t’/t|.
Experimentally, we study the pressure dependence of p FS by looking at R H for p ≥ p*. In LSCO in the regime above p FS ~0.19, R H decreases linearly with doping as the system moves away from p FS (Supplementary Fig. 3), to eventually become negative abovep~0.3516,17. Quantitatively, an increase in doping by δp = 0.02 corresponds to a ~13% drop in R H (Fig. 5b). Since all there is in this regime is a single large electron-like Fermi surface, Nd-LSCO in the regime above p FS ~0.22 must display a similar linear decrease of R H with doping, possibly with a different absolute value. Hence, the same relative change in R H is expected to correspond to a similar displacement in doping. In Fig. 5a (see also Supplementary Fig. 4), we see that R H in Nd-LSCO at p = 0.25 decreases by ~12% under 2 GPa, which implies that p FS in Nd-LSCO shifts down by δp FS ~0.02 under 2 GPa, based on the LSCO data.
To study the pressure dependence of p*, we measured the high-field normal-state resistivity under pressure up to 2 GPa. Our data on LSCO below p* show that the pseudogap is unaffected by pressure, in the sense that the amplitude of the low-T upturn in the resistivity at p = 0.143 (ref. 9) is unchanged (Supplementary Fig. 5). In Nd-LSCO at p = 0.15, our measurements (Fig. 2b and Supplementary Fig. 6) also show that T* is independent of pressure, as previously observed in YBa2Cu3O y (ref. 18). So a pressure of 2 GPa does not tune T* directly. Nevertheless, in Nd-LSCO just below p* we observe a dramatic effect of pressure on the pseudogap: at p = 0.22, 2.0 GPa completely eliminates the low-T upturn in the resistivity (Fig. 2c), resulting in a linear T behaviour characteristic of the regime at p* and above (refs. 4,8). A suppression of the low-T upturn is also seen at p = 0.21 (Fig. 3b). This large and unexpected effect of pressure on the pseudogap is our main experimental finding.
In Fig. 3, we compare the effect of pressure on the resistivity and Hall coefficient of Nd-LSCO with the effect of doping. (Note that unlike for YBa2Cu3Oy, pressure does not change the doping in Nd-LSCO, which is set by the Sr content.) We see that pressure has the same effect as doping, consistent with a lowering of p* induced by pressure. Quantitatively, p* moves down from 0.23 at P = 0 to 0.21 at P = 2.0 GPa (Fig. 4). A downward shift δp* = −0.02 in 2.0 GPa is the same shift (δp FS ~ −0.02) that is observed for p FS. We infer that it is the downward movement of p FS that constrains p* to move down with pressure, thereby showing that the condition p* ≤ p FS must hold.
Discussion
This elucidates why the pseudogap phase of LSCO ends at a lower doping than in Nd-LSCO, for indeed p* = p FS in LSCO, within error bars (Fig. 1e). In most cuprates, p FS is much higher, as in the single-layer material Bi2201, for example, where p FS = 0.41 ± 0.02 (ref. 12). Remarkably, p* is nearly as high, with p* = 0.38 ± 0.02 in Bi2201 (ref. 10), as illustrated in Fig. 1e.
Our finding that p* ≤ p FS is consistent with the known properties of all cuprates. In particular, it holds true for all known single-layer cuprates, including not only those in Fig. 1e, but also Tl2Ba2CuO6+δ, for example, where at p ~0.3 the Fermi surface is hole-like and there is no pseudogap19. It also holds for bi-layer cuprates, such as Bi2Sr2CaCu2O8+δ, in the sense that the pseudogap opens only once20 or after21 both Fermi surfaces (bonding and anti-bonding) have become hole-like22. The close proximity of p* to a van Hove singularity (at p FS) may have some impact on the physics of the pseudogap. However, since the velocity vanishes at the van Hove point, we do not expect any singularity in the transport properties. Moreover, in the presence of substantial c-axis dispersion, of the order of t z ~20 meV in Nd-LSCO, the divergence in the density of states gets cut off at low temperature23.
It is striking that a minute change in the Fermi surface, smaller than that illustrated between Fig. 1c (p slightly below p FS) and Fig. 1d (p slightly above p FS), can switch off a gap of magnitude ~20 meV (ref. 3). This extreme sensitivity of the pseudogap on the details of the Fermi surface suggests that for the pseudogap to form it is necessary that the Fermi surface intersects the anti ferromagnetic zone boundary (AFZB), the dashed line in Fig. 1d, as proposed in refs. 20,24. This is precisely what happens when the doping drops below p FS. There is empirical evidence that this intersection may indeed be a crucial element of the pseudogap mechanism. First, this AFZB is where in k-space the separation of ungapped and (pseudo)gapped states occurs, as detected by quasiparticle interference in scanning tunnelling microscopy21. In other words, the AFZB is the pseudogap phase’s organising principle in k-space: it defines the so-called 'Fermi arcs'. Note thatwhen the pseudogap turns on (with decreasing T or p), the k-space area contained by the ungapped states (between the Fermi arcs and the AFZB) goes from A ~ 1 + p to A ~ p (ref. 21). Second, upon crossing p* from above, the carrier density measured by the Hall number goes from n = 1 + p to n = p (refs. 5,13), consistent with A ~ n. The simplest way to obtain a loss of 1.0 hole per planar Cu atom is to reconstruct the large hole-like Fermi surface (with 1 + p holes) by folding it about the AFZB, which produces four small nodal hole pockets (with p holes)14. This can be achieved either by AF order with a wavevector Q = (π, π) or by an Umklapp surface coincident with the AFZB, as in the YRZ model25. If this is indeed how the pseudogap phase transforms the Fermi surface, then no Fermi arcs (or nodal pockets) can form when p > p FS. Electron-doped cuprates provide a clear example of Fermi surface reconstruction caused by long-range AF order, where the AFZB plays a key role, but where no pseudogap phase forms26. The issue of why there is a pseudogap in hole-doped cuprates and not in electron-doped cuprates, however, is an open question.
If the pseudogap phase needs states near (π, 0) to form, the question is at what energy do those states have to be relative to ε F? We presume that they should be within the pseudogap energy ΔPG of ε F. This implies that for p just above p FS, the pseudogap phase can still form. This introduces some 'width' to the criterion p* ≤ p FS. In a similar vein, a 3D dispersion of the Fermi surface in the k z (or c) direction will also give some 'width' to the criterion, since at a given doping the Fermi surface can be electron-like at some k z value but still hole-like at some other k z value.
The requirement that a pseudogap cannot form in a cuprate with an electron-like Fermi surface imposes a stringent constraint on theories of the pseudogap phase25,27,28,29,30,31. In the YRZ model25, a pseudogap forms because carriers undergo Umklapp scattering, inherited from the Mott insulator, at points where the Fermi surface intersects the AFZB; this model therefore agrees with our proposed constraint. Our findings are also broadly consistent with spin-fermion models that hinge on the hot spots that lie at the intersection of Fermi surface and AFZB27,28. More specifically, two recent theoretical studies29,32 find that a pseudogap only opens on hole-like Fermi surfaces and that p* ≤ p FS for a wide range of band–structure parameters, even in the strong-coupling regime where the anti ferromagnetic correlations responsible for the pseudogap are short ranged. On the other hand, in scenarios characterised by a wavevector Q = (0, 0), the AFZB plays no special role and there is then no obvious reason for the constraint to be effective. This would seem to rule out nematic order31 and intra-unit cell magnetic order30,33 as possible drivers of the pseudogap phase. Instead, these orders would be secondary instabilities6.
On the experimental side, the ability to continuously suppress and restore the pseudogap with pressure in a given sample without changing the doping or disorder level provides a promising avenue to study the pseudogap state, compatible with a range of probes such as Raman, optics, X-ray and neutron scattering.
Methods
LSCO samples
Single crystals of La2−x Sr x CuO4 (LSCO) were grown by the flux-zone technique, with nominal Sr concentrations of x = 0.145 at Hokkaido University and x = 0.18 at the University of Tokyo. Samples for resistivity measurements were cut in the shape of small rectangular platelets, of typical dimensions 1 mm × 2 mm × 0.5 mm, with the smallest dimension along the c axis. Contacts were made using H20E silver epoxy, diffused by annealing. The hole concentration (doping) p for our nominal x = 0.145 sample was determined using the doping dependence of the (tetragonal to orthorhombic) structural transition temperature, T LTO, which is detected in the resistivity as a small but sharp kink. This yields p = 0.143 (ref. 9). For our sample with x = 0.18, we take p = x.
Nd-LSCO samples
Single crystals of La2−y−x Nd y Sr x CuO4 (Nd-LSCO) were grown at the University of Texas at Austin with a Nd content y = 0.4, using a travelling-float-zone technique, and cut from boules with nominal Sr concentrations x = 0.15, 0.21, 0.22, 0.23 and 0.25. The samples were prepared for transport measurements as described above for the LSCO samples. For all five samples, the hole concentration p is given by p = x, with an error bar ±0.003. The samples labelled here p = 0.21, 0.22, 0.23 and 0.24 are the same samples as those studied in ref. 5; the sample labelled here p = 0.25 is a new sample, with p = 0.25 ± 0.003.
Resistivity and Hall measurements
The electrical transport measurements were performed via a standard four-point low AC technique using an SR830 lock-in amplifier and a Keithley 6221 current source. A current of typically 2 mA was applied within the CuO2 planes and the magnetic field along the c-axis. The longitudinal and Hall resistances R xx and R xy were measured at Sherbrooke in steady fields up to 16 T and at the NHMFL in steady fields up to 45 T. The Hall resistance R xy is obtained by reversing the field and anti-symmetrizing the data, as R xy (H) = (R xy ( + H) − R xy (−H))/2.
Application of pressure
Pressure was applied on our samples using a miniature non-magnetic piston-cylinder cell. The pressure medium is Daphne oil 7474, which remains liquid at all pressures measured here at 300 K, ensuring a high degree of hydrostaticity. The internal pressure is measured both at room temperature and at 4.2 K, using either the fluorescence of a small ruby chip or a Sn manometer. The values quoted throughout are the low temperature pressures. The error bar on all the pressure values is ± 0.05 GPa, which comes from the uncertainty in measuring the position of the fluorescence peaks. For each measurement, the cell was cooled slowly (<1 K min−1) to ensure a homogeneous freezing of the pressure medium.
Band–structure calculations
Band–structure calculations were performed by using the full potential augmented plane wave band method, implemented in the WIEN2k package. We used the local density approximation for the exchange-correlation potential. We used 1000 k-points inside the first Brillouin zone. The convergence of total energy with respect to the number of k-points was checked to have a precision better than 0.007 eV per formula unit. We calculated the electronic structure of La2CuO4 using the structural parameters of Nd-LSCO measured experimentally by X-ray diffraction for both ambient pressure (LTT structure; ref. 34 and P = 4.2 GPa (HTT structure; ref. 15). In the case of P = 4.2 GPa (HTT), in order to determine the internal position of atoms inside the CuO6 octahedron, we assumed an isotropic contraction of the CuO6 octahedra from hydrostatic pressure. Experiments on La2CuO4 have shown this assumption to be valid35. Tight-binding hopping parameters were obtained by fitting Cu(d x2-y2)-driven bands for high-symmetry points of the anti ferromagnetic zone boundary.
Sample size
No statistical methods were used to predetermine sample size.
Data availability
All relevant data are available from the authors.
References
Keimer, B., Kivelson, S. A., Norman, M. R., Uchida, S. & Zaanen, J. From quantum matter to high-temperature superconductivity in copper oxides. Nature 518, 179–186 (2015).
Yoshida, T. et al. Universal versus material-dependent two-gap behaviors of the high-T c cuprate superconductors: angle-resolved photoemission study of La2-xSrxCuO4. Phys. Rev. Lett. 103, 037004 (2009).
Matt, C. E. et al. Electron scattering, charge order, and pseudogap physics in La1.6−xNd0.4SrxCuO4: an angle-resolved photoemission spectroscopy study. Phys. Rev. B 92, 134524 (2015).
Daou, R. et al. Linear temperature dependence of resistivity and change in the Fermi surface at the pseudogap critical point of a high-T c superconductor. Nat. Phys. 5, 31–34 (2009).
Collignon, C. et al. Fermi-surface transformation across the pseudogap critical point of the cuprate superconductor La2-xNd0.4SrxCuO4. Phys. Rev. B 95, 224517 (2017).
Cyr-Choinière, O. et al. Pseudogap temperature T* of cuprate superconductors from the Nernst effect. Preprint at http://arxiv.org/abs/1703.06927 (2017).
Rullier-Albenque, F., Alloul, H., Balakirev, F. & Proust, C. Disorder, metal-insulator crossover and phase diagram in high-T c cuprates. Europhys. Lett. 81, 37008 (2008).
Cooper, R. A. et al. Anomalous criticality in the electrical resistivity of La2-xSrxCuO4. Science 323, 603–607 (2009).
Laliberté, F. et al. Origin of the metal-to-insulator crossover in cuprate superconductors. Preprint at http://arxiv.org/abs/1606.04491 (2016).
Kawasaki, S. et al. Carrier-concentration dependence of the pseudogap ground state of superconducting Bi2Sr2-xLaxCuO6+δ revealed by Cu nuclear magnetic resonance in very high magnetic fields. Phys. Rev. Lett. 105, 137002 (2010).
Chang, J. et al. Anisotropic quasiparticle scattering rates in slightly underdoped to optimally-doped high-temperature La2−xSrxCuO4 superconductors. Phys. Rev. B 78, 205103 (2008).
Kondo, T. et al. Hole-concentration dependence of band structure in (Bi,Pb)2(Sr,La)2CuO6+δ determined by angle-resolved photoemission spectroscopy. JESRP 137-140, 663–668 (2004).
Badoux, S. et al. Change of carrier density at the pseudogap critical point of a cuprate superconductor. Nature 531, 210–214 (2016).
Storey, J. G. Hall effect and Fermi surface reconstruction via electron pockets in the high-T c cuprates. Europhys. Lett. 113, 27003 (2016).
Crawford, M. K. et al. High-pressure study of structural phase transitions and superconductivity in La1.48Nd0.4Sr0.12CuO4. Phys. Rev. B 71, 104513 (2005).
Ando, Y. et al. Evolution of the Hall coefficient and the peculiar electronic structure of the cuprate superconductors. Phys. Rev. Lett. 92, 197001 (2004).
Tsukada, I. & Ono, S. Hall coefficients of heavily overdoped La2-xSrxCuO4. Phys. Rev. B 74, 134508 (2006).
Cyr-Choinière, O. et al. Suppression of charge order by pressure in the cuprate superconductor YBa2Cu3Oy: Restoring the full superconducting dome. Preprint at http://arxiv.org/abs/1503.02033 (2015).
Platé, M. et al. Fermi surface and quasiparticle excitations of overdoped Tl2Ba2CuO6+δ cuprate superconductor. Phys. Rev. Lett. 95, 077001 (2005).
Benhabib, S. et al. Collapse of the normal-state pseudogap at a Lifshitz transition in the Bi2Sr2CaCu2O8+δ cuprate superconductor. Phys. Rev. Lett. 114, 147001 (2015).
Fujita, K. et al. Simultaneous transitions in cuprate momentum-space topology and electronic symmetry breaking. Science 344, 612–616 (2014).
Kaminski, A. et al. Change of Fermi-surface topology in Bi2Sr2CaCu2O8+δ with doping. Phys. Rev. B 73, 174511 (2006).
Markiewicz, R. S., Sahrakorpi, S., Lindroos, M., Lin, H. & Bansil, A. One-band tight-binding model parametrization of the high-T c cuprates including the effect of k z dispersion. Phys. Rev. B 72, 054519 (2005).
Loret, B. et al. Vertical temperature boundary of the pseudogap under the superconducting dome in the phase diagram of Bi2Sr2CaCu2O8+d. Phys. Rev. B 96, 094525 (2017).
Yang, K.-Y., Rice, T. M. & Zhang, F.-C. Phenomenological theory of the pseudogap state. Phys. Rev. B 73, 174501 (2006).
Armitage, N. P., Fournier, P. & Greene, R. L. Progress and perspectives on electron-doped cuprates. Rev. Mod. Phys. 82, 2421–2487 (2010).
Efetov, K. B., Meier, H. & Pépin, C. Pseudogap state near a quantum critical point. Nat. Phys. 9, 442–446 (2013).
Chowdhury, D. & Sachdev, S. Higgs criticality in a two-dimensional metal. Phys. Rev. B 91, 115123 (2015).
Wu, W., Georges, A. & Ferrero, M. Pseudogap and Fermi-surface topology in the two-dimensional Hubbard model. Preprint at http://arxiv.org/abs/1707.06602 (2017).
Varma, C. M. Pseudogap phase and the quantum critical point in copper oxide metals. Phys. Rev. Lett. 83, 3538–3541 (1999).
Nie, L., Tarjus, G. & Kivelson, S. A. Quenched disorder and vestigial nematicity in the pseudogap regime of the cuprates. PNAS 111, 7980–7985 (2014).
Braganca, H., Sakai, S., Aguiar, M. C. O. & Civelli, M. Correlation-driven Lifshitz transition at the emergence of the pseudogap phase in the two-dimensional Hubbard model. Preprint at http://arxiv.org/abs/1708.02084 (2017).
Sidis, Y. & Bourges, P. Evidence for intra-unit-cell magnetic order in the pseudogap state of high-Tc cuprates. Preprint at http://arxiv.org/abs/1306.5124 (2013).
Axe, J. D. & Crawford, M. K. Structural instabilities in lanthanum cuprate superconductors. J. Low. Temp. Phys. 95, 271–284 (1994).
Akhtar, M. J. et al. The pressure dependence of the crystal structure of La2CuO4. J. Phys. C Solid State Phys. 21, L917–L920 (1988).
Fink, J. et al. Phase diagram of charge order in La1.8−xEu0.2SrxCuO4 from resonant soft X-ray diffraction. Phys. Rev. B 83, 092503 (2011).
Acknowledgements
We thank the following for enlightening discussions: S. Benhabib, G. Boebinger, C. Bourbonnais, J. Chang, S. Chakravarty, M. Ferrero, A. Georges, G. Kotliar, G. G. Lonzarich, A. J. Millis, C. Pépin, C. Proust, A. Sacuto, D. Sénéchal, A.-M. Tremblay, S. Verret, and W. Wu. A portion of this work was performed at the National High Magnetic Field Laboratory, which is supported by National Science Foundation Cooperative Agreement No. DMR-1157490 and the State of Florida. L.T. thanks the Collège de France for its hospitality and the European Research Council (Grant No. ERC-319286 QMAC) and LABEX PALM (ANR-10-LABX-0039-PALM) for their support, while this article was written. J.-S.Z. was supported by DOD-ARMY (W911NF-16-1-0559) in the United States. H.T. acknowledges MEXT Japan for a Grant-in-Aid for Scientific Research. L.T. acknowledges support from the Canadian Institute for Advanced Research (CIFAR) and funding from the Natural Sciences and Engineering Research Council of Canada (NSERC; PIN:123817), the Fonds de recherche du Québec – Nature et Technologies (FRQNT), the Canada Foundation for Innovation (CFI) and a Canada Research Chair. Part of this work was funded by the Gordon and Betty Moore Foundation’s EPiQS Initiative (Grant GBMF5306 to L.T.).
Author information
Authors and Affiliations
Contributions
N.D.-L., O.C.-C., S.B., A.A., A.G., S.D.-B., F.F.T., and F.L. performed the transport measurements under pressure and ambient conditions at Sherbrooke. N.D.-L., O.C.-C., S.B., C.C., A.G., S.D.-B., M.-E.B., M.M., and D.G. performed the transport measurements under pressure and ambient conditions at the NHMFL in Tallahassee. M.K. performed the band–structure calculations. J.-S.Z. grew the Nd-LSCO single crystals. N.M. and T.K. grew the LSCO single crystal with x = 0.145. H.T. grew the single crystal with x = 0.18. N.D.-L. and L.T. wrote the manuscript, in consultation with all authors. N.D.-L. and L.T. supervised the project.
Corresponding authors
Ethics declarations
Competing interests
The authors declare no competing financial interests.
Additional information
Publisher's note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Electronic supplementary material
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Doiron-Leyraud, N., Cyr-Choinière, O., Badoux, S. et al. Pseudogap phase of cuprate superconductors confined by Fermi surface topology. Nat Commun 8, 2044 (2017). https://doi.org/10.1038/s41467-017-02122-x
Received:
Accepted:
Published:
DOI: https://doi.org/10.1038/s41467-017-02122-x
This article is cited by
-
Planckian dissipation and non-Ginzburg-Landau type upper critical field in Bi2201
Science China Physics, Mechanics & Astronomy (2023)
-
Ultra-high critical current densities of superconducting YBa2Cu3O7-δ thin films in the overdoped state
Scientific Reports (2021)
-
Fluctuation induced conductivity and pseudogap state studies of Bi1.6Pb0.4Sr2Ca2Cu3O10+δ superconductor added with ZnO nanoparticles
Scientific Reports (2021)
-
Magnetotransport of dirty-limit van Hove singularity quasiparticles
Communications Physics (2021)
-
A picture of pseudogap phase related to charge fluxes
npj Computational Materials (2020)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.