Anomalous density fluctuations in a strange metal

M. Mitrano; A. A. Husain; S. Vig; A. Kogar; M. S. Rak; S. I. Rubeck; J. Schmalian; B. Uchoa; J. Schneeloch; R. Zhong; G. D. Gu; P. Abbamonte

doi:10.1073/pnas.1721495115

Edited by Steven A. Kivelson, Stanford University, Stanford, CA, and approved April 10, 2018 (received for review December 10, 2017)

Significance

The strange metal is a poorly understood state of matter found in a variety of quantum materials, notably both Cu- and Fe-based high-temperature superconductors. Strange metals exhibit a nonsaturating, T-linear electrical resistivity, seemingly indicating the absence of electron quasiparticles. Using inelastic electron scattering, we report a momentum-resolved measurement of the dynamic charge susceptibility of a strange metal, optimally doped Bi_2.1Sr_1.9CaCu₂O_8+x. We find that it does not exhibit propagating collective modes, such as the plasmon excitation of normal metals, but instead exhibits a featureless continuum lacking either temperature or momentum dependence. Our study suggests the defining characteristic of the strange metal is a singular type of charge dynamics of a new kind for which there is no generally accepted theory.

Abstract

A central mystery in high-temperature superconductivity is the origin of the so-called strange metal (i.e., the anomalous conductor from which superconductivity emerges at low temperature). Measuring the dynamic charge response of the copper oxides, χ″(q,ω), would directly reveal the collective properties of the strange metal, but it has never been possible to measure this quantity with millielectronvolt resolution. Here, we present a measurement of χ″(q,ω) for a cuprate, optimally doped Bi_2.1Sr_1.9CaCu₂O_8+x (T_c = 91 K), using momentum-resolved inelastic electron scattering. In the medium energy range 0.1–2 eV relevant to the strange metal, the spectra are dominated by a featureless, temperature- and momentum-independent continuum persisting to the electronvolt energy scale. This continuum displays a simple power-law form, exhibiting q² behavior at low energy and q²/ω² behavior at high energy. Measurements of an overdoped crystal (T_c = 50 K) showed the emergence of a gap-like feature at low temperature, indicating deviation from power law form outside the strange-metal regime. Our study suggests the strange metal exhibits a new type of charge dynamics in which excitations are local to such a degree that space and time axes are decoupled.

The nonsuperconducting normal state of the high-temperature superconductors, usually referred to as the “strange metal,” has many properties that cannot be explained by the conventional Landau–Fermi liquid theory of metals (1, 2). These include a resistivity that is linear in temperature and exceeds the Mott–Ioffe–Regel limit (2 ⇓⇓–5), an in-plane conductivity exhibiting an anomalous power-law dependence on frequency (6, 7), a magnetoresistance that violates Kohler’s rule (8), a quasiparticle damping, Σ″(ω), that is linear in ω (9, 10), and a nuclear relaxation rate that violates the Korringa law (11). These properties, many of which are also observed in Fe- and Ru-based strange metals (2, 12 ⇓–14), imply that metallic quasiparticles are either absent or exist only marginally (15).

The main spectroscopic signature of the strange metal is a featureless continuum observed to the highest measurable energy in Raman scattering experiments (16, 17). Its origin is still unknown, exemplifying the need for a new experimental probe of the collective excitations of strange metals, particularly one that could determine how this continuum evolves at finite momentum, q. Generically, the most direct measure of the collective excitations of any material is its dynamic charge susceptibility, χ(q,ω), which reveals bosonic modes such as the plasmon excitations in ordinary metals (18). Unfortunately, it has never been possible to measure this quantity for the cuprates, at least for q≠0 at the millielectronvolt scale relevant to these materials (19).

Here we report a millielectronvolt-resolved, q≠0 measurement of the low-energy dynamic charge response of a strange metal, the optimally doped cuprate Bi_2.1Sr_1.9CaCu₂O_8+x (BSCCO), using high-resolution, momentum-resolved electron energy-loss spectroscopy (M-EELS) (19 ⇓–21). We focus here on the medium-energy region, 0.1–2 eV, most relevant to the strange metal physics. Note that this energy scale is large compared with the temperature or the superconducting gap, comparable to the superexchange, J, and small compared with the bandwidth or the Hubbard U, and so reflects the properties of the metallic phase out of which superconductivity forms. M-EELS measurements were performed on cleaved crystals of optimally doped (OP) (T_c = 91 K) and overdoped (OD) (T_c = 50 K) BSCCO (Fig. 1B) using 50-eV electrons in reflection geometry (Fig. 1A) with the energy resolution set to 4 meV. In this paper the momentum, q= |(qx,qy)|, will be expressed in tetragonal reciprocal lattice units (r.l.u.) with lattice parameter a=3.81 Å.

Fig. 1.

Probing anomalous density fluctuations in the normal state of cuprates. (A) Scattering geometry of the M-EELS experiment. ki and kf represent momenta of the incident and scattered electron, respectively, and q is the in-plane momentum transfer. (B) Schematic temperature-doping phase diagram of BSCCO showing the points investigated in this work, with filled symbols indicating where a complete q dependence was carried out. AFI, antiferromagnetic insulator; FL, Fermi liquid; PG, pseudogap; SC, superconductivity; SM, strange metal; T*, pseudogap temperature; T_c, superconducting critical temperature; T_N, Néel temperature. (C) Charge susceptibility, χ″(q,ω), of a layered electron gas calculated in the RPA using the Fermi surface parameterization of ref. 40. (D) Associated charge polarizability Π″(q,ω).

M-EELS measures the surface density–density correlation function, S(q,ω), which is related to the imaginary part of the dynamic charge response, χ″(q,ω), by the fluctuation-dissipation theorem (19, 21). χ″(q,ω) was determined from the M-EELS data by antisymmetrizing the spectra, which eliminates the Bose factor, and scaling the overall magnitude according to the f-sum rule (19). The latter (Eq. 6) normalizes out minor intensity drifts in the experiment and determines χ″(q,ω) in absolute units (Methods).

Fig. 2A shows χ″(q,ω) for optimally doped BSCCO at T = 295 K for selected momenta along the (1,1¯) direction, perpendicular to the structural supermodulation (22). The large signal at energies below 0.1 eV is from phonon excitations reported previously (19). At low momenta (q<0.15 r.l.u.), the spectra exhibit a plasmon mode at ωp∼1 eV, which was previously reported in many studies (SI Appendix, Fig. S1). Its broad linewidth indicates that this plasmon is overdamped.

Fig. 2.

Continuum collapse in OP BSCCO. (A) Dynamic charge susceptibility, χ″(q,ω), for a selection of momenta along the (1,1¯) direction at 295 K (red symbols). The spectra were divided by q² and offset for clarity. The base line for each curve is indicated by the solid line next to its momentum label. Error bars represent statistical, Poisson error. Gray lines are fits to the data using Eqs. 1 and 2. (B–D) Parameters used for the fits at every momentum measured (red symbols). Π0 represents the overall magnitude of the continuum, ωc is the cross-over energy, and V(q) is the Coulomb propagator near the surface. The dashed line in B represents a q² fit. The dashed line in D represents a fit using V(q)∝exp[−qz]/q with z=(8.1±1.5)Å. Errors in q are given by the experimental momentum resolution. Parameter errors represent systematic uncertainty derived from a variation of ±0.5 in the exponent of the ratio ωc(q)/ω in Eq. 2. (E) Scaled collapse of the polarizability, Π″(q,ω), for all measured momenta. The gray line is the fit function reported in Eq. 2. (F) Plot of the polarizability against the rescaled energy ω/vFq, showing q2/ω2 behavior above the cutoff. The gray dashed line corresponds to Π″∝q2/ω2.

As the momentum is increased to beyond q>0.15 r.l.u., the plasmon fades into a featureless, energy-independent continuum resembling that of early Raman studies (16, 17). This continuum is extremely strong, comprising >99% of the total spectral weight in the f-sum rule, and is constant up to an energy scale of 1 eV, suggesting it is electronic in origin. The continuum was found to be essentially isotropic in the (a,b) plane (SI Appendix, Fig. S2) and temperature-independent between room temperature and T = 20 K (Fig. 3A). At energies above 1 eV the susceptibility decays like a power law, χ″∼1/ω2.

Fig. 3.

Appearance of an emergent energy scale in OD BSCCO. Temperature-dependent χ″(q,ω) at q = 0.24 r.l.u. along (1,1¯) for (A) OP BSCCO and for (B) OD BSCCO. The OD data show the emergence of a ∼0.5-eV energy scale as the temperature is lowered through the cross-over region (Fig. 1B) (15).

The momentum dependence of χ″(q,ω) is highly anomalous (Fig. 2A). While its magnitude grows like q², which is required to be consistent with the f-sum rule (18, 19), the shape of the spectrum is momentum-independent from q = 0.15 r.l.u. up to the highest momentum studied, q = 0.5 r.l.u. This behavior is highly unlike that of a Fermi liquid whose propagating quasiparticles lead to a strongly momentum-dependent susceptibility, as illustrated in Fig. 1 C and D.

The broad plasmon linewidth at small momentum is evidence that the continuum is present even for q < 0.15 r.l.u., which would lead to decay of the plasmon via Landau damping (18). To evaluate this possibility, we determined the polarizability of the system, Π(q,ω), which is related to the susceptibility by (18)χ(q,ω)=Π(q,ω)ε∞−V(q)Π(q,ω),[1]where V(q) is the Coulomb interaction and ε∞ is the background dielectric constant, equal to 4.5 in this case (23). The denominator of Eq. 1, ε(q,ω)=ε∞−V(q)Π(q,ω), may be thought of as the dielectric function of the system. The difference between the polarizability and the susceptibility is that the former excludes the long-ranged part of the Coulomb interaction, revealing the particle-hole excitation spectrum without interference from plasmon effects.

Determining Π(q,ω) from Eq. 1 is complicated by the fact that the functional form of the Coulomb interaction, V(q), is not precisely known. In a homogeneous, 3D system, V(q)=4πe2/q2; however, M-EELS is a surface probe, and other functional forms are possible near a surface, in layered materials like BSCCO, or in the presence of strong screening (24, 25).

For this reason, we modeled the particle-hole continuum using the empirical expression (26)Π″(q,ω)=−Π0(q)tanh[ωc2(q)ω2].[2]This function mimics the experimental data at q > 0.15 r.l.u., where Π and χ are expected to be equal, interpolating between a constant at low energy and 1/ω2 behavior at high energy. The quantity ωc(q) defines the cross-over energy between the two regimes and Π0(q) sets the overall magnitude (26). We fit the data for ω > 0.1 eV, that is, above the phonon features, by Kramers–Kronig transforming Eq. 2 and using ωc(q), Π0(q), and V(q) as adjustable parameters. An excellent fit is obtained at all momenta, even those for q<0.15 r.l.u. in which the plasmon peak is present (Fig. 2 A–D). The resulting fit values for V(q) (Fig. 2D) have the form of a 2D Coulomb interaction, V(q)∝exp(−qz)/q, where q is the in-plane momentum and z∼10 Å, which is consistent with M-EELS being a surface probe. That Eq. 2 fits the data at all momenta suggests that the continuum is present with the functional form of Eq. 2 everywhere in momentum space—not only for q > 0.15 r.l.u. but also in the plasmon regime at low momentum.

Having established a plausible form for V(q) (Fig. 2D), we compute an empirical polarizability by multiplying the experimentally measured χ"(q,ω) by the fitted function |ε(q,ω)|2/ε∞. Note that the polarizability obtained in this manner is identical to the susceptibility for all q>0.15 r.l.u. Two distinct regimes are observed. The first is illustrated in Fig. 2E, which shows the scaled value Π″(q,ω)/Π0(q) against the scaled energy ω/ωc(q) for each experimentally measured momentum value. All of the spectra collapse to a single curve, indicating that, at energies below ωc(q), the polarizability Π″(q,ω)∝q2. The second is illustrated in Fig. 2F, which shows the unscaled value Π″(q,ω) against the scaled energy ω/vFq, where vF=2.8 eV/r.l.u. is the nodal Fermi velocity (27). All of the curves collapse again, this time demonstrating that, at energies higher than ωc(q), the polarizability Π″(q,ω)∝q2/ω2.

Stated more succinctly, the polarizability Π″(q,ω) has a simple power-law form, exhibiting an energy-independent, q2 form at low energy and q2/ω2 form at high energy. The transition between the two regions is defined by the cross-over energy, ωc(q). Note that a classic Drude response would decay like 1/ω3 at high energy (6), which is required for a convergent sum rule integral, so the observed response is unconventional to the highest energy measured. Moreover, the absence of any dispersing features in the data leads to the surprising conclusion that the collective excitations are completely local (i.e., density fluctuations in space are decoupled from those in time).

The observed power laws might be interpreted as evidence for a quantum critical point near optimal doping claimed by many authors (1). To evaluate this possibility, we repeated our experiment on OD BSCCO with T_c = 50 K, which is widely believed to exhibit a cross-over to a more Fermi liquid-like phase at low temperature (1, 5, 15). One would expect to observe deviation from simple power law behavior at low temperature. Fig. 3 shows the temperature dependence of the M-EELS spectra from OD BSCCO compared with that of the OP material. At T = 295 K, the spectra are similar, indicating that the power-law region persists over a finite range of doping at high temperature. As the temperature is lowered, however, a gap-like feature appears in the OD spectra below 0.5 eV, indicating the emergence of an energy scale not present at optimal doping. This behavior is, at first glance, consistent with the emergence of a more Fermi liquid-like phase at low temperature, and the presence of a fan-shaped quantum critical region centered on optimal doping (1, 26, 28, 29).

The data do not, however, exhibit the generic properties of a quantum critical point (29). For one, the ∼0.5-eV gap-like feature is more than an order of magnitude larger than the temperature scale on which it emerges, kBT∼20 meV.

Furthermore, the M-EELS spectra are momentum-independent even in OD samples in which the gap-like feature is observed. Fig. 4 shows the momentum dependence of the OD data at T = 115 K (SI Appendix, Fig. S4 shows the data at 295 K). The spectra show very little q dependence, just as in the OP case. We fit the data using Eqs. 1 and 2, though only for ω>0.5 eV (Fig. 4A), and obtain the fit parameters shown in Fig. 4 B–D. Despite the clear appearance of an energy scale, the spectra still collapse (Fig. 4E), with Π″(q,ω) again exhibiting q² dependence below the cross-over energy, ωc(q) (Fig. 4B). Above the cross-over energy (Fig. 4C), Π″(q,ω)∼q2/ω2 as in the OP case. We conclude that the momentum independence of the susceptibility and the absence of an observable energy scale at optimal doping are unrelated effects with different physical origin.

Fig. 4.

Continuum collapse in OD BSCCO. (A) Dynamic charge susceptibility, χ″(q,ω), of OD BSCCO (T_c = 50 K) for selected momenta along the (1,1¯) direction at 115 K (red symbols). The spectra were divided by q² and offset for clarity. The base line for each curve is indicated by the solid line next to its momentum label. Error bars represent statistical, Poisson error. Gray lines represent fits to the ω > 0.5-eV region of the spectrum using Eqs. 1 and 2. (B–D) Parameters used for the fits at every momentum measured (red symbols). Π0 represents the overall magnitude of the continuum, ωc is the cross-over energy, and V(q) is the Coulomb propagator near the surface. The dashed line in B represents a q² fit. The dashed line in D represents a fit using V(q)∝exp[−qz]/q with z=(13.23±0.60)Å. Errors in q are given by the experimental momentum resolution. Parameter errors are the systematic uncertainty derived from a variation of ±0.5 in the exponent of the ratio ωc(q)/ω in Eq. 2. (E) Scaled collapse of the polarizability, Π″(q,ω), for all measured momenta. The gray line from Fig. 2E is reproduced here for visual comparison with the gap-like feature. (F) Plot of the polarizability against the rescaled energy ω/vFq, showing q2/ω2 behavior above the cutoff. The gray dashed line corresponds to Π″∝q2/ω2.

We close by speculating about the underlying cause of the density fluctuations we observe. Our results bear a striking similarity to the so-called marginal Fermi liquid (MFL) hypothesis, which asserts that the strange metal is a consequence of a featureless continuum of fluctuations that pervades all time and length scales (30). This continuum is conjectured to arise from quantum fluctuations of some hidden order parameter that exhibits “local criticality,” meaning that the spatial correlation length ξx∼log⁡ξt, where ξt is the temporal correlation length—a situation sometimes described as having a dynamical critical exponent z=∞ (31). Our experiment affirms two aspects of the MFL hypothesis. The first is that a featureless continuum exists and contains enough spectral weight to saturate the f sum rule. The second is that, on energy scales less than ωc∼ 1 eV or 10,000 K, the polarizability factors into independent functions of momentum and energy, Π″(q,ω)=f(q)g(ω), which in MFL is the defining characteristic of local criticality, that is, decoupling of space and time axes (31). We emphasize, however, that our experiment detects only charge fluctuations and provides no evidence either for or against the existence of loop currents. Furthermore, it would be important in future work to extend these measurements to lower energies, that is, ω≤kBT, to test the postulated ω/T prediction of the MFL polarizability.

Another possibility is that the response functions of the strange metal are dominated by disorder. BSCCO is known to be electronically inhomogeneous (32) and also exhibits an incommensurate supermodulation due to structural misfit between the CuO₂ and BiO layers (33). Disorder breaks translational symmetry and can explicitly broaden features in a momentum-resolved measurement such as M-EELS. Furthermore, random disorder has been shown, in simple spin models, to give rise to singular, frequency-independent correlation functions of the sort we observe here (34, 35). Further studies of the response of strongly correlated systems to disorder are needed to clarify this issue.

Recently, theoretical approaches have been developed to address the strange metal problem from a completely new perspective. The anti-de Sitter/conformal field theory correspondence, which relates a gravity theory in a curved spacetime to a strongly interacting quantum field theory on its boundary (36), is one such approach that has already been used to reproduce some properties of the strange metal holographically (37). Rapid developments in this area may shed new light on this problem.

In summary, we present a q-resolved measurement of the dynamic charge susceptibility of a strange metal at the millielectronvolt scale. We have uncovered a type of charge dynamics in which the fluctuations are local to such a degree that space and time axes are effectively decoupled. Explaining this observation may require a new kind of theory of interacting matter.

Methods

Sample Growth and Characterization.

OP single crystals of Bi_2.1Sr_1.9Ca_1.0Cu_2.0O_8+x with T_c = 91 K were grown by the floating-zone method (38). Overdoping was achieved by annealing in a hot, isostatic press with gas pressure 6.8 kbar at temperature 500 °C for 100 h. The gas mixture was 20% O–80% Ar with oxygen partial pressures up to 1.35 kbar. The T_c values were determined using superconducting quantum interference device magnetometry.

M-EELS Measurements.

M-EELS measurements were performed using an Ibach-type HR-EELS spectrometer (39) that was motorized and mated to a custom, multiaxis sample goniometer. Centering of the rotation axes was done using remote cameras and reference scatterers, as described previously (19). Experiments were done in a magnetically shielded ultrahigh vacuum (UHV) chamber at 5 × 10⁻¹¹ torr vacuum and residual field of 3 mG using a 50-eV beam energy at 170 pA current and overall resolutions of 4 meV in energy and 0.02 Å⁻¹ in momentum. The BSCCO surfaces were prepared by cleaving along a (001) surface normal in a UHV prep chamber. Measurements were performed on three different OP and four OD crystals and tested on several cleaves of the same sample. Each figure of this paper reports data collected on a single, independent cleave. The crystals were oriented by locating elastic scattering from the (1,0) and (0,0) (specular) Bragg reflections and building an orientation matrix relating goniometer angles to momentum space (19). In this paper, Miller indices (H,K) indicate an in-plane momentum transfer q=2π(H,K)/a, where a = 3.81 Å is the tetragonal lattice parameter. All measurements were carried out at a fixed out-of-plane momentum transfer of L=20, defined in terms of a c-axis lattice parameter 30.8 Å. Wide-energy scans were binned into 30-meV groups to improve statistics.

Determining the Susceptibility from M-EELS Data.

The M-EELS cross-section is given by (19, 21)∂2σ∂Ω∂ω=σ0M2(q)⋅S(q,ω),[3]

where σ0=I0(Ei−ω)/Ei (E_i being the incident electron energy) is a weakly energy-dependent prefactor and S(q,ω) is the dynamic structure factor of the surface. The Coulomb matrix element is given byM(q)=4πe2q2+(kiz+ksz)2,[4]

where q is the in-plane component of the momentum transfer and kiz and ksz are the out-of-plane momenta of the incident and scattered electrons, respectively. As described previously (19), we obtained the density response, χ″(q,ω), using the following procedure. First, M2(q) and σ0 were divided from the experimental data, which yields S(q,ω) to within a multiplicative constant. We then removed the Bose factor by antisymmetrizing:χ″(q,ω)=−π[S(q,ω)−S(q,−ω)].[5]

The overall scale was determined by applying the f-sum rule [4],∫0ω*ω χ″(q,ω) dω=−πNeff(ω∗)q22m,[6]

where m is the bare electron mass and Neff=1.81×10−4 Å⁻³ is the effective carrier density derived from the optical loss function integral to ω* = 2.0 eV (23). In addition to providing an overall scale, the sum rule normalizes out systematic drifts in the beam intensity, changing beam footprint on the sample, and so on.

Random Phase Approximation Calculations.

The charge susceptibility, χ″(q,ω), and polarizability, Π″(q,ω), reported in Fig. 1 are calculated within the random phase approximation (RPA) (18). The bare polarization bubble is determined by use of the Lindhard formula using a realistic tight-binding parametrization of the BSCCO band structure (40). The charge susceptibility is then determined through Eq. 1 using the Coulomb interaction for a layered electron gas, V(q), for 2D layers separated by a constant c = 15.4 Å (41).

Acknowledgments

We thank C. M. Varma for discussions and assistance analyzing the data and J. Zaanen, N. D. Goldenfeld, and P. W. Phillips for helpful discussions. This work was supported by the Center for Emergent Superconductivity, an Energy Frontier Research Center funded by the US Department of Energy (DOE), Office of Basic Energy Sciences under Award DE-AC02-98CH10886. Crystal growth was supported by DOE Grant DE-SC0012704. P.A. acknowledges support from the EPiQS program of the Gordon and Betty Moore Foundation, Grant GBMF4542. B.U. acknowledges NSF CAREER Grant DMR-1352604. M.M. acknowledges support by the Alexander von Humboldt Foundation through the Feodor Lynen Fellowship program.

Footnotes

↵¹To whom correspondence may be addressed. Email: mmitrano{at}illinois.edu or abbamont{at}illinois.edu.
↵²Present address: Department of Physics, Massachusetts Institute of Technology, Cambridge, MA 02139.

Author contributions: P.A. designed research; M.M., A.A.H., S.V., A.K., M.S.R., S.I.R., J. Schmalian, B.U., J. Schneeloch, R.Z., G.D.G., and P.A. performed research; M.M. and A.A.H. analyzed data; J. Schneeloch, R.Z., and G.D.G. grew and characterized samples; and M.M. and P.A. wrote the paper.
The authors declare no conflict of interest.
This article is a PNAS Direct Submission.
Data deposition: The data reported in this paper have been deposited on Zenodo (available at https://zenodo.org/record/1229614#.WuDdum4vxpg).
This article contains supporting information online at www.pnas.org/lookup/suppl/doi:10.1073/pnas.1721495115/-/DCSupplemental.

Published under the PNAS license.

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1. Zhu L,
2. Chen Y,
3. Varma CM
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1. Lee J, et al.
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1. Damascelli A,
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OpenUrl CrossRef PubMed
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1. Zaanen J, et al.
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(2010) Strange metal transport realized by gauge/gravity duality. Science 329:1043–1047.
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1. Wen JS, et al.
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1. Ibach H,
2. Mills DL
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2. Randeria M,
3. Ding H,
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OpenUrl CrossRef PubMed
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1. Morawitz H, et al.
(1993) The plasmon density of states of a layered electron gas. Z Phys B Condens Matter 90:277–281.
OpenUrl

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Proceedings of the National Academy of Sciences: 115 (21)

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[106] Dobrosavljević V,

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Vegh D
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OpenUrl Abstract/FREE Full Text

[111] Faulkner T,

[112] Iqbal N,

[113] Liu H,

[114] McGreevy J,

[115] Vegh D

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OpenUrl

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[119] Ibach H,

[120] Mills DL

[121] ↵
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Randeria M,
Ding H,
Campuzano JC
(1995) Phenomenological models for the gap anisotropy of Bi₂Sr₂CaCu₂O₈ as measured by angle-resolved photoemission spectroscopy. Phys Rev B Condens Matter 52:615–622.
OpenUrl CrossRef PubMed

[122] Norman MR,

[123] Randeria M,

[124] Ding H,

[125] Campuzano JC

[126] ↵
Morawitz H, et al.
(1993) The plasmon density of states of a layered electron gas. Z Phys B Condens Matter 90:277–281.
OpenUrl

[127] Morawitz H, et al.

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Anomalous density fluctuations in a strange metal

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Abstract