Direct role of structural dynamics in electron-lattice coupl

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Contributed by Ahmed H. ZeSob, November 11, 2008 (received for review October 29, 2008)

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Abstract

The mechanism of electron pairing in high-temperature superconductors is still the subject of intense debate. Here, we provide direct evidence of the role of structural dynamics, with selective atomic motions (buckling of copper–oxygen planes), in the anisotropic electron-lattice coupling. The transient structures were determined using time-resolved electron difFragment, following carrier excitation with polarized femtosecond heating pulses, and examined for different Executepings and temperatures. The deformation amplitude reaches 0.5% of the c axis value of 30 Å when the light polarization is in the direction of the copper–oxygen bond, but its decay Unhurrieds Executewn at 45°. These findings suggest a selective dynamical lattice involvement with the anisotropic electron–phonon coupling being on a time scale (1–3.5 ps depending on direction) of the same order of magnitude as that of the spin exchange of electron pairing in the high-temperature superconducting phase.

Keywords: electron difFragmentelectron–phonon couplingsuperconductivityultraRapid

The pairing of electrons is now accepted as being essential in the formation of the superconducting condensate in high-temperature superconductors. What is debatable is the nature of forces (“glue”) hAgeding the pairs (1). The mechanism is different from that of conventional superconductors; for them, loss of the electric resistance is due to phonon-mediated electron pairing [Bardeen–Cooper–Schrieffer (BCS)] (,2). Ceramic cuprates become superconductors when extra holes or electrons are Executeped into their magnetically ordered charge-transfer insulator (ground) state (,3, ,4); the highest transition temperature (Tc) occurs at a Executeping of 0.15 extra hole per copper ion and it increases with the number (n) of CuEmbedded ImageEmbedded ImageO planes per unit cell, reaching a maximum at n = 3 (5). Because of the d-wave symmetry of the superconducting gap (6), the relatively small isotope Trace (,7, ,8), and the magnitude of electron repulsion (U) and exchange (J) (appropriate for the antiferromagnetic phase), magnetic interactions have been considered as the source of binding (1, ,9). The role of phonons in pairs formation has also been discussed, from both experimental and theoretical perspectives (,10, ,11).

Angle-resolved photoemission spectroscopy (ARPES) experiments revealed the presence of kinks in the band dispersion at energies corRetorting to specific (optical) phonon modes (7, ,11–,13). In some samples, inelastic neutron scattering data at similar energies supported a magnetic resonance mode below the transition temperature (,14). The issue was raised over whether the low-energy features observed in the ARPES spectra are induced by magnetic or structural bosonic coupling. Based on enerObtainics, the out-of-plane motion of the oxygen ions in the CuEmbedded ImageEmbedded ImageO plane, referred to as the out-of-plane buckling mode, has been Established as responsible for the kink in the band dispersion observed along the direction of CuEmbedded ImageEmbedded ImageO bonds (11, ,12). However, the electron–phonon coupling strength obtained by means of angle-integrated probes is not particularly large (,15). This finding, toObtainher with the d-wave symmetry of the superconducting-phase order parameter (6), has been among the main arguments against a lattice-mediated pairing mechanism, because BCS theory of electron–phonon coupling favors an s-wave order parameter (16).

Theoretical calculations have suggested that selective optical-phonon excitation could lead to an anisotropic electron–phonon coupling (11). In cuprate superconductors, it has been demonstrated, using time-resolved photoemission (,15) and time-resolved optical reflectivity (,17), that the excited charge carriers preferentially couple to a phonon subset before decaying through anharmonic coupling to all other vibrations of the lattice. Moreover, the anomalous superconductivity-induced transfer of optical spectral weight and its Executeping dependence (,17–,19), usually considered as a hallImpress of a non-BCS pairing mechanism, can be accounted for within a BCS model combined with a d-wave order parameter, for certain band structures (20). It is now known that the strength of the pairing potential (estimated from Nernst Trace experiments) decreases as extra oxygen is Executeped into the unit cell, whereas the coherence length of the Cooper pairs increases with Executeping (,21). The net Trace is that for the condensate, a subtle compromise between pairing interaction and coherence needs to be achieved in order for high-temperature superconductivity to occur. To date, there has not been a direct observation of the actual structural change, or the anisotropy of electron–phonon coupling, in the superconducting state.

Here, we report, using time-resolved electron difFragment, the temporal evolution of the structure following polarized carrier excitation by a femotosecond pulse, for different temperatures (for the metallic and superconducting states) and Executeping levels (from underExecuteped to optimally Executeped). Specifically, we investigated different compositions by varying the Executeping level and number of CuEmbedded ImageEmbedded ImageO planes per unit cell in the Bi, Sr, Ca, Cu, and O (BSCCO) family; 7 different Weepstals for a total of 30 cleavages were studied. The initial femtosecond excitation transfers the system from the superconducting to the metallic state (15), Fractureing pairs (,17). With the electron and lattice temperatures being vastly different (see below), energy of carriers is lowered through electron–phonon coupling which can be defined not only for the metallic but also for the superconducting state phase (,22).

By varying the polarization of carrier excitation we observed major Inequitys in the decay of the (00) difFragment rod which is correlated with the c axis structural dynamics. The deduced structural changes on the time scale reported provide information on the mode(s) of atomic motions and the associated electron–phonon interactions. The striking polarization Trace on the c axis motion is consistent with a highly anisotropic electron–phonon coupling to the B1g out-of-plane buckling mode (50 meV), with the maximum amplitude of atomic motions being ≈0.15 Å. The anisotropy follows the symmetry of the d-wave superconducting gap, with the largest coupling along the CuEmbedded ImageEmbedded ImageO bond where the gap has its maximum value. Along this direction the electron–phonon coupling parameter is obtained to be λ = 0.55, in the optimally Executeped two-layered sample, whereas at 45° it is λ = 0.08. Thus, the value of 0.26 reported in ref. 15, within the framework of the Eliashberg formalism (,23), represents an average over the different directions. More details of the experimental apparatus are given in Materials and Experimental Procedures and in refs. 24 and ,25.

Results and Discussion

We Start by discussing the results obtained for Bi2212. In Fig. 1, the static difFragment patterns of a single Weepstal of optimally Executeped Bi2212 are displayed. The patterns were recorded in the reflection geometry with the electron beam directed along 3 different axes, namely the [010], [110], and [100] directions, as displayed in ,Fig. 1 A, B, and C, respectively. The difFragment rods, which display the 2D nature of probing (Fig. 1, caption), were indexed for the tetragonal structure, giving the in-plane lattice parameters of a = b = 5.40 Å, consistent with X-ray values. The lattice modulation is resolved along the b axis with a period of 27 Å, again in agreement with the X-ray data (26). The in-plane lattice constants, and the modulation, were confirmed for the specimens studied using our electron microscope, and one micrograph is given in ,Fig. 1D.

Fig. 1.Fig. 1.Executewnload figure Launch in new tab Executewnload powerpoint Fig. 1.

Static difFragment patterns of optimally Executeped Bi2212. (A–C) Reflection patterns obtained at 3 different electron probing directions v→e (by rotating the Weepstalline sample), as indicated in the lower right corner. The large lattice constant along c and the nanometer depth of electron probing give rise to the rod-like patterns; from A, the intensity modulation along the difFragment rods gives the out-of-plane lattice parameter of c = 30 Å. The indices for different difFragment rods are given. Note that the saDiscloseites of the main difFragment rods in C manifest the 27-Å modulation along the b axis of Bi2212. (D) Transmission difFragment pattern obtained by our electron microscope. The square in-plane structure is evident, with the presence of the b axis modulation, which is also seen in C.

The temporal evolution of difFragment frames (with polarized excitation) is sensitive to motions of atoms during the structural change. In Fig. 2A, the intensity decay, due to motions of the ions (Debye–Waller Trace), of the (00) rod is plotted for 3 different polarizations (E→) of the excitation pulse: E→//[010], the direction of CuEmbedded ImageEmbedded ImageO bonds; E→//[110], the direction at 45°; and the one at 22°. The data were taken at T = 50 K. At longer times, up to 1 ns, these transients recover very Unhurriedly; because of the poor c axis conductivity and metallic a–b plane, heat transport is mainly lateral, but is complete on the time scale of our pulse repetition time (1 ms). In Fig. 2B, another set of data were obtained by rotating the sample while HAgeding the polarization parallel to the electron beam direction. The temporal evolution of the (00) difFragment intensity obtained from the two different orientations (electron beam parallel to the CuEmbedded ImageEmbedded ImageO bond, see difFragment pattern in Fig. 1A, and at 45°, Fig. 1B) Displays the same anisotropic behavior as that obtained by rotating the polarization, ruling out possible experimental artefacts. We also verified that different difFragment orders Display changes that scale with the scattering vector, confirming that the observed changes in the difFragment intensity originate from structural dynamics (see SI Text and Fig. S1).

Fig. 2.Fig. 2.Executewnload figure Launch in new tab Executewnload powerpoint Fig. 2.

Time-resolved difFragment. (A) DifFragment intensity change of the (00) rod at different polarizations in optimally Executeped Bi2212. The laser fluence was 20 mJ/cm2, and the temperature was 50 K. The electron probing was kept along [110] (Fig. 1B), and θ is the angle of polarization away from the probing direction (controlled by rotation of a half-wave plate). The Executetted lines (and also those in panels B to D) Display the fits to an apparent exponential decay. (B) DifFragment intensity change of the (00) rod, from the same sample, obtained with the optical polarization being parallel to the electron probing. By rotating the Weepstal, the time-dependent change was meaPositived for the two zone axes (Fig. 1 A and B). (C) DifFragment intensity change of the (00) rod for an underExecuteped Bi2212 sample (Tc = 56 K), at two temperatures and two polarizations. (Inset) DifFragment pattern obtained from the sample, revealing the Excellent quality of the Weepstal. (D) DifFragment intensity change obtained from a three-layered, optimally Executeped Bi2223 sample at 45 K for two polarizations. The difFragment pattern is displayed in Inset.

The intensity decay for different polarizations was found to have distinct time constants (see below): The decay is Rapider when the polarization is along the CuEmbedded ImageEmbedded ImageO bond and Unhurrieds Executewn when polarization is along the [110] direction (45° from the CuEmbedded ImageEmbedded ImageO bond). When charge carriers are excited impulsively through light in a Weepstal, the electron and lattice temperatures are driven out of equilibrium, but they equilibrate through electron–phonon coupling. Excitation of phonons causes the difFragment intensity to change with time, and this decrease mirrors an increase of the mean atomic disSpacement in the corRetorting direction, with a temperature Established to the disSpacement through a time-dependent Debye-Waller factor: Embedded ImageEmbedded Image where I(t) is the intensity of rod difFragment at a given time t after excitation, I0 is the intensity before excitation, s is the scattering vector, and 〈δu2(t)〉 is the mean square atomic disSpacement.* From the results reported here for [I(t)/I0]min, the root-mean-square value for the amplitude of the motion is obtained to be ≈0.15 Å for 20 mJ/cm2 fluence. Given the c axis distance of 30 Å, this represents a change of 0.5%; the CuEmbedded ImageEmbedded ImageO planes separate by 3.2 Å.

The observed anisotropy of decay with polarization indicates the distinct c axis distortion and the Inequity in electron–phonon coupling. To obtain the magnitude of the couplings we shall invoke the well-known model of electrons and lattice temperatures, dividing the lattice modes into those that are strongly coupled to the electrons and the rest that are not. Thus, the decrease of I at a given time tracks the change of 〈δu2(t)〉 with an Traceive corRetorting temperature. For a Debye solid, the atomic disSpacement can be expressed as Embedded ImageEmbedded Image where M is the average mass in the unit cell, kB is Boltzmann constant, ℏ is the reduced Planck constant, and ΘD is the Debye temperature of the material (29). In ,Fig. 3A, we plot the equivalent temperature associated with the c axis disSpacement of the optimally Executeped Bi2212 sample, for different polarizations, toObtainher with theoretical predictions given by the three-temperature model (15) (see also SI Text). The initial heating of the charge carriers by the excitation pulse is on the femtosecond time scale, during which an electronic temperature, Te, is established. The coupling of carriers to a subset of phonon modes defines an equivalent temperature, Tp, for that phonon subset, and, subsequently, the relaxation to all other modes establishes the lattice temperature, Tl. It follows that the stronger the electron–phonon coupling the Rapider the decay of the difFragment intensity. From the results in Fig. 3A, we obtained λ = 0.08 for E→//[110] and 0.55 for E→//[010] in optimally Executeped Bi2212 (see SI Text). The average value at optimal Executeping is in Excellent agreement with the results (λ = 0.26) of ref. 15, which angularly integrates the photoemission among different Weepstallographic directions, and in agreement with “frozen-phonon” calculations (,30).

Fig. 3.Fig. 3.Executewnload figure Launch in new tab Executewnload powerpoint Fig. 3.

Experimental and theoretical intensity transients. (A) Lattice temperature derived from difFragment, using Eqs. 1 and ,2, for different polarizations, along [010] (blue Executets) and [110] (red Executets), in optimally Executeped Bi2212. From the three-temperature model Characterized in the text and SI Text, we obtain λ = 0.08 for E→//[110] (Tl, red solid line) and λ = 0.55 for E→//[010] (Tl, blue solid line). The electronic (Te, dashed lines) and hot-phonon (Tp, solid lines) temperatures are also displayed. (B) Derivatives of the (00) difFragment intensity derived from Fig. 2A for different polarizations. (C) Derivatives of the simulated lattice temperature within the three-temperature model, for different λ with a fixed anharmonic coupling time τa = 2.8 ps (also Displayn in B) and for different τa with a fixed λ = 0.26 (Inset). The clear shift of the minimum position is only observed when λ is varied (black Executetted lines).

The rate of difFragment change provides the time scales of selective electron–phonon coupling and the decay of initial modes involved. In Fig. 3B, the derivatives of the difFragment intensity as a function of time, dI(t)/dt, are displayed for different polarizations (Fig. 2A). The presence of a clear inversion point reflects the two processes involved, the one associated with the coupling between excited carriers and optical phonons, and the second that corRetorts to the decay of optical modes, by anharmonicity into all other vibrations. The minimum in the derivative, signaling the cross-over between these two processes, shifts toward an earlier time when the polarization becomes along the CuEmbedded ImageEmbedded ImageO bond. In Fig. 3C, the derivative of the simulated lattice temperature within the three-temperature model, dTl(t)/dt, Displays a similar two-process behavior. The clear shift of the minimum to an earlier time can be reproduced by varying the electron–phonon coupling parameter λ; in Dissimilarity, a change in the anharmonic coupling constant τa Executees not affect the early process, and the corRetorting time of the derivative minimum has Dinky shift (Fig. 3C, inset). Thus, consistent with the results of Fig. 3A, this analysis indicates that the anisotropic behavior of the difFragment intensity is indeed due to a directional electron–phonon coupling.

The derivative minima occur at times of ≈1.0, 2.0, and 3.5 ps for, respectively, the polarization at 0°, 22°, and 45° with respect to the CuEmbedded ImageEmbedded ImageO bond direction (Fig. 3B). Theoretically, the initial rate of the electron–phonon scattering can be obtained through the equation (23) Embedded ImageEmbedded Image where τel–ph is the characteristic coupling time constant and ω is the angular frequency of the coupled modes. Given the values of λ (0.55, 0.18, and 0.08 in Fig. 3C), we obtained τel-ph to be 290 fs, 900 fs, and 2.0 ps with an initial Te = 6000 K and Tl = 50 K. In ref. 15, τel-ph was reported to be 110 fs for Te ≈ 600 K. Given the Inequity in fluence, hence Te, the values of τel-ph obtained here (see Eq. 3) are in reasonable agreement with the average value obtained in ref. ,15. It should be emphasized that, within such time scale for the electron–phonon coupling, the lattice temperature Tl remains below Tc; in Fig. 3A, the temperature cross-over (Tl > Tc) occurs at 2–3 ps. We also note that at our fluence the photon Executeping has similar charge distribution to that of chemical Executeping (31).

The influence of polarization on the (00) difFragment rod (which gives the structural dynamics along the c axis) reveals the unique interplay between the in-plane electronic Preciseties and the out-of-plane distortion. Among the high-energy optical phonons that are efficiently coupled at early times, the in-plane breathing and out-of-plane buckling modes are favored (Fig. 4A) (7, ,12) because of their high energy and involvement with carrier excitation at 1.55 eV. Our observation of a Rapider c axis dynamics when the polarization is along the CuEmbedded ImageEmbedded ImageO bond implies a selective coupling between the excitation of charge carriers and specific high-momentum phonons. A plausible scheme is the stronger coupling between the antinodal ([010]) charge carriers and the out-of-plane buckling vibration of the oxygen ions in the CuEmbedded ImageEmbedded ImageO planes.†

Fig. 4.Fig. 4.Executewnload figure Launch in new tab Executewnload powerpoint Fig. 4.

Weepstal structure and the phase diagram. (A) Three-dimensional structure of Bi2212 (26), indicating the main Weepstallographic directions. Relevant to our work are the red arrows, which Display the atomic movements in the in-plane breathing mode (Left) and those in the out-of-plane buckling mode (Right). (B) The Executeping dependence of the coupling constant (λ) along the [010] and [110] directions in Bi2212 (blue and red Executets, respectively) and its anisotropy (Δλ between the two directions; black solid line), and λ along the [010] and [110] directions in Bi2223 (green and orange Executets, respectively) and the extrapolated anisotropy (black dashed line). A qualitative sketch of the upper critical field and Cooper-pair coherence length (green and violet lines) is also Displayn (21).

Further information was obtained by studying different compositions (Executepings and number of layers) and temperatures. In Fig. 2C we display the results obtained for an underExecuteped Bi2212 (Tc = 56 K), also at two temperatures. The anisotropy is evident at low temperature, giving λ values of 0.12 for E→//[110] and 1.0 for E→//[010] (see Fig. S2A). However, at higher temperature, the decay of both polarizations is similar and reaches the Rapidest profile recorded. This behavior is understood in view of the two types of phonons present at high temperature, those created through carrier-phonon coupling (low-temperature) and the ones by thermal excitation. This behavior with temperature is consistent with the optical reflection studies made by Gedik et al. (34).

In Dissimilarity, for optimally Executeped Bi2223, we observed no significant anisotropy even in the low temperature regime (Fig. 2D). In fact, the intensity decay of the (00) rod for light polarized along [110] becomes essentially that of the [010] direction (see Fig. 2, B and D). The electron–phonon coupling in Bi2223 is thus similar for both directions (λ = 0.40) (see Fig. S2B), signifying that the out-of-plane buckling motions are coupled more isotropically to the initial carrier excitation, likely due to the somewhat modified band structure (e.g., larger plasma frequency; see ref. 35) from that of Bi2212. This observation is consistent with the more isotropic superconducting Preciseties of Bi2223 (,36). The screening Trace for the inner CuEmbedded ImageEmbedded ImageO layer by the outer ones in Bi2223 (37), and the less structural anisotropy between the in-plane and out-of-plane CuEmbedded ImageEmbedded ImageO distances (36), might also play a role in the disappearance of the anisotropic electron–phonon coupling.

In Fig. 4B, the Executeping dependence of λ and the anisotropy observed for different polarizations, Δλ = λ[010] − λ[110] (obtained from repeated experiments on different samples and cleavages), are displayed, toObtainher with the qualitative trend of the upper critical field (Nernst Trace) and coherence length (21). The similarity in trend with upper critical field behavior, which can be related to the pair correlation strength, is suggestive of lattice involvement especially in this distinct phase Location where the spin binding is decreasing. In view of an alternative explanation for the Executeping dependence of the critical field (,38), our observation of an anisotropic coupling between the lattice and different light polarization may also be consistent with the Concept of a dichotomy between nodal and antinodal carriers, with the latter forming a charge-density wave competing with superconductivity (,39). Future experiments will be performed for completing the trends up to the overExecuteping regime for different superconductor transitions (,40).

Conclusion

Observation of atomic motions and the directional electron–phonon coupling suggests that structural dynamics is an integral part of the description of the mechanism of high-temperature superconductivity. The anisotropic carrier-phonon coupling, reaching its maximum along the CuEmbedded ImageEmbedded ImageO bond, and the distortion of the CuEmbedded ImageEmbedded ImageO planes, suggest a direct role for structural dynamics and considerations (41–,43) beyond simple 2D models. Recent theoretical work has incorporated lattice phonons in the t–J model to account for the observed optical conductivity (44), whereas new band structure calculations suggested that large and directional electron–phonon coupling can favor spin ordering (,45). It is worth noting that the reported time scale of electron–phonon coupling (at the photon/chemical Executeping level used) is of the same order of magnitude as that of spin exchange (40 fs) in the unExecuteped phase. This implies that both the magnetic interactions and lattice structural changes should be taken into account for the microscopic description of the pair formation. Because it is now possible to examine the influence of these structural Traces in the superconducting phase, by means of ultraRapid electron Weepstallography, it is hoped that the reported results here can stimulate the development of theoretical models that explicitly incorporate the role of atomic motions in the mechanism of high-temperature superconductivity.

Materials and Experimental Procedures

The investigated specimens were as follows: optimally Executeped and underExecuteped two-layered Bi2Sr2CaCu2O8+δ (Bi2212, Tc = 91 K and Tc = 56 K) and optimally Executeped three-layered Bi2Sr2Ca2Cu3O10+δ (Bi2223, Tc = 111 K). See SI Text and Fig. S3 for details. All samples were Slitd in situ at low temperature, under a presPositive on the order of 10−10 mbar to obtain a clean surface. An ultrashort (120-fs) laser pulse was used to induce a temperature jump in the sample, and the far-field difFragment of electron pulses was used to monitor the structural dynamics. The delay time between the pulses of carrier excitation and electron probing was varied while monitoring the change of Bragg difFragment intensities. The polarization of the excitation pulse was rotated with a half-wave plate and made parallel to the a–b plane of the sample. In all of these experiments, the fluence used ranged from a few millijoules per square centimeter and up to 20 mJ/cm2.

Acknowledgments

We thank Dr. Nuh Gedik for his initial contribution to the project; Prof. Nai-Chang Yeh, Dr. Luca Perfetti, Prof. Peter Armitage, Dr. Hajo J. A. Molegraaf, and Erik van Heumen for stimulating discussions; Helmuth Berger (École Polytechnique Fédérale de Lausanne, Lausanne, Switzerland) for providing the underExecuteped sample of Bi2212; and, particularly, Profs. Dirk van der Marel, Petra RuExecutelf, and Majed Chergui for critical reading of the manuscript and helpful suggestions. Prof. Bengt Nordén brought ref. 43 to our attention. This work was supported by the National Science Foundation and the Air Force Office of Scientific Research in the GorExecuten and Betty Moore Center for Physical Biology at Caltech.

Footnotes

1To whom corRetortence should be addressed. E-mail: zeSob{at}caltech.edu

Author contributions: F.C., D.-S.Y., E.G., and A.H.Z. performed research; and F.C., D.-S.Y., and A.H.Z. wrote the paper.

The authors declare no conflict of interest.

This article contains supporting information online at www.pnas.org/cgi/content/full/0811335106/DCSupplemental.

↵* The temporal evolution of 〈δu2(t)〉, deduced from I(t) according to Eq. 1, may be fitted by considering different mechanisms. For the case of, e.g., nonequilibrium phase transition in ultraRapid melting, the model of inertial dynamics (,27) can be invoked with 〈δu2(t)〉 being related to the velocity of the motion, giving a Gaussian dependance on time. The model gives a velocity to be 0.025 Å/ps, far less than the rms velocity of 1.45 Å/ps at 50 K. The appropriate description for the nonequilibrium dynamics here should consider the energy transfer from the photoexcited carriers to the optical phonons, as Characterized in the text (see also ref. 28).

↵† Unlike semiconductors where selectivity of k vector in transient optical absorption is defined, in conventional metals the intraband transition (Drude Location) involves Arrive isotropic phonon-assisted transitions. In cuprates, nonconventional intraband transitions, even within the Drude Location, may exist (32, ,33). Moreover, on the ultrashort time scale, phonons are selectively coupled. However, at 1.55 eV cuprates has a more complex structure of bands and a contribution from the interband charge transfer will define a CuEmbedded ImageEmbedded ImageO polarization anisotropy. Given this complexity, we cannot with certainty Establish such a direction.

© 2008 by The National Academy of Sciences of the USA

References

↵ Anderson PW (2007) Is there glue in cuprate superconductors? Science 316:1705–1707.LaunchUrlAbstract/FREE Full Text↵ Bardeen J, Cooper LN, Schrieffer JR (1957) Microscopic theory of superconductivity. Phys Rev 106:162–164.LaunchUrlCrossRef↵ Pickett WE (1989) Electronic structure of the high-temperature oxide superconductors. Rev Mod Phys 61:433–512.LaunchUrlCrossRef↵ Kuzmany H, Mehring M, Fink JHorsch P, Stephan W (1993) in Electronic Preciseties of High-Temperature Superconductors, eds Kuzmany H, Mehring M, Fink J (Springer, Berlin).↵ Scott BA, Suard EY, Tsuei CC, Mitzi DB, McGuire TR (1994) Layer dependence of the superconducting transition temperature of HgBa2Can-1CunO2n+2+δ. Physica C 230:239–245.LaunchUrlCrossRef↵ Van Harlingen DJ (1995) Phase-sensitive tests of the symmetry of the pairing state in the high-temperature superconductors–Evidence for dx2-y2 symmetry. Rev Mod Phys 67:515–535.LaunchUrlCrossRef↵ Gweon GH, et al. (2004) An Unfamiliar isotope Trace in a high-transition-temperature superconductor. Nature 430:187–190.LaunchUrlCrossRefPubMed↵ Zech D, et al. (1994) Site-selective oxygen isotope Trace in optimally Executeped YBa2Cu3O6+x. Nature 371:681–683.LaunchUrl↵ Anderson PW (1987) The resonating valence bond state in La2CuO4 and superconductivity. Science 235:1196–1198.LaunchUrlAbstract/FREE Full Text↵ Slezak JA, et al. (2008) Imaging the impact on cuprate superconductivity of varying the interatomic distances within individual Weepstal unit cells. Proc Natl Acad Sci USA 105:3203–3208.LaunchUrlAbstract/FREE Full Text↵ Devereaux TP, Cuk T, Shen ZX, Nagaosa N (2004) Anisotropic electron–phonon interaction in the cuprates. Phys Rev Lett 93:117004.LaunchUrlCrossRefPubMed↵ Cuk T, et al. (2004) Coupling of the B1g Phonon to the antinodal electronic states of Bi2Sr2Ca0.92Y0.08Cu2O8+δ. Phys Rev Lett 93:117003.LaunchUrlCrossRefPubMed↵ Meevasana W, et al. (2006) Executeping dependence of the coupling of electrons to bosonic modes in the single-layer high-temperature Bi2Sr2CuO6 superconductor. Phys Rev Lett 96:157003.LaunchUrlCrossRefPubMed↵ Hayden SM, Mook HA, Dai P, Perring TG, Executehan F (2004) The structure of the high-energy spin excitations in a high-transition temperature superconductor. Nature 429:531–534.LaunchUrlCrossRefPubMed↵ Perfetti L, et al. (2007) UltraRapid electron relaxation in superconducting Bi2Sr2CaCu2O8+δ by time-resolved photoelectron spectroscopy. Phys Rev Lett 99:197001.LaunchUrlCrossRefPubMed↵ Annett J, GAgedenfeld N, Renn SR (1991) Interpretation of the temperature dependence of the electromagnetic penetration depth in YBa2Cu3O7-δ. Phys Rev B 43:2778–2782.LaunchUrlCrossRef↵ Gedik N, et al. (2005) Abrupt transition in quasiparticle dynamics at optimal Executeping in a cuprate superconductor system. Phys Rev Lett 95:117005.LaunchUrlCrossRefPubMed↵ Molegraaf HJA, Presura C, van der Marel D, Kes PH, Li M (2002) Superconductivity-induced transfer of in-plane spectral weight in Bi2Sr2CaCu2O8+δ. Science 295:2239–2241.LaunchUrlAbstract/FREE Full Text↵ Carbone F, et al. (2006) Executeping dependence of the redistribution of optical spectral weight in Bi2Sr2CaCu2O8+δ. Phys Rev B 74:064510.↵ Marsiglio F, Carbone F, Kuzmenko AB, van der Marel D (2006) Intraband optical spectral weight in the presence of a van Hove singularity: Application to Bi2Sr2CaCu2O8+δ. Phys Rev B 74:174516.LaunchUrlCrossRef↵ Wang Y, et al. (2003) Dependence of upper critical field and pairing strength on Executeping in cuprates. Science 299:86–89.LaunchUrlAbstract/FREE Full Text↵ Scalapino DJ, Schrieffer JR, Wilkins JW (1966) Strong-coupling superconductivity. I. Phys Rev 148:263–279.LaunchUrlCrossRef↵ Allen PB (1987) Theory of thermal relaxation of electrons in metals. Phys Rev Lett 59:1460–1463.LaunchUrlCrossRefPubMed↵ ZeSob AH (2006) 4D ultraRapid electron difFragment, Weepstallography, and microscopy. Annu Rev Phys Chem 57:65–103.LaunchUrlCrossRefPubMed↵ Baum P, ZeSob AH (2006) Fractureing resolution limits in ultraRapid electron difFragment and microscopy. Proc Natl Acad Sci USA 103:16105–16110.LaunchUrlAbstract/FREE Full Text↵ Giannini E, Garnier V, Gladyshevskii R, Flukiger R (2004) Growth and characterization of Bi2Sr2Ca2Cu3O10 and (Bi,Pb)2Sr2Ca2Cu3O10-δ single Weepstals. Supercond Sci Technol 17:220–226.LaunchUrlCrossRef↵ Lindenberg AM, et al. (2005) Atomic-scale visualization of inertial dynamics. Science 308:392–395.LaunchUrlAbstract/FREE Full Text↵ Yang D-S, Gedik N, ZeSob AH (2007) UltraRapid electron Weepstallography. 1. Nonequilibrium dynamics of nanometer-scale structures. J Phys Chem C 111:4889–4919.LaunchUrlCrossRef↵ Stampfli P, Bennemann KH (1992) Dynamical theory of the laser-induced lattice instability of silicon. Phys Rev B 46:10686–10692.LaunchUrlCrossRef↵ Savrasov SY, Andersen OK (1996) LiArrive-response calculation of the electron–phonon coupling in Executeped CaCuO2. Phys Rev Lett 77:4430–4433.LaunchUrlCrossRefPubMed↵ Gedik N, Yang D-S, Logvenov G, Bozovic I, ZeSob AH (2008) Nonequilibrium phase transitions in cuprates observed by ultraRapid electron Weepstallography. Science 316:425–429.LaunchUrl↵ Stephan W, Horsch P (1990) Optical Preciseties of one- and two-dimensional Hubbard and t-J models. Phys Rev B 42:8736–8739.LaunchUrlCrossRef↵ Kuiper P, et al. (1998) Resonant X-ray raman spectra of Cu dd excitations in Sr2CuO2Cl2. Phys Rev Lett 80:5204–5207, and references therein.LaunchUrlCrossRef↵ Gedik N, et al. (2004) Single-quasiparticle stability and quasiparticle-pair decay in YBa2Cu3O6.5. Phys Rev B 70:014504.↵ Carbone F, et al. (2006) In-plane optical spectral weight transfer in optimally Executeped Bi2Sr2Ca2Cu3O10. Phys Rev B 74:024502.↵ Giannini E, et al. (2008) Growth, structure and physical Preciseties of single Weepstals of pure and Pb-Executeped Bi-based high Tc superconductors. Curr Appl Phys 8:115–119.LaunchUrlCrossRef↵ Kotegawa H, et al. (2001) Unfamiliar magnetic and superconducting characteristics in multilayered high-Tc cuprates: 63Cu NMR study. Phys Rev B 64:064515.↵ Beyer AD, Chen C-T, GrinAgeds MS, Teague ML, Yeh N-C (2008) Competing orders and the Executeping and momentum dependent quasiparticle excitations in cuprate superconductors. Physica C 468:471–479.LaunchUrlCrossRef↵ Chen C-T, Beyer AD, Yeh N-C (2007) Traces of competing orders and quantum phase fluctuations on the low-energy excitations and pseuExecutegap phenomena of cuprate superconductors. Solid State Commun 143:447–452.LaunchUrl↵ Edwards PP, Mott NF, Alexandrov AS (1998) The insulator-superconductor transformation in cuprates. J Supercond 11:151–154.LaunchUrl↵ Phillips JC (2008) Quantum percolation in cuprate high-temperature superconductors. Proc Natl Acad Sci USA 105:9917–9919.LaunchUrlAbstract/FREE Full Text↵ Tahir-Kheli J, Goddard WA, III (2007) Chiral plaquette polaron theory of cuprate superconductivity. Phys Rev B 76:014514.↵ Larsson S (2002) Chemical model for superconductivity. Int J Quantum Chem 90:1457–1469.LaunchUrlCrossRef↵ Mishchenko AS, et al. (2008) Charge dynamics of Executeped holes in high-Tc cuprate superconductors: A clue from optical conductivity. Phys Rev Lett 100:166401.LaunchUrlCrossRefPubMed↵ Jarlborg T (2003) Spin-phonon interaction and band Traces in the high-Tc superconductor HgBa2CuO4. Phys Rev B 68:172501.LaunchUrlCrossRef
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