J. Phys. Soc. Jpn. 83, 061001 (2014) [8 Pages]
SPECIAL TOPICS: Advances in Physics of Strongly Correlated Electron Systems

Evidence of a Kondo Destroying Quantum Critical Point in YbRh2Si2

+ Affiliations
1Max Planck Institute for Chemical Physics of Solids, 01187 Dresden, Germany2Institute of Physics, Chinese Academy of Sciences, Beijing, China3Cavendish Laboratory, University of Cambridge, Cambridge, U.K.4Physics Institute, Goethe University, Frankfurt/Main, Germany5Max Planck Institute for Physics of Complex Systems, 01187 Dresden, Germany6Department of Physics and Astronomy, University of California Los Angeles, Los Angeles, CA 90095, U.S.A.7Department of Physics and Astronomy, Rice University, Houston, TX 77005, U.S.A.

The heavy-fermion metal YbRh2Si2 is a weak antiferromagnet below TN = 0.07 K. Application of a low magnetic field Bc = 0.06 T (⊥c) is sufficient to continuously suppress the antiferromagnetic (AF) order. Below T ≈ 10 K, the Sommerfeld coefficient of the electronic specific heat γ(T) exhibits a logarithmic divergence. At T < 0.3 K, γ(T) ∼ T−ε (ε: 0.3–0.4), while the electrical resistivity ρ(T) = ρ0 + aT0: residual resistivity). Upon extrapolating finite-T data of transport and thermodynamic quantities to T = 0, one observes (i) a vanishing of the “Fermi surface crossover” scale \(T^{*}\)(B), (ii) an abrupt jump of the initial Hall coefficient RH(B) and (iii) a violation of the Wiedemann Franz law at B = Bc, the field-induced quantum critical point (QCP). These observations are interpreted as evidence of a critical destruction of the heavy quasiparticles, i.e., propagating Kondo singlets, at the QCP of this material.

©2014 The Physical Society of Japan
1. Heavy-Fermion Quantum Criticality

Rare-earth-based intermetallic compounds with heavy-fermion (HF) phenomena (“HF metals”) are well described within the framework of the Kondo lattice.1) In contrast to other families of correlated electron materials, HF metals exhibit a clear hierarchy of relevant energy scales, i.e., spin–orbit coupling, crystal-field (CF) splitting of the localized \(4f\) shell, single-ion Kondo energy and Kondo coherence.2) Following the discovery of HF phenomena in thermodynamic and transport properties of CeAl3,3) the surprising observation of HF superconductivity in CeCu2Si24) and subsequently in a few U-based intermetallics, like UBe135) and UPt3,6) initiated intense studies in this field. In addition to superconductivity, a second “revolution” sparked by HF research led to worldwide research activities on quantum criticality.79) Antiferromagnetic (AF) quantum critical points (QCPs) in HF metals have served as prototypical settings to study non-Fermi-liquid (NFL) phenomena as well as quantum-criticality-driven novel phases, notably unconventional superconductivity.10)

In itinerant (d-electron-based) metals a spin-density-wave (SDW) QCP commonly occurs.1114) A SDW QCP may also be realized in HF metals, namely if the heavy (composite) charge carriers behave like d electrons in that they keep their integrity at the QCP. For example, the HF superconductor CeCu2Si2 exhibits a three-dimensional SDW QCP,15) whose critical fluctuations were found to drive the formation of the Cooper pairs.1618)

For CeCu2(Si0.9Ge0.1)2 two separate superconducting domes exist at different pressure ranges:19) One of them is centered at the SDW QCP at ambient pressure (\(p\)), resembling the dome of superconductivity which forms around the p-induced QCP in CePd2Si2.10) The second dome occurs at about \(p = 5\) GPa and is believed to be located close to a weak valence transition, where Cooper pairing is ascribed to nearly quantum critical valence fluctuations,20,21) as expected within a “valence-crossover” QCP scenario.22,23) The latter has been assumed to also apply22) to the p-induced AF QCP in the HF superconductor CeRhIn5.24) For this material, de Haas–van Alphen measurements25) performed in the field range \(10\leq B\leq 17\) T, i.e., not far above \(B_{\text{c2}}\approx 9\) T, revealed an abrupt reconstruction of the Fermi surface (FS) to occur at \(p_{\text{c}}\approx 2.3\) GPa, where the AF order is suppressed.26) However, the fact that this suppression of the AF order occurs smoothly26,27) rules out the valence-crossover QCP scenario,22) as this description would require the AF quantum phase transition in CeRhIn5 to be of first order. Therefore, the nature of the p-induced quantum criticality in CeRhIn5 suggests an unconventional QCP.2830) In case of a “local” QCP28,29) strong low-dimensional spin fluctuations are assumed to cause a critical destruction of the HFs, i.e., the propagating Kondo singlets. This has led to a new low-energy scale \(E^{*}(\delta)\), where δ is the control parameter. Distinct anomalies in physical properties observed at \(E^{*}(\delta)\), as discussed below, hint at an abrupt FS reconstruction at the QCP [see Fig. 1(a)]: The heavy quasiparticles exist only well below the Kondo temperature \(T_{\text{K}}\) on the paramagnetic side where they form a heavy Landau Fermi liquid below \(T_{\text{FL}}\). As here the \(4f\) states are delocalized, they contribute to a “large” FS. At an SDW QCP, \(E^{*}(\delta)\) is finite and the FS remains large [see Fig. 1(b)].

Figure 1. (Color online) Schematic view of the temperature (T)–control parameter (δ) phase diagram near antiferromagnetic (AF) quantum critical points (QCPs) of Kondo break-down (a) and spin-density-wave (b) types. \(T_{0}\) indicates the onset of local Kondo screening, once all Kondo ions have adapted the lowest lying, crystal-field derived Kramers doublet. \(E^{*}(\delta)\) is a quantum critical energy scale indicating a Fermi surface crossover from “small” to “large”. From Ref. 9.

In the following, we discuss salient NFL phenomena as well as several pieces of evidence for a sudden FS reconstruction at the AF QCP in the tetragonal HF metal YbRh2Si2.3133) This compound has been shown to behave as a prototypical Kondo lattice system,34) with a characteristic Kondo temperature \(T_{\text{K}}\approx 30\) K, referring to the lowest-lying CF-derived Kramers doublet (labeled \(T_{0}\) in Fig. 1). At \(T_{\text{K}}\), where most of the Yb3+ ions are identical, spatial coherence among the charge carriers sets in.34)

2. Non Fermi Liquid Effects in YbRh2Si2

YbRh2Si2 is a weak antiferromagnet below \(T_{\text{N}}\approx 0.07\) K,31) with a tiny ordered moment \(\mu_{\text{ord}}\approx 2\times 10^{-3}\) μ\(_{\text{B}}\)/Yb3+.35) A small magnetic field \(B_{\text{c}}\approx 0.06\) T (\(B\perp c\)) respectively 0.66 T (\(B\parallel c\)) is sufficient to suppress the AF order. This suppression occurs continuously when increasing the field through \(B_{\text{c}}\): Measurements of the magnetostriction reveal the AF phase transition to remain of second order to the lowest accessible transition temperature of 20 mK.36) From Fig. 2(a) one infers that upon cooling, the Sommerfeld coefficient of the electronic specific heat, \(\gamma(T) = C_{\text{el}}(T)/T\), is diverging at the critical field \(B = B_{\text{c}}\). In addition, below \(T\approx 0.15\) K, the electrical resistivity measured at \(B = B_{\text{c}}\) depends linearly on temperature, \(\rho(T) =\rho_{0} + aT\) [Fig. 2(b)]; \(\rho_{0}\) being the residual resistivity. Extrapolation of these T dependences of \(\gamma(T)\) and \(\rho(T)\) to zero temperature yields a NFL ground state with diverging quasiparticle mass \(m^{*}\) exactly at the field-induced QCP. At \(B\neq B_{\text{c}}\), on the other hand, YbRh2Si2 behaves as a heavy Fermi liquid, cf. Figs. 2(a) and 2(b).

Figure 2. (Color online) Low-temperature thermodynamic and transport properties near the QCP in YbRh2Si2. (a) Sommerfeld coefficient of the electronic specific heat γ vs T at three magnetic fields applied within the basal, tetragonal plane (\({\perp}c\)). At the critical field (\(B_{\text{c}}\approx 0.06\) T), one observes \(\gamma\sim T^{-\varepsilon}\) (\(\varepsilon\approx 0.3{\text{--}}0.4\)) at the lowest temperatures and \(\gamma\sim\ln\) (\(T_{0}/T\)) at elevated temperatures (\(T_{0}\approx 24\) K, i.e., close to \(T_{\text{K}}\approx 30\) K). Inset: γ vs T at zero field over an extended T range. (b) Electrical resistivity ρ vs T at the same fields as in (a). From Ref. 9.

In this context, several remarkable observations are worth mentioning:

The temperature range, within which the asymptotic \(\Delta\rho\sim T\) behavior is observed, extends to higher temperatures upon increasing disorder, e.g., from \(T< 0.15\) K for the high-quality single crystal exploited in Fig. 2 (\(\rho_{0}\approx 0.5\) µΩ cm, residual-resistivity ratio \(\mathrm{RRR}\approx 150\)) to \(T\leq 10\) K for YbRh2(Si,Ge)2 with \(\rho_{0}\approx 5\) µΩ cm.33) Here, \(\Delta\rho =\rho(T) -\rho_{0}\).

The T-dependence of \(\rho(T)\) for \(0.15 < T < 0.3\) K [see Fig. 2(b)] and at \(B = B_{\text{c}}\) is well described, within the framework of a new “critical Fermi liquid” theory, by \(\rho =\rho'_{0} + a'T^{\alpha}\), with \(\alpha = 3/4\).37)

Though the FS associated with the antiferromagnetically ordered phase of YbRh2Si2 is assumed to be small (as argued below), the low-field Fermi liquid phase appears to be particularly heavy: Its quasiparticle mass even exceeds the one in the paramagnetic Fermi liquid phase [see Fig. 2(a)]. While surprising at first sight, this observation is attributed to the dynamical Kondo screening,38) which determines thermodynamics — although the static Kondo effect is absent in the ground state.

3. Discontinuous Reconstruction of the Fermi Surface at the AF QCP in YbRh2Si2

Direct FS studies at the QCP in YbRh2Si2 are not possible. Angle-resolved photoemission spectroscopy (ARPES) below \(T = 0.1\) K with a correspondingly high energy resolution is not available at present. On the other hand, measurements of magnetic quantum oscillations require the application of magnetic fields of several T, which would fully suppress the quantum critical fluctuations in YbRh2Si2.9) Therefore, in order to investigate the evolution of the FS in the quantum critical regime of this material one has to rely on thermodynamic and transport measurements.

Isothermal studies of the magnetic field dependence of the initial Hall coefficient \(R_{\text{H}}\) (being almost identical with the normal Hall coefficient at \(T < 1\) K) revealed a large drop in \(R_{\text{H}}(B)\) at a crossover field \(B^{*}(T)\) and a substantial narrowing of this crossover upon cooling.40) Figure 3(a) displays the crossover line \(T^{*}(B)\) [\(=T(B^{*})\)], which is found to merge with both \(T_{\text{N}}(B)\) and \(T_{\text{FL}}(B)\) at \(B = B_{\text{c}}\) in the zero-temperature limit41) and has been shown36) to represent a new thermodynamic energy scale.28,29) Careful investigations of single crystals of widely differing quality showed, via various types of magnetotransport probes, that the crossover width is proportional to temperature41) [cf. Fig. 3(b)]. This implies, upon extrapolation to \(T = 0\), an abrupt finite jump of \(R_{\text{H}}(B)\) at the field-induced QCP and verifies the nature of the Kondo breakdown QCP as predicted by Si et al.28) and Coleman et al.29) In the following, we shall address the dynamical processes associated with this unique type of instability.

Figure 3. (Color online) (a) Position of the Fermi surface crossover in various magneto-transport experiments on samples of different quality in the temperature-field phase diagram of YbRh2Si2. Red horizontal bars are crossover widths, cf. (b). Dotted/dashed line marks the magnetic phase boundary \(T_{\text{N}}(B)\)/crossover to paramagnetic Landau-Fermi liquid phase \(T_{\text{FL}}(B)\). (b) Crossover width (full width at half maximum, FWHM) obtained from the same measurements exploited in (a). From Ref. 41.

4. Violation of the Wiedemann Franz Law at the AF QCP in YbRh2Si2

The Wiedemann Franz (WF) law describes the combined heat and charge transport in a metal at absolute zero temperature, where all scatterings are elastic. Defining the thermal resistivity by \(w = L_{0}T/\kappa\), where κ is the thermal conductivity and \(L_{0} = (\pi k_{\text{B}})^{2}/3e^{2}\) Sommerfeld's constant, the WF law states that (as \(T\rightarrow 0\)) the residual thermal and electrical resistivities are identical: \(\rho_{0}/w_{0} = L/L_{0} = 1\). Here, \(L =\rho\kappa/T\) denotes the Lorenz number, while \(L/L_{0}\) is called the Lorenz ratio. The WF law, one of the fundamental laws in metal physics, can in principle be violated in two very different ways: If, in addition to the electronic quasiparticles, charge-neutral fermionic excitations (“spinons”) contribute to the heat current but not to the charge current, the Lorenz ratio \(L/L_{0} > 1\), even in the zero-temperature limit. On the other hand, a breakdown of Landau's quasiparticle concept may lead to \(L/L_{0} < 1\) at \(T = 0\).

In Fig. 4 the low-T behavior of \(\rho(T)\) and \(w(T)\) is displayed for a single-crystalline YbRh2Si2 sample of medium quality (\(\mathrm{RRR}\approx 40\)) at several different values of the control parameter, magnetic field B.42) For the highest applied fields of 0.6 T [Fig. 4(i)] and 1 T [Fig. 4(j)], both \(\rho(T)\) and \(w(T)\) show a very strong \(T^{2}\) dependence at sufficiently low temperature, characteristic of a heavy Fermi liquid phase. Extrapolating these results to \(T = 0\), one recognizes \(w_{0} =\rho_{0}\) within the experimental uncertainty; i.o.w., the WF law holds even in case of such an extremely heavy Landau Fermi liquid phase.

Figure 4. (Color online) Thermal resistivity \(w(T) = L_{0}T/\kappa(T)\) (red) and electrical resistivity \(\rho(T)\) (blue) below \(T = 0.5\) K for \(B = 0\) (a), 0.02 (b), 0.06 (c), 0.08 (d), 0.1 (e), 0.2 (f), 0.3 (g), 0.4 (h), 0.6 (i), and 1 T (j), \(B\perp c\). Arrows indicate crossover to Fermi liquid (\(\rho -\rho_{0} = AT^{2}\)) behavior. Representative error bars are shown for a few selected temperatures. Dashed lines in (a)–(c) indicate linear regimes used for extrapolation to \(T = 0\). From Ref. 42.

In contrast, at \(B = 0\) both the electrical and thermal resistivities exhibit a linear temperature dependence above, respectively, \(T_{\text{N}} = 0.07\) K and \(T\approx 0.12\) K, where \(w(T)\) starts to drop [see Fig. 4(a)]. Below the Néel temperature, one finds \(\rho =\rho_{0} + AT^{2}\) with a huge value of the coefficient A. At the lowest accessible temperature of ≈25 mK the thermal resistivity is clearly smaller than its electrical counterpart: \(w <\rho\). This proves that, in addition to the electronic ones, another species of heat carriers is present at finite temperatures. These are the acoustic AF magnons, as identified with the aid of low-T specific heat results, see Fig. 5:33) The magnon specific heat obeys \(C_{\text{m}}\sim T^{3}\) below \(T\approx 0.05\) K, which implies a magnon thermal conductivity \(\kappa\sim T^{3}\) at sufficiently low temperatures, too. At \(T = 0\), the heat current is carried exclusively by the electronic quasiparticles. Because of the Fermi liquid phase, the WF law must hold in the antiferromagnetically ordered state (\(w_{0} =\rho_{0}\)). Unfortunately, this cannot be observed directly as the electronic heat transport is fully masked by the bosonic one, due to magnons below \(T_{\text{N}} = 0.07\) K and due to short-lived magnon excitations (“paramagnons”) in the temperature window \(T_{\text{N}} < T < 0.12\) K at \(B = 0\). At finite \(B < B_{\text{c}}\) an analogous behavior is observed [Fig. 4(b), \(B = 0.02\) T]. This paramagnon contribution is also visible below \(T\approx 0.07\) K at \(B\approx B_{\text{c}}\) [Fig. 4(c)], but becomes suppressed at sufficiently high magnetic fields, \(B\geq 0.2\) T [Figs. 4(f)–4(j)].

Figure 5. (Color online) Specific heat of YbRh2Si2 as \(\Delta C/T\) vs \(T^{2}\). \(\Delta C(T) = C(T) - C_{\text{ph}}(T) - C_{\text{Q}}(T)\), where \(C_{\text{ph}}\) (\(C_{\text{Q}}\)) denotes the phonon (nuclear-quadrupole) contribution. Red line indicates a \(T^{3}\) contribution to \(\Delta C(T)\) below \(T\approx 0.05\) K. From Ref. 33.

The values of the residual electrical and electronic thermal resistivities at \(B = B_{\text{c}}\), \(\rho_{0}\) and \(w_{0}\), are obtained by extrapolating the NFL-type linear-in-T dependences of \(\rho(T)\) and \(w(T)\) to zero temperature, cf. Supplementary Information of Ref. 42. Such an extrapolation is necessary because of the influence of the above-mentioned paramagnons. It yields \(w_{0} >\rho_{0}\) or \(L/L_{0} < 1\), i.e., a violation of the WF law, exactly at the QCP.

Very similar experimental data have recently been reported by three groups,4345) who studied YbRh2Si2 single crystals of considerably higher quality (\(\mathrm{RRR}\gtrsim 100\)) compared to our sample. As is evident from Refs. 4345, the paramagnon heat transport in cleaner samples appears to persist at higher fields.46) This, along with their limitation in applying large enough magnetic fields (compared to \(B_{\text{c}}\) of the respective sample orientation), prevented the authors of Refs. 43 and 44 to observe both the field-induced suppression of the bosonic contribution to the heat transport and the validity of the WF law in the paramagnetic phase. Therefore, they attribute the downturn in \(w(T)\) from the linear-in-T behavior seen at \(B = B_{\text{c}}\) to the electronic heat carriers and claim the WF law to hold at the field-induced QCP in YbRh2Si2. In contrast, more recent measurements to lower temperatures and higher fields45) confirm the existence of paramagnon excitations and their contribution to the heat transport.

In order to support our conclusion that the WF law is indeed violated as \(T\rightarrow 0\) at \(B = B_{\text{c}}\), we show in Fig. 6 the isothermal field dependence \(L(B)/L_{0}\) for \(0.1\leq T\leq 0.4\) K. Data at lower temperatures have been ignored because of the interfering bosonic contribution in the low-field range as discussed above. This means that all \(L(B)/L_{0}\) data in Fig. 6 are representative of purely electronic transport. Except for the results taken at \(T = 0.1\) K and the highest fields of 0.6 and 1 T which, within the error bars, are close to the “WF value” \(L/L_{0} = 1\), all Lorenz ratios are clearly smaller than 1. This indicates that the electronic heat carriers are subject to dominating inelastic scatterings, i.e., from both AF spin fluctuations and electronic charge carriers. At zero temperature these scatterings are frozen out, which is in accordance with the validity of the WF law in a Fermi liquid with sharp FS, e.g., at both \(B < B_{\text{c}}\) and \(B > B_{\text{c}}\) for YbRh2Si2.

Figure 6. (Color online) Isothermal field scans of the Lorenz ratio \(L(B)/L_{0}\) at varying temperatures \(0.1\leq T < 0.5\) K. From Refs. 42 and 47. Inset: Data from isothermal field scans of the thermal conductivity and electrical resistivity at \(T = 0.49\) K and \(B\leq 12\) T. From Ref. 47.

In the quantum critical regime, where the FS is fluctuating, the quasiparticle weights taken at the respective small and large values of the Fermi wave vector satisfy dynamical, \(\omega/T\), scaling and smoothly vanish exactly at the QCP,42) cf. Fig. 7. This warrants the critical FS fluctuations to exist in the whole temperature range of quantum critical behavior, \(0\leq T\lesssim 1\) K. They represent a novel type of quantum critical fluctuations, i.e., they are fermionic in origin and operate as additional inelastic scatterers for the electronic quasiparticles. These FS fluctuations give rise to the distinct minimum in the \(L(B)/L_{0}\) isotherms close to \(T^{*}(B)\) (Fig. 6), which highlights an intimate relationship between those additional inelastic scatterings and the Fermi surface crossover.

Figure 7. (Color online) Collapse of the quasiparticle weights across the local QCP. \(Z_{\text{L}}\) and \(Z_{\text{S}}\) are the quasiparticle weights for the “small” (left inset) and “large” (right inset) Fermi surfaces, respectively. At the QCP, the quasiparticles are critical on both the small and the large Fermi surfaces. From Ref. 42.

Recent results of isothermal measurements of \(\kappa(B)\) and \(\rho(B)\), performed on a high-quality YbRh2Si2 single crystal (\(\mathrm{RRR}\approx 150\)) at \(T = 0.49\) K47) fit well to those obtained from the T-scans on our medium-quality sample with \(\mathrm{RRR}\approx 40\), cf. Fig. 6. This proves that the minimum in the \(L(B)/L_{0}\) isotherms is a robust feature which, like the Hall crossover, becomes considerably narrower upon cooling (Fig. 6). As a consequence of the \(\omega/T\) scaling, the additional electronic inelastic scatterings extend to \(\omega = 0\) exactly at the QCP. This provides a very natural explanation for our main result that \(L(T\rightarrow 0)/L_{0} < 1\) at \(B = B_{\text{c}}\) and \(L(T\rightarrow 0)/L_{0} = 1\) at \(B\neq B_{\text{c}}\).

The fact that we find a reduction of the Lorenz ratio by “only” 10% is in full accord with the generalized quasiparticle–quasiparticle nature of the underlying scatterings. Though many-body in origin they include a finite moderate fraction of small-angle-scattering processes — in analogy to the electron–electron scatterings in simple metals.48)

The data presented in Fig. 8 lend further support to our conclusion of the WF law being violated at the QCP in YbRh2Si2: The electrical resistivity \(\rho(T)\), measured by S. Lausberg on a medium-quality single crystal similar to the one used for our study of the heat conductivity, clearly displays that the sample is heated up only in the vicinity of \(B_{\text{c}} = 0.059\) T, namely, if an appropriately large current is applied at low temperatures. Obviously, an extra Joule's heat is generated here which, despite of the additional bosonic heat carriers, cannot be properly lead away. Very likely, this extra heat results from the presence of particularly strong inelastic scatterings, i.e., those discussed before. Some heating effect is still visible at \(B = 0.06\) T even when a rather low current is injected into the sample (see black trace). Upon proper extrapolation of these low-current data from the regime where \(\Delta\rho\sim T\) to \(T = 0\), the residual resistivity at \(B = 0.06\) T is found to be almost identical to the \(\rho_{0}\) values extrapolated for both \(B = 0.1\) and 0.2 T. As a result, \(\rho_{0}(B)\) is found to jump abruptly from a larger to smaller value upon raising the field through \(B_{\text{c}}\), manifesting an abrupt increase in the charge carrier concentration as already inferred from the Hall measurements discussed in Sect. 3.40,41,49)

Figure 8. (Color online) Temperature dependence of the electrical resistivity below \(T = 0.1\) K with two different excitation currents (black and red traces, respectively) at several magnetic fields. Where black and red traces overlap, the red ones are extrapolated (in green) to \(T = 0\) assuming a \(\Delta\rho\sim T^{2}\) dependence. The splitting between red and black traces close to the critical field, \(B_{\text{c}} = 0.059\) T, below \(T = 0.07\) K (marked by arrows) illustrates a heating of the sample under the applied larger current. This illustrates the violation of the Wiedemann Franz law at the QCP in YbRh2Si2. Very recent resistivity measurements on an YbRh2Si2 single crystal of similar quality by S. Hamann with \(j\perp B\parallel c\) reveal a similar heating effect at \(B = 0.6\) T, which is absent at \(B = 0\), 2, and 4 T, respectively. For \(B\perp c\), a sample heating below \(T = 0.06\) K is still visible at \(B = 0.06\) T under the smaller current, cf. extrapolated dashed straight line. Horizontal blue hatching displays an almost field-independent residual (\(T\rightarrow 0\)) resistivity in the paramagnetic regime. The weak field dependence of \(\rho_{0}\) inside the antiferromagnetic phase41) is masked by the width of the grey hatching. The difference between the hatched horizontal regions indicates an abrupt decrease in \(\rho_{0}(B)\) upon increasing the field through \(B_{\text{c}}\). This illustrates a corresponding abrupt increase in the charge-carrier concentration at \(T = 0\).

Recently, \(L(B)/L_{0}\) was also determined for the HF metal YbAgGe.50) When the results taken at \(B = 4.5\) T are extrapolated to \(T = 0\), where a bi-quantum critical point is anticipated,51) \(L_{\text{el}}/L_{0}\approx 0.92\) is obtained. Thus, for YbAgGe this fundamental type of violation of the WF law seems to be clearly demonstrated, too.52)

5. Perspective

In this paper, we have presented and discussed three pieces of evidence for a field-induced Kondo destroying AF QCP in YbRh2Si2. Upon reliably extrapolating our data taken at finite temperature to \(T = 0\), we recognize exactly at \(B = B_{\text{c}}\): (i) a merging of the quantum-critical energy scale \(T^{*}(B)\) with the magnetic phase boundary \(T_{\text{N}}(B)\) and the crossover line \(T_{\text{FL}}(B)\), (ii) an abrupt jump of the initial Hall coefficient \(R_{\text{H}}(B)\) and (iii) a violation of the WF law. While the first result locates the Kondo breakdown in the phase diagram and the second one quantifies the strength of this phenomenon, the latter result illustrates the dynamical processes, causing the apparent breakup of the Kondo singlets. Future research will focus on studies of this Mott-type instability in the absence of any interfering magnetism as expected for, e.g., Yb(Rh\(_{1-x}\)Irx)2Si2 with \(x\gtrsim 0.1\).57)

Another promising area of future investigations concerns the occurrence of a ferromagnetic QCP in HF metals, like YbNi4(P\(_{1-x}\)Asx)2, \(x\approx 0.1\).58) This type of instability does apparently not exist in itinerant (d-electron-based) metallic materials.59) On the other hand, it was shown60) that for Kondo lattice systems the Kondo effect can be fully suppressed inside a ferromagnetically ordered phase. It has yet to be explored, whether in YbNi4(P0.9As0.1)2 the breakdown of the Kondo effect coincides with the ferromagnetic QCP, in analogy to the observation in the weak antiferromagnet YbRh2Si2.61)


Valuable conversations with E. Bauer, S. Bühler-Paschen, P. Coleman, R. Daou, H. Fukuyama, S. Hartmann, K. Kanoda, J.-Ph. Reid, J. Schmalian, L. Taillefer, H. von Löhneysen, P. Wölfle, and G. Zwicknagl are gratefully acknowledged. The work performed at the MPI for Chemical Physics of Solids was partly supported by the DFG under the auspices of FOR 960 “Quantum Phase Transitions”. The work at Rice University was in part supported by the NSF Grant No. DMR-1309531 and the Robert A. Welch Grant No. C-1411.


  • 1 S. Doniach, Physica B+C 91, 231 (1977). 10.1016/0378-4363(77)90190-5 CrossrefGoogle Scholar
  • 2 N. Grewe and F. Steglich, in Handbook on the Physics and Chemistry of Rare Earths, ed. K. A. Gschneidner and J. L. Eyring (Elsevier, Amsterdam, 1991) Vol. 14, p. 343. CrossrefGoogle Scholar
  • 3 K. Andres, J. E. Graebner, and H. R. Ott, Phys. Rev. Lett. 35, 1779 (1975). 10.1103/PhysRevLett.35.1779 CrossrefGoogle Scholar
  • 4 F. Steglich, J. Aarts, C. D. Bredl, W. Lieke, D. Meschede, W. Franz, and H. Schäfer, Phys. Rev. Lett. 43, 1892 (1979). 10.1103/PhysRevLett.43.1892 CrossrefGoogle Scholar
  • 5 H. R. Ott, H. Rudigier, Z. Fisk, and J. L. Smith, Phys. Rev. Lett. 50, 1595 (1983). 10.1103/PhysRevLett.50.1595 CrossrefGoogle Scholar
  • 6 G. R. Stewart, Z. Fisk, J. O. Willis, and J. L. Smith, Phys. Rev. Lett. 52, 679 (1984). 10.1103/PhysRevLett.52.679 CrossrefGoogle Scholar
  • 7 G. R. Stewart, Rev. Mod. Phys. 73, 797 (2001); 10.1103/RevModPhys.73.797 Crossref;, Google ScholarG. R. Stewart, Rev. Mod. Phys. 78, 743 (2006). 10.1103/RevModPhys.78.743 CrossrefGoogle Scholar
  • 8 H. von Löhneysen, A. Rosch, M. Vojta, and P. Wölfle, Rev. Mod. Phys. 79, 1015 (2007). 10.1103/RevModPhys.79.1015 CrossrefGoogle Scholar
  • 9 P. Gegenwart, Q. Si, and F. Steglich, Nat. Phys. 4, 186 (2008). 10.1038/nphys892 CrossrefGoogle Scholar
  • 10 N. D. Mathur, F. M. Grosche, S. R. Julian, I. R. Walker, D. M. Freye, R. K. W. Haselwimmer, and G. G. Lonzarich, Nature 394, 39 (1998). 10.1038/27838 CrossrefGoogle Scholar
  • 11 J. A. Hertz, Phys. Rev. B 14, 1165 (1976). 10.1103/PhysRevB.14.1165 CrossrefGoogle Scholar
  • 12 T. Moriya, Spin Fluctuations in Itinerant Electron Magnetism (Springer, Berlin, 1985). CrossrefGoogle Scholar
  • 13 A. J. Millis, Phys. Rev. B 48, 7183 (1993). 10.1103/PhysRevB.48.7183 CrossrefGoogle Scholar
  • 14 M. A. Continentino, G. M. Japiassu, and A. Troper, Phys. Rev. B 39, 9734(R) (1989). 10.1103/PhysRevB.39.9734 CrossrefGoogle Scholar
  • 15 J. Arndt, O. Stockert, K. Schmalzl, E. Faulhaber, H. S. Jeevan, C. Geibel, W. Schmidt, M. Loewenhaupt, and F. Steglich, Phys. Rev. Lett. 106, 246401 (2011). 10.1103/PhysRevLett.106.246401 CrossrefGoogle Scholar
  • 16 O. Stockert, J. Arndt, E. Faulhaber, C. Geibel, H. S. Jeevan, S. Kirchner, M. Loewenhaupt, K. Schmalzl, W. Schmidt, Q. Si, and F. Steglich, Nat. Phys. 7, 119 (2011). 10.1038/nphys1852 CrossrefGoogle Scholar
  • 17 O. Stockert, S. Kirchner, F. Steglich, and Q. Si, J. Phys. Soc. Jpn. 81, 011001 (2012). 10.1143/JPSJ.81.011001 LinkGoogle Scholar
  •   (18 ) The exchange-energy saving, extracted from the difference between the dynamical susceptibilities of the normal and superconducting states, largely exceeds the superconducting condensation energy (by a factor of about 20). This has been interpreted in terms of quantum critical fluctuations beyond the SDW description at intermediate energies and temperatures.16,17) Google Scholar
  • 19 H. Q. Yuan, F. M. Grosche, M. Deppe, C. Geibel, G. Sparn, and F. Steglich, Science 302, 2104 (2003). 10.1126/science.1091648 CrossrefGoogle Scholar
  • 20 K. Miyake, O. Narikiyo, and Y. Onishi, Physica B 259–261, 676 (1999); 10.1016/S0921-4526(98)00754-6 Crossref;, Google ScholarY. Onishi and K. Miyake, J. Phys. Soc. Jpn. 69, 3955 (2000); 10.1143/JPSJ.69.3955 Link;, Google ScholarA. Holmes, D. Jaccard, and K. Miyake, Phys. Rev. B 69, 024508 (2004). 10.1103/PhysRevB.69.024508 CrossrefGoogle Scholar
  • 21 P. Monthoux and G. G. Lonzarich, Phys. Rev. B 69, 064517 (2004). 10.1103/PhysRevB.69.064517 CrossrefGoogle Scholar
  • 22 S. Watanabe and K. Miyake, J. Phys. Soc. Jpn. 82, 083704 (2013). 10.7566/JPSJ.82.083704 LinkGoogle Scholar
  • 23 The interpretation given for CeCu2Si2 in Refs. 20 and 21 is questioned by L. V. Pourovskii, P. Hansmann, M. Ferrero, and A. Georges, arXiv:1305.5204v1. Google Scholar
  • 24 H. Hegger, C. Petrovic, E. G. Moshopoulou, M. F. Hundley, J. L. Sarrao, Z. Fisk, and J. D. Thompson, Phys. Rev. Lett. 84, 4986 (2000). 10.1103/PhysRevLett.84.4986 CrossrefGoogle Scholar
  • 25 H. Shishido, R. Settai, H. Harima, and Y. Ōnuki, J. Phys. Soc. Jpn. 74, 1103 (2005). 10.1143/JPSJ.74.1103 LinkGoogle Scholar
  • 26 T. Park, F. Ronning, H. Q. Yuan, M. B. Salamon, R. Movshovich, J. L. Sarrao, and J. D. Thompson, Nature 440, 65 (2006). 10.1038/nature04571 CrossrefGoogle Scholar
  • 27 G. Knebel, D. Aoki, D. Braithwaite, B. Salce, and J. Flouquet, Phys. Rev. B 74, 020501(R) (2006). 10.1103/PhysRevB.74.020501 CrossrefGoogle Scholar
  • 28 Q. Si, S. Rabello, K. Ingersent, and J. L. Smith, Nature 413, 804 (2001). 10.1038/35101507 CrossrefGoogle Scholar
  • 29 P. Coleman, C. Pépin, Q. Si, and R. Ramazashvili, J. Phys.: Condens. Matter 13, R723 (2001). 10.1088/0953-8984/13/35/202 CrossrefGoogle Scholar
  • 30 T. Senthil, M. Vojta, and S. Sachdev, Phys. Rev. B 69, 035111 (2004). 10.1103/PhysRevB.69.035111 CrossrefGoogle Scholar
  • 31 O. Trovarelli, C. Geibel, S. Mederle, C. Langhammer, F. M. Grosche, P. Gegenwart, M. Lang, G. Sparn, and F. Steglich, Phys. Rev. Lett. 85, 626 (2000). 10.1103/PhysRevLett.85.626 CrossrefGoogle Scholar
  • 32 P. Gegenwart, J. Custers, C. Geibel, K. Neumaier, T. Tayama, K. Tenya, O. Trovarelli, and F. Steglich, Phys. Rev. Lett. 89, 056402 (2002). 10.1103/PhysRevLett.89.056402 CrossrefGoogle Scholar
  • 33 J. Custers, P. Gegenwart, H. Wilhelm, K. Neumaier, Y. Tokiwa, O. Trovarelli, C. Geibel, F. Steglich, C. Pépin, and P. Coleman, Nature 424, 524 (2003). 10.1038/nature01774 CrossrefGoogle Scholar
  • 34 S. Ernst, S. Kirchner, C. Krellner, C. Geibel, G. Zwicknagl, F. Steglich, and S. Wirth, Nature 474, 362 (2011). 10.1038/nature10148 CrossrefGoogle Scholar
  • 35 K. Ishida, D. E. MacLaughlin, B.-L. Young, K. Okamoto, Y. Kawasaki, Y. Kitaoka, G. J. Nieuwenhuys, R. H. Heffner, O. O. Bernal, W. Higemoto, A. Koda, R. Kadono, O. Trovarelli, C. Geibel, and F. Steglich, Phys. Rev. B 68, 184401 (2003). 10.1103/PhysRevB.68.184401 CrossrefGoogle Scholar
  • 36 P. Gegenwart, T. Westerkamp, C. Krellner, Y. Tokiwa, S. Paschen, C. Geibel, F. Steglich, E. Abrahams, and Q. Si, Science 315, 969 (2007). 10.1126/science.1136020 CrossrefGoogle Scholar
  • 37 P. Wölfle and E. Abrahams, Phys. Rev. B 84, 041101(R) (2011). 10.1103/PhysRevB.84.041101 CrossrefGoogle Scholar
  • 38 J.-X. Zhu, D. R. Grempel, and Q. Si, Phys. Rev. Lett. 91, 156404 (2003). For a recent review on this issue, see Sect. 3.2 of Ref. 39. 10.1103/PhysRevLett.91.156404 CrossrefGoogle Scholar
  • 39 Q. Si and S. Paschen, Phys. Status Solidi B 250, 425 (2013). 10.1002/pssb.201300005 CrossrefGoogle Scholar
  • 40 S. Paschen, T. Lühmann, S. Wirth, P. Gegenwart, O. Trovarelli, C. Geibel, F. Steglich, P. Coleman, and Q. Si, Nature 432, 881 (2004). 10.1038/nature03129 CrossrefGoogle Scholar
  • 41 S. Friedemann, N. Oeschler, S. Wirth, C. Krellner, C. Geibel, F. Steglich, S. Paschen, S. Kirchner, and Q. Si, Proc. Natl. Acad. Sci. U.S.A. 107, 14547 (2010). 10.1073/pnas.1009202107 CrossrefGoogle Scholar
  • 42 H. Pfau, S. Hartmann, U. Stockert, P. Sun, S. Lausberg, M. Brando, S. Friedemann, C. Krellner, C. Geibel, S. Wirth, S. Kirchner, E. Abrahams, Q. Si, and F. Steglich, Nature 484, 493 (2012). 10.1038/nature11072 CrossrefGoogle Scholar
  • 43 Y. Machida, K. Tomokuni, K. Izawa, G. Lapertot, G. Knebel, J.-P. Brison, and J. Flouquet, Phys. Rev. Lett. 110, 236402 (2013). 10.1103/PhysRevLett.110.236402 CrossrefGoogle Scholar
  • 44 J.-Ph. Reid, M. A. Tanatar, R. Daou, R. Hu, C. Petrovic, and L. Taillefer, Phys. Rev. B 89, 045130 (2014).10.1103/PhysRevB.89.045130 Google Scholar
  • 45 A. Pourret, D. Aoki, M. Boukahil, J.-P. Brison, W. Knafo, G. Knebel, S. Raymond, M. Taupin, Y. Ōnuki, and J. Flouquet, arXiv:1311.1239. Google Scholar
  •   (46 ) For example, compare our results shown in Fig. 4(f) with those in Fig. 2(d)44) taken at B = 0.2 T, the largest field applied for B ⊥ c in Ref. 44. While for our medium-quality sample (RRR = 40), a downturn in w(T) cannot be resolved anymore, it is still visible for the crystal with higher quality (RRR ≥ 100) studied in Ref. 44. The suppression of this downturn by higher magnetic fields has recently been observed for such a clean sample.45) Google Scholar
  • 47 H. Pfau, R. Daou, S. Lausberg, H. R. Naren, M. Brando, S. Friedemann, S. Wirth, T. Westerkamp, U. Stockert, P. Gegenwart, C. Krellner, C. Geibel, G. Zwicknagl, and F. Steglich, Phys. Rev. Lett. 110, 256403 (2013). 10.1103/PhysRevLett.110.256403 CrossrefGoogle Scholar
  • 48 J. M. Ziman, Electrons and Phonons (Oxford University Press, Oxford, U.K., 1960). Google Scholar
  • 49 S. Friedemann, S. Wirth, N. Oeschler, C. Krellner, C. Geibel, F. Steglich, S. MaQuilon, Z. Fisk, S. Paschen, and G. Zwicknagl, Phys. Rev. B 82, 035103 (2010). 10.1103/PhysRevB.82.035103 CrossrefGoogle Scholar
  • 50 J. K. Dong, Y. Tokiwa, S. L. Bud’ko, P. C. Canfield, and P. Gegenwart, Phys. Rev. Lett. 110, 176402 (2013). 10.1103/PhysRevLett.110.176402 CrossrefGoogle Scholar
  • 51 Y. Tokiwa, M. Garst, P. Gegenwart, S. L. Bud’ko, and P. C. Canfield, Phys. Rev. Lett. 111, 116401 (2013).10.1103/PhysRevLett.111.116401 Google Scholar
  •   (52 ) For the tetragonal, quasi-two-dimensional HF metal CeCoIn5, for which an AF QCP is suspected at \(B \approx 4 \,\text{T} < B_{\text{c2}}(0)\)53) but not identified, the Lorenz ratio L/L0 was extrapolated to about 0.8 as T → 0 for c-axis transport at \(B \approx B_{\text{c2}}(0) \approx 5\,\text{T}\), while it approaches L/L0 = 1 for in-plane transport.54) This finding was discussed in terms of putative strongly anisotropic quantum critical spin fluctuations although, in the zero-temperature limit, spin fluctuations are unapt to raise w0 relative to ρ0.55) Subsequently, these results were consistently explained within the framework of quasi-two-dimensional transport.56) Google Scholar
  • 53 S. Zaum, K. Grube, R. Schäfer, E. D. Bauer, J. D. Thompson, and H. von Löhneysen, Phys. Rev. Lett. 106, 087003 (2011). 10.1103/PhysRevLett.106.087003 CrossrefGoogle Scholar
  • 54 M. A. Tanatar, J. Paglione, C. Petrovic, and L. Taillefer, Science 316, 1320 (2007). 10.1126/science.1140762 CrossrefGoogle Scholar
  • 55 See, e.g., R. P. Smith, M. Sutherland, G. G. Lonzarich, S. S. Saxena, N. Kimura, S. Takashima, M. Nohara, and H. Takagi, Nature 455, 1220 (2008). 10.1038/nature07401 CrossrefGoogle Scholar
  • 56 M. F. Smith and R. H. McKenzie, Phys. Rev. Lett. 101, 266403 (2008). 10.1103/PhysRevLett.101.266403 CrossrefGoogle Scholar
  • 57 S. Friedemann, T. Westerkamp, M. Brando, N. Oeschler, S. Wirth, P. Gegenwart, C. Krellner, C. Geibel, and F. Steglich, Nat. Phys. 5, 465 (2009). 10.1038/nphys1299 CrossrefGoogle Scholar
  • 58 A. Steppke, R. Küchler, S. Lausberg, E. Lengyel, L. Steinke, R. Borth, T. Lühmann, C. Krellner, M. Nicklas, C. Geibel, F. Steglich, and M. Brando, Science 339, 933 (2013). 10.1126/science.1230583 CrossrefGoogle Scholar
  • 59 D. Belitz, T. Kirkpatrick, and T. Vojta, Phys. Rev. Lett. 82, 4707 (1999). 10.1103/PhysRevLett.82.4707 CrossrefGoogle Scholar
  • 60 S. J. Yamamoto and Q. Si, Proc. Natl. Acad. Sci. U.S.A. 107, 15704 (2010). 10.1073/pnas.1009498107 CrossrefGoogle Scholar
  • 61 After submission of this manuscript, we became aware of a related theoretical publication by R. Mahajan, M. Barkeshli, and S. A. Hartnoll, Phys. Rev. B 88, 125107 (2013). 10.1103/PhysRevB.88.125107 CrossrefGoogle Scholar

Author Biographies

Frank Steglich was born in Dresden, Germany. He got his Diploma (1966) and Doctoral Degree (1969) from the University of Göttingen as well as his habilitation (1976) from the University of Köln. He was a Professor of Physics at the Technical University of Darmstadt from 1978 to 1998. In 1996 he became the Founding Director of the Max Planck Institute for Chemical Physics of Solids in Dresden. His research has been devoted to highly disordered, magnetic and superconducting as well as thermoelectric materials. Following his 1979 discovery of heavy-fermion superconductivity the main focus of his activities has been on the physics of strongly correlated electron systems.

Heike Pfau was born in Frankfurt (Oder), Germany in 1984. She obtained her Diploma in Physics from Technical University of Dresden. She has been a doctoral student at the Max Planck Institute for Chemical Physics of Solids since 2010. Her research is focusing on thermal transport in strongly correlated electron systems with emphasis on Kondo physics, quantum criticality and superconductivity.

Stefan Lausberg was born in Schwelm, Germany, in 1979. He obtained his Diploma in Physics at the University of Heidelberg, Germany, in 2008 and his PhD at the Technical University of Dresden, Germany, in 2013. He was PhD student and postdoc at the Max Planck Institute for Chemical Physics of Solids in Dresden till 2014. Currently, he is working for Oerlikon Leybold Vacuum GmbH in Cologne, Germany. He has worked on quantum phase transitions in strongly correlated electron systems, in particular in heavy-fermion systems.

Sandra Hamann was born in Dresden, Germany, in 1989. She obtained her Diploma in Physics at the Technical University of Dresden in 2013. Currently, she is PhD student at the Max Planck Institute for Chemical Physics of Solids in Dresden, working on quantum phase transitions in strongly correlated electron systems.

Peijie Sun was born in Henan Province, China in 1976. He obtained his M. Sc. degree in 2002 and Ph. D. in 2005 from Toyama University, Japan. He was a postdoctoral fellow in Iwate University (2005–2007) and Max Planck Institute for Chemical Physics of Solids (2007–2012). Since 2012, he has been a professor at the Institute of Physics, Chinese Academy of Sciences in Beijing. His research focuses on the physics of heavy fermions, correlated semiconductors, and particularly on electrical, thermal and thermoelectric transport properties at very low temperatures.

Ulrike Stockert née Köhler was born in Dresden, Germany (1977). She obtained her Diploma from Leipzig University (2003) and her Ph. D. degree from Technical University Dresden (2008). She worked as a research assistant at MPI for Chemical Physics of Solids, Dresden (2007–2008) and at the Leibniz Institute for Solid State and Materials Research, Dresden (2008–2010). Since 2010 she is a research associate at MPI for Chemical Physics of Solids. Her main research focus lies on the thermoelectric transport properties of correlated compounds including the influence of magnetic fields (Nernst effect, angular dependence). For a while she has also worked on magnetic and superconducting properties of FeAs-based compounds.

Manuel Brando was born in Macerata, Italy, in 1971. He obtained his Graduation in Physics at the University of Camerino, Italy, in 1997 and his PhD at the University of Augsburg, Germany, in 2001. He was teacher in physics at the Liceo Scientifico “G. Leopardi” in Recanati, Italy (2001–2004), research associate at the Royal Holloway University of London, UK (2004–2006), research associate at the Max Planck Institute for Chemical Physics of Solids in Dresden, Germany (2006–2008). Since 2008 he is group leader of the Extreme Conditions group at the Max Planck Institute for Chemical Physics of Solids in Dresden, working on quantum phase transitions and non-Fermi-liquid phenomena in strongly correlated electron systems, in particular on ferromagnetic quantum criticality.

Sven Friedemann was born in Leipzig, Germany in 1980. He obtained his Diplom in physics in 2004 from the University of Leipzig, Germany and his Dr. rer. nat. from the Technical University of Dresden, Germany in 2009. He was a research fellow at the Cavendish Laboratory at the University of Cambridge, UK 2010–2013. Since 2014 he is a lecturer in physics at the University of Bristol, UK. His research focuses on correlated electron systems, particularly, in the vicinity of quantum phase transitions. He has worked on electronic transport measurements and electronic structure studies. He has implemented those under high pressure and at very low temperatures.

Cornelius Krellner was born in Dresden, Germany in 1978. He studied physics in Dresden and at the ETH Zurich (Diplom in 2004). He obtained the Dr. rer. nat. from the Technical University of Dresden in 2009 and was a research associate at the Max-Planck-Institute for Chemical Physics of Solids in Dresden (2005–2011). He was a PostDoc at the Cavendish Laboratory, University of Cambridge (2011–2012) and became full professor for experimental solid state physics in 2012 at the Goethe-University Frankfurt/Main. His research interest is on the crystal growth and characterization of strongly correlated electron materials with special focus on unconventional superconductors as well as magnetic materials close to a quantum critical point. For his achievements he was awarded with the Otto–Hahn–Medal and the ThyssenKrupp Electrical Steel Dissertation prize.

Christoph Geibel was born in Heidelberg, Germany, in 1954. He obtained his Diploma in Physics (1978) and D. Sc. (1982) from Karlsruhe Technical University, Germany. He was a researcher at the Telefunken Electronic Company (1984–1988) and a research associate at the faculty of Physics at the Technical University Darmstadt, Germany (1988– 1997). Since 1997 he is group leader of the material development group at the Max Planck Institute for Chemical Physics of Solids in Dresden, Germany. He has worked on the search for and the investigation of new strongly correlated electron system, especially heavy fermion systems. Current areas of research are unconventional metallic, superconducting, and magnetic states near quantum critical points.

Steffen Wirth was born in Grimma/Saxony, Germany in 1963. He obtained a diploma (1990) as well as doctoral degree (1995) in physics from the Technical University in Dresden while he conducted graduate work at the Institute for Solid State and Materials Research Dresden. He was postdoctoral scientist at Trinity College Dublin (1995–1996) and at Florida State University (1996–2000) before becoming a staff member at the Max-Planck-Institute for Chemical Physics of Solids Dresden in 2000. In 2009, he completed his habilitation at TU Dresden and was a visiting professor at the University of Goettingen, Germany. He became a group leader at the MPI for Chemical Physics of Solids Dresden in 2010. His research has focused on magnetism and superconductivity, with emphasis on strongly correlated electron systems and their properties at small length scales. His expertise includes Scanning Tunneling Microscopy, magnetic and electronic transport measurements at low temperatures and high magnetic fields.

Stefan Kirchner was born in Fulda, Germany in 1971. He studied physics at the State University of New York, USA and the University of Würzburg, Germany. After completion of his diploma, he moved to Karlsruhe to work on his PhD. He received his PhD from the Technical University of Karlsruhe (now Karlsruhe Institute of Technology). From 2003 to 2009 he worked as a research associate and later as a research assistant at Rice University in Houston, USA. Since 2009 he is junior research group leader of the Max Planck Institute for Physics of Complex Systems and Chemical Physics of Solids in Dresden, Germany. He works on the theoretical description of strongly interacting systems, in particular dilute and dense Kondo systems with a recent emphasis on quantum phase transitions and the emergence of novel states associated with quantum criticality.

Elihu Abrahams was born in New York State, USA. He obtained his Ph. D. (1952) degree from the University of California, Berkeley. He was a research associate (1953–55) and a research assistant professor (1955–56) at the University of Illinois at Urbana-Champaign. He was assistant professor (1956–59), associate professor (1959–1966), full professor (1966–1998), and professor emeritus (1999–2010) at Rutgers University. Since 2010 he has been adjunct professor at the University of California, Los Angeles. He has worked on various aspects of condensed matter theory, including superconductivity, phase transitions, and strongly-correlated electron systems, and disorder.

Qimiao Si was born in Zhuji, Zhejiang Province China in 1966. He obtained his B.S. (1986) degree from University of Science and Technology of China and his Ph. D. (1991) degree from the University of Chicago. He did his postdoctoral works (1991–1995) at Rutgers University and University of Illinois at Urbana-Champaign. In 1995 he joined the faculty of Rice University, where he is the Harry C. and Olga K. Wiess Professor of Physics. His research is in the field of theoretical condensed matter physics, with a focus on strongly correlated electron systems. Specific research subjects have included quantum criticality, non-Fermi liquid physics, heavy fermion phenomena, high temperature cuprate and iron-pnictide superconductivity, and mesoscopic and disordered electronic systems.

Cited by

View all 16 citing articles

no accessTransport Spectroscopy of the Field Induced Cascade of Lifshitz Transitions in YbRh2Si2

104702, 10.7566/JPSJ.88.104702

no accessNon-Fermi-Liquid Behavior in CeRu2Si2 at Ultralow Temperatures Studied by Thermal Expansion and Magnetostriction

124712, 10.7566/JPSJ.86.124712

no accessKondo Effect of a Jahn–Teller Ion Vibrating in a Cubic Anharmonic Potential

104706, 10.7566/JPSJ.83.104706