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Modeling the Localized-to-Itinerant Electronic Transition in the Heavy Fermion System CeIrIn5

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Science  07 Dec 2007:
Vol. 318, Issue 5856, pp. 1615-1617
DOI: 10.1126/science.1149064

Abstract

We address the fundamental question of crossover from the localized to the itinerant state of a paradigmatic heavy fermion material: CeIrIn5. The temperature evolution of the one-electron spectra and the optical conductivity are predicted from first-principles calculation. The buildup of coherence in the form of a dispersive many-body feature is followed in detail, and its effects on the conduction electrons of the material are revealed. We find multiple hybridization gaps and link them to the crystal structure of the material. Our theoretical approach explains the multiple peak structures observed in optical experiments and the sensitivity of CeIrIn5 to substitutions of the transition metal element and may provide a microscopic basis for the more phenomenological descriptions currently used to interpret experiments in heavy fermion systems.

Heavy fermion materials have unusual properties arising from the presence of a partially filled shell of f orbitals and a very broad band of conduction electrons. At high temperatures, the f electrons behave as atomic local moments. As the temperature is reduced, the moments combine with the conduction electrons to form a fluid of very heavy quasiparticles, with masses that are two to three orders of magnitude larger than the mass of the electron (1, 2).

These heavy quasiparticles can undergo superconducting or magnetic transitions at much lower temperatures. Understanding how the itinerant low-energy excitations emerge from the localized moments of the f shell is one of the central challenges of condensed-matter physics. It requires the understanding of how the dual, atomic particle–like character and itinerant, wave-like character of the electron manifest themselves in the different physical properties of a material.

CeIrIn5 (3) has a layered tetragonal crystal structure (4, 5) (Fig. 1A) in which the layers of CeIn3 (shown as red and gray spheres) are stacked between layers of IrIn2 (shown as yellow and gray spheres). Each Ce atom is surrounded by four In atoms in the same plane and by eight In atoms out of plane.

Fig. 1.

(A) Crystal structure of CeIrIn5. Red, yellow, and gray spheres correspond to Ce, Ir, and In atoms, respectively. (B) Ce 4f local density of state (DOS) calculated by LDA+DMFT at 10 and 300 K. (C) The quasiparticle peak height versus temperature (blue points), the imaginary part of Ce 4f5/2 self-energy Σf(ω = 0) (red points), and its temperature derivative (green points). The buildup of coherence is very slow and gradual. Around T* ∼ 50 K, the coherence first sets in and manifests itself in a fast increase of the quasiparticle peak (blue line) and crossover in the scattering rate [the derivative of scattering rate (green line) is peaked at T*]. The quasiparticle peak weight saturates at much lower temperature (<5 K) and drops to zero at very high temperature, displaying a very long logarithmic tail.

To describe the electronic structure of these classes of materials, one needs to go beyond the traditional concepts of bands and atomic states and focus on the concept of a spectral function A(k,ω)LL, the function which describes the quantum mechanical probability of removing or adding an electron with angular momentum and atomic character L = (l, m, a), momentum k, and energy ω. It is measured directly in angle-resolved photoemission experiments (ARPES) and inverse photoemission experiments.

To evaluate the spectral function, we use dynamical mean field theory (DMFT) (6) in combination with the local density approximation (LDA+DMFT) (7), which can treat the realistic band structure, the atomic multiplet splitting, and Kondo screening on the same footing. The spectral function A(k,ω) is computed from the corresponding one-electron Green's function Embedded Image through the relation A(k,ω) = [G(k,ω) – G(k,ω)]/(2πi). Here, Hk and Ok are the Hamiltonian and overlap matrix obtained by the LDA method (8), μ is the chemical potential, i is the imaginary unit, G is the conjugate transpose of G, and Σ is the DMFT self-energy, which requires a solution of the quantum impurity problem embedded in a self-consistent medium. We used a vertex-corrected one-crossing approximation (7), and the results were further cross-checked against a continuous-time quantum Monte Carlo method (9, 10). The Slater integrals F2, F4, and F6 were computed by the atomic physics program of (11), and F0 was estimated by the constrained LDA to be 5 eV (12). The localized Ce 4f orbital was constructed from the nonorthogonal linear muffin-tin orbitals in a particular way to maximize its f character, as explained elsewhere (13).

The spectral function of f electron materials has been known to exhibit notable many-body effects. Setting the stage for their theoretical description, Fig. 1B displays the Ce 4f local spectral function [i.e., A(ω) ΣkA(k,ω)], which is measured in angle-integrated photoemission experiments.

At room temperature, there is very little spectral weight at the Fermi level because the f electrons are tightly bound and localized on the Ce atom, giving rise to a broad spectrum concentrated mainly in the lower and upper Hubbard bands at –2.5 and +3 eV, respectively.

As the temperature is decreased, a narrow peak appears near the Fermi level (Fig. 1B). The states forming this peak have a small but finite dispersion, and therefore the area of the peak can be interpreted as the degree of f electron delocalization. This quantity, as well as the scattering rate of the Ce 4f states [Im Σ(ω = 0)], exhibit a clear crossover at a temperature scale T* of the order of 50 K (Fig. 1C).

Our results are consistent with the angle-integrated photoemission measurements (14) in which the onset of states with f character at the Fermi level was observed. But the experimental resolution has to be improved by one order of magnitude to resolve the narrow peak predicted by the theory.

We now turn to the total (traced over all orbitals) momentum-resolved spectral function Tr[A(k,ω)] plotted along symmetry directions in the Brillouin zone. In a band-theory description, it would be sharply peaked on a series of bands ϵn(k), and the weight of those peaks would be unity. It is worthwhile to compare the high-intensity features of the LDA+DMFT spectra (color coded) with the LDA bands [ϵn(k), shown as blue lines] (Fig. 2A). In the region below –1 eV, there is a good correspondence between them. However, there is the systematic downshift (indicated by a green arrow) of the LDA+DMFT features relative to the LDA bands (which have mainly In 5p and Ir 5d character). Unexpectedly, a similar trend is seen in the ARPES of (15), which we redraw in Fig. 2B. The position of these bands is weakly temperature dependent and, if warmed to room temperature, an almost rigid upward shift of 5 meV was identified in our theoretical treatment. Experimentally, it was not possible to resolve the momentum in the z direction; therefore, the same experimental data (which can be thought as the average of the two paths from Γ to X and from Z to R), where Γ, X, Z, and R are symmetry points in the momentum space shown in Fig. 2B, are repeated in the two directions.

Fig. 2.

(A) Momentum-resolved total spectral functions calculated by the LDA+DMFT method at 10 K are shown by color scheme. The LDA bands are indicated as blue lines. (B) Color plot shows experimental ARPES data reproduced from (15). (C and D) The momentum-resolved Ce 4f spectral function at 10 K (C) and 300 K (D).

Near the Fermi level (between –0.5 and +1 eV), there are substantial discrepancies between the LDA bands (which, in this region, have substantial f character) and the LDA+DMFT features. The correlations treated by LDA+DMFT substantially modify the spectral function features with f content, transferring spectral weight into the upper Hubbard band located around +3 eV (white region in Fig. 2A).

Hubbard bands are excitations localized in real space, without a well-defined momentum, and therefore they show up as a blurred region of spectral weight in the momentum plot of Fig. 2A. There is also a lower Hubbard band around –2.5 eV, which is hardly detectable in this figure. The reason for this is that it carries a very small spectral weight, which is redistributed over a broad frequency region as shown in Fig. 1B.

It is also useful to compare the LDA+DMFT Hubbard bands with those obtained with the more familiar LDA+U method, which is equivalent to the Hartree-Fock approximation of the LDA+DMFT method. The LDA+U method inserts a sharp nondispersive band around –2.5 eV and substantially twists the rest of the conduction bands. For the purpose of describing the set of bands below –1 eV, the LDA+DMFT method is therefore closer to the LDA type of calculation with f bands removed from the valence band.

To obtain further insights into the nature of the low-energy spectra, we show the momentum-resolved f electron spectral function of Fig. 1B in Fig. 2, C and D. The two plots correspond to the low-temperature (10 K) and high-temperature (300 K) spectra, respectively. At room temperature, a set of broad and dispersive bands is seen and should be interpreted as the spd bands leaving an imprint in the f electron spectral function resulting from hybridization. At low temperature, a narrow stripe of spectral weight appears at zero frequency, which cuts the conduction bands and splits them into two separate pieces, divided by a new hybridization gap.

The two straight nondispersive bands at –0.3 and +0.3 eV can also be identified in Fig. 2C and are due to the spin-orbit coupling (16). The same splitting of the coherence peak can be identified in the local spectra plotted in Fig. 1B and was recently observed in an ARPES study (14).

A detailed analysis of the zero-energy stripe of spectra in Fig. 2C reveals that the low-energy features correspond to the three very narrow bands (the dispersion is of the order of 3 meV) crossing the Fermi level. This is the origin of the large effective mass and large specific heat of the material at low temperatures. The low-energy band structure and its temperature dependence are theoretical predictions that can be verified experimentally in future ARPES studies.

Optical conductivity is a very sensitive probe of the electronic structure and has been applied to numerous heavy fermion materials (17). It is a technique that is largely complementary to the photoemission on two counts: It probes the bulk (and not the surface), and it is most sensitive to the itinerant spd electrons (rather than the f electrons).

A prototypical heavy fermion at high temperatures has an optical conductivity characterized by a very broad Drude peak. At low temperatures, optical data are usually modeled in terms of transitions between two renormalized bands, separated by a hybridization gap. These two bands give rise to a very narrow Drude peak of small weight and an optical absorption feature above the hybridization gap, termed the mid-infrared peak. This picture qualitatively describes the experimental data of CeIrIn5 (18, 19), which we reproduce in Fig. 3B. However, this simplified two-band model fails to account for some aspects of the data. For example, at 10 K, there is a clear structure in the mid-infrared peak. In addition to the broad shoulder around 0.07 eV, a second peak around 0.03 eV can be identified, which was previously interpreted as the absorption on the bosonic mode that might bind electrons in the unconventional superconducting state (18, 20).

Fig. 3.

The optical conductivity at several temperatures (A) obtained by LDA+DMFT and (B) measured experimentally and reproduced from (18). (C and D) The momentum-resolved non–Ce 4f spectral function (AtotalACe 4f) at 10 K (C) and 300 K (D). Blue arrow, 30-meV hybridization gap; green arrow, 70-meV hybridization gap.

Also, the hybridization gap in simplified theories gives rise to a sharp drop of conductivity below the energy of the gap, whereas broader features are seen experimentally.

Optical conductivity within LDA+DMFT was recently implemented (21), and we show the results in Fig. 3A. They bear a strong resemblance to the experimental data in Fig. 3B. For example, a broad Drude peak at high temperature and a very clear splitting of the mid-infrared peak at low temperature are visible.

To understand the physical origin of these multiple peaks, we plot the momentum-resolved conduction electron (non–Ce 4f) spectral function along a representative high-symmetry line at 10 and 300 K, respectively (Fig. 3, C and D). There is a dramatic difference between the two temperatures. At high temperature, we see two bands in this momentum direction: One has a very short lifetime and the other has a long lifetime. The spread of the left band in Fig. 3D is due to electron-electron scattering, which broadens the band for about 100 meV. The character of both bands is primarily of In 5p, with an important difference. The left band comes mostly from the In atoms in the IrIn2 layer, whereas the right band is mostly due to In in the CeIn3 layer. The latter In atoms will be called in plane (each Ce atom has four neighbors of this type), and the former will be called out of plane (there are eight nearest neighbors to the Ce atom). As the temperature is lowered, the two In bands hybridize in a very different way with the Ce 4f moment. It is quite unexpected that the in-plane In atoms hybridize less with the Ce moment, leading to a small hybridization gap of the magnitude 30 meV (blue arrow in Fig. 3C). The out-of-plane In atoms are more coupled to the Ce moment, which leads to a larger hybridization gap of the order of 70 meV (green arrow in Fig. 3C). The existence of multiple hybridization gaps results in the splitting of the mid-infrared peak in optical conductivity (Fig. 3A).

The fact that the Ce moment is more coupled to out-of-plane In than to in-plane In provides a natural explanation for why these materials are sensitive to the substitution of transition metal ion Ir with Co or Rh. Namely, the out-of-plane In atoms are strongly coupled not only to Ce but also to the transition metal ion in their immediate neighborhood, whereas the in-plane In atoms are insensitive to the substitution.

Some of the results of the microscopic theory, such as the momentum-dependent hybridization (19) and the slow buildup of coherence (22), were foreshadowed by earlier phenomenological approaches. The first-principles DMFT treatment places these ideas within a microscopic framework.

In investigating the formation of the heavy fermion state with temperature in CeIrIn5, we have shown that incorporating local correlations, only on the f site, allows for a coherent description of the evolution of the one-electron spectra and the optical conductivity with temperature. The approach provides a natural explanation for many unexpected features observed in this material and makes several quantitative predictions for the evolution of the spectra as a function of temperature, which can be tested by ARPES measurements currently under way. Although the single-site DMFT description is sufficient in a broad region of temperatures and parameters, cluster extensions of DMFT will be necessary to address the quantum criticality that takes place as Ir is replaced by Rh and Co and to address the possible instabilities toward unconventional superconductivity. Although model cluster DMFT studies seem very promising, the implementation of these methods, in conjunction with realistic electronic structure, remains a challenge for the future. Furthermore, in the treatment of other compounds of the same class (Ir substituted by Co or Rh), the correlations on the 3d or 4d transition metal will require GW approximation to treat the electronic structure.

References and Notes

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