Parasitic small-moment-antiferromagnetism and non-linear coupling of hidden order and antiferromagnetism in URu{}_{2}Si{}_{2} observed by Larmor diffraction

Parasitic small-moment-antiferromagnetism and non-linear coupling of hidden order and antiferromagnetism in URuSi observed by Larmor diffraction

P. G. Niklowitz Physik Department E21, Technische Universität München, 85748 Garching, Germany Department of Physics, Royal Holloway, University of London, Egham TW20 0EX, UK    C. Pfleiderer Physik Department E21, Technische Universität München, 85748 Garching, Germany    T. Keller ZWE FRM II, Technische Universität München, 85748 Garching, Germany Max-Planck-Institut für Festkörperforschung, Heisenbergstrasse 1, 70569 Stuttgart, Germany    M. Vojta Institute for Theoretical Physics Universität zu Köln, Zülpicher Strasse 77, 50937 Köln, Germany    Y.-K. Huang Van der Waals-Zeeman Institute, University of Amsterdam, 1018XE Amsterdam, The Netherlands    J. A. Mydosh Kamerlingh Onnes Laboratory, Leiden University, 2300RA Leiden, The Netherlands

We report simultaneous measurements of the distribution of lattice constants and the antiferromagnetic moment in high-purity URuSi, using both Larmor and conventional neutron diffraction, as a function of temperature and pressure up to 18 kbar. We establish that the tiny moment in the hidden order (HO) state is purely parasitic and quantitatively originates from the distribution of lattice constants. Moreover, the HO and large-moment antiferromagnetism (LMAF) at high pressure are separated by a line of first-order phase transitions, which ends in a bicritical point. Thus the HO and LMAF are coupled non-linearly and must have different symmetry, as expected of the HO being, e.g., incommensurate orbital currents, helicity order, or multipolar order.

hidden order, antiferromagnetism, Larmor diffraction, pressure, neutron diffraction

In recent years hydrostatic pressure has become widely used in the search for new forms of electronic order, because it is believed to represent a controlled and clean tuning technique. Novel states discovered in high-pressure studies include superconducting phases at the border of magnetism and candidates for genuine non-Fermi liquid metallic states. However, a major uncertainty in these studies concerns the possible role of pressure inhomogeneities, that originate, for instance, in the pressure-transmitting medium and inhomogeneities of the samples. To settle this issue requires microscopic measurements of the distribution of lattice constants across the entire sample volume, which, to the best of our knowledge, has not been available so far.

The perhaps most prominent and controversial example that highlights the importance of sample inhomogeneities and pressure tuning is the heavy-fermion superconductor URuSi. The reduction of entropy at a phase transition at , discovered in URuSi over twenty years ago, is still not explained Palstra et al. (1985); Maple et al. (1986); Schlabitz et al. (1986). The associated state in turn is known as ’hidden order’ (HO). The discovery of the HO was soon followed by the observation of a small antiferromagnetic moment (SMAF),   per U atom Broholm et al. (1987) then believed to be an intrinsic property of the HO. The emergence of large-moment antiferromagnetism (LMAF) of   per U atom Amitsuka et al. (1999) under pressure consequently prompted intense theoretical efforts to connect the LMAF with the SMAF and the HO. In particular, models have been proposed that are based on competing order parameters of the same symmetry, i.e., linearly coupled order parameters, in which the SMAF is intrinsic to the HO Gor’kov and Sokol (1992); Agterberg and Walker (1994); Shah et al. (2000); Mineev and Zhitomirsky (2005). This is contrasted by proposals for the HO parameter such as incommensurate orbital currents Chandra et al. (2002), multipolar order Kiss and Fazekas (2005), or helicity order Varma and Zhu (2006), where HO and LMAF break different symmetries.

The symmetry relationship of HO and LMAF clearly yields the key to unravelling the nature of the HO state Shah et al. (2000); Mineev and Zhitomirsky (2005). While some neutron scattering studies of the temperature–pressure phase diagram suggest that the HO–LMAF phase boundary ends in a critical end point Bourdarot et al. (2005), other studies concluded that it meets the boundaries of HO and LMAF in a bicritical point Motoyama et al. (2003); Uemura et al. (2005); Hassinger et al. (2008); Motoyama et al. (2008). This distinction is crucial, as a critical end point (bicritical point) implies that HO and LMAF have the same (different) symmetries, respectively Mineev and Zhitomirsky (2005). Moreover, there is a substantial disagreement w.r.t. the location and shape of the HO–LMAF phase boundary (see e.g. Ref. Amitsuka et al. (2007)). This lack of consistency is, finally, accompanied by considerable variations of the size and pressure dependence of the moment reported for the SMAF Amitsuka et al. (2007), where NMR studies in powder samples suggested the SMAF to be parasitic Matsuda et al. (2003). Accordingly, to identify the HO in URuSi it is essential to clarify unambiguously the nature of the SMAF and the symmetry relationship of HO and LMAF.

It was long suspected that the conflicting results are due to a distribution of lattice distortions due to defects. Notably, uniaxial stress studies showed that LMAF is stabilized if the ratio of the tetragonal crystal is reduced by the small amount Yokoyama et al. (2005). Hence, the parasitic SMAF may in principle result from a distribution of values across the sample, with its magnitude depending on sample quality and experimental conditions. In particular, differences of compressibility of wires, samples supports or strain gauges that are welded, glued or soldered to the samples will forcibly generate uncontrolled local strains that strongly affect any conclusions about the SMAF signal (see, e.g., Refs Motoyama et al. (2003); Uemura et al. (2005); Hassinger et al. (2008); Motoyama et al. (2008)).

In this Letter we report simultaneous measurements of the distribution and temperature dependence of the lattice constants, as well as the antiferromagnetic moment, of a pure single crystal of URuSi utilizing a novel neutron scattering technique called Larmor diffraction (LD). This allowed to study samples that are completely free to float in the pressure transmitting medium, thereby experiencing essentially ideal hydrostatic conditions at high pressures. Our data of the distribution of lattices constants establishes quantitatively that the SMAF is purely parasitic. In addition, we find a rather abrupt transition from HO to LMAF which extends from up to a bicritical point (preliminary data of were reported in nik ()). We conclude that the HO–LMAF transition is of first order and that HO and LMAF must be coupled non-linearly. This settles the perhaps most important, long-standing experimental issue on the route to identifying the HO.

Figure 1: (a) Schematic of Larmor diffraction Rekveldt et al. (2001); Keller et al. (2002), see text for details. (b) Typical variation of the polarization as a function of the total Larmor phase . (c) Pressure dependence of the width of the lattice-constant distribution for the a- and c-axis in URuSi. With increasing pressure the width of the distribution increases.

Larmor diffraction permits high-intensity measurements of lattice constants with an unprecedented high resolution of Rekveldt et al. (2001); Keller et al. (2002). As shown in Fig. 1 (a) the sample is thereby illuminated by a polarized neutron beam (arrows indicate the polarization); is the reciprocal lattice vector; is the Bragg angle; ’AD’ is the polarization analyzer and detector. The radio frequency (RF) spin resonance coils (C1-C4) change the polarization direction, as if the neutrons undergo a Larmor precession with frequency along the distance . The total Larmor phase of precession thereby depends linearly on the lattice constant : ( is the mass of the neutron Rekveldt et al. (2001); Keller et al. (2002)).

The Larmor diffraction was carried out at the spectrometer TRISP at the neutron source FRM II. The temperature and pressure dependence of the lattice constants was inferred from the (400) Bragg peak for the axis and the (008) Bragg peak for the axis. The magnetic ordered moment was monitored with the same setup using conventional diffraction. For our high-pressure studies a Cu:Be clamp cell was used with a Fluorinert mixture Pfleiderer et al. (2005). The pressure was inferred at low temperatures from the (002) reflection of graphite as well as absolute changes of the lattice constants of URuSi taking into account published values of the compressibility.

The single crystal studied was grown by means of an optical floating-zone technique at the Amsterdam/Leiden Center. High sample quality was confirmed via X-ray diffraction and detailed electron probe microanalysis. Samples cut-off from the ingot showed good resistance ratios (20 for the axis and 10 for the axis) and a high superconducting transition temperature  K. The magnetization of the large single crystal agreed very well with data shown in Ref. Pfleiderer et al. (2006) and confirmed the absence of ferromagnetic inclusions. Most importantly, in our neutron scattering measurements we found an antiferromagnetic moment per U atom, which matches the smallest moment reported so far Amitsuka et al. (2007).

As the Larmor phase is proportional to the lattice constant , the polarization of the scattered neutron beam reflects the distribution of lattice constants across the entire sample volume Keller et al. (2002). While Larmor diffraction was recently employed for the first time in a high-pressure study Pfleiderer et al. (2007), measurements of the distribution of lattice have not been exploited to resolve a major scientific issue (for proof of principle studies in Al-alloys see Ref. Rekveldt et al. (2001)).

In order to explore the origin of the SMAF moment we have measured the spread of lattice constants, keeping in mind that a distribution of the lattice-constant ratio may be responsible for AF order in parts of the sample. As shown in Fig. 1 (b) changes only weakly between ambient pressure and 17.3 kbar. Accordingly the distribution of lattice constants, which is given by the Fourier transform of , changes only weakly as a function pressure as shown in Fig. 1c). Thus pressure only slightly boosts the distribution of lattice constants, but does not generate substantial additional inhomogeneities. Moreover, we confirmed that the size of remained unchanged tiny after our high-pressure studies.

Assuming a Gaussian distribution of both lattice constants, we infer the distribution of . At low pressure, we arrive at a full width at half-maximum of . Recalling that the tail of the Gaussian distribution beyond represents the sample’s volume fraction in which LMAF forms Yokoyama et al. (2005), an average magnetic moment of is expected in our sample. This is in excellent quantitative agreement with the experimental value and represents the first main result we report.

Figure 2: Temperature dependence of the lattice constants and thermal expansion at various pressures. The HO and LMAF transitions are indicated by empty and filled arrows, respectively. (a) Data for the -axis; (b) thermal expansion of the -axis derived from the data shown in (a). (c) Data for the -axis; (d) thermal expansion of the -axis derived from the data shown in (c).

We continue with a discussion of the temperature dependence of the lattice constants and its change with pressure. At zero pressure in a wide temperature range below room temperature (not shown) the thermal expansion is positive for both axes de Visser et al. (1986). However, for the c-axis, the lattice constant shows a minimum close to 40 K and turns negative at lower temperatures. This general behavior is unchanged under pressure.

Shown in Fig. 2 are typical low-temperature data for the a- and c-axis. At ambient pressure can be barely resolved. However, when crossing a pronounced additional signature emerges rapidly and merges with . Measurements of the antiferromagnetic moment (see below), identify this anomaly as the onset of the LMAF order below its . At the transition the lattice constant for the a- and c-axis show a pronounced contraction and expansion, respectively.

The pressure and temperature dependence of determined at is shown in the inset of Fig. 3 (a). Close to , where is near base temperature, we observe first evidence of the LMAF magnetic signal, which rises steeply and already reaches almost its high-pressure limit at 5 kbar. The pressure dependence was determined by assuming the widely reported high-pressure value of and comparing the magnetic (100) and nuclear (004) peak intensity.

Figure 3: (a) Pressure dependence of the low-temperature magnetic moment. The inset shows the temperature dependence of the magnetic peak height at various pressures. (b) Phase diagram based on Larmor diffraction and conventional magnetic diffraction data. The onset of LMAF is marked by full and of HO by empty symbols (x marks a transition near base temperature). For better comparison data of (black symbols) from Refs. Amitsuka et al. (2007); Motoyama et al. (2003); Hassinger et al. (2008); Motoyama et al. (2008) are shown. The values (red symbols) of all references are consistent. Inset: background-free specific-heat jump derived from thermal-expansion data via the Ehrenfest relation (full circles). Heat capacity data is taken from Refs. Palstra et al., 1985 (square) and Hassinger et al., 2008 (empty circle).

The temperature–pressure phase diagram shown in Fig. 3 (b) displays and taken from the magnetic Bragg peak (Fig. 3 (a)) and from the Larmor diffraction data (Fig. 2), respectively. The different data sets show excellent agreement (except at , due to the variable parasitic nature of the SMAF). The main results contained in Fig. 3 are (i) the very small value of 0.012  of the average low-temperature ordered moment at zero pressure, (ii) a particularly abrupt increase of the low-temperature moment at  kbar (as compared to previous studies Motoyama et al. (2003); Uemura et al. (2005); Hassinger et al. (2008); Motoyama et al. (2008); Amitsuka et al. (2007)), (iii) the steep slope of the HO–LMAF phase boundary, and (iv) the merging of the HO–LMAF phase boundary with the transition lines at approximately 9 kbar. Fig. 2 (b) shows that we can follow this phase boundary from low up to .

Figure 4: Extended phase diagram of URuSi based on the data presented here (diamonds) and signatures in resistivity (brownKagayama et al. (1994) and greyHassinger et al. (2008) circles). and denote coherence maxima in the resistivity Kagayama et al. (1994) and magnetisation Pfleiderer et al. (2006), respectively. The HO might either mask a QCP (I) or replace LMAF (II) near quantum criticality.

Most importantly, (iv) implies that HO and LMAF are fully separated by a phase boundary which has to be of first order with a bicritical point, since three second-order phase transition lines cannot meet in one point. (Note that the phase boundaries from the HO and LMAF to the disordered high-temperature phase are already known to be of second order from qualitative heat capacity measurements Palstra et al. (1985); Hassinger et al. (2008).) This conclusion is perfectly consistent with (ii) and (iii), and it excludes a linear coupling between the HO and LMAF order parameters Mineev and Zhitomirsky (2005).

Although our results show that the HO and LMAF must have different symmetry, they also suggest that both types of order may have a common origin. Using the Ehrenfest relation, we have converted our thermal expansion data into a background-free estimate of the specific-heat jump, , at the PM to LMAF transition. The inset in Fig. 3 (b) shows a continuous evolution with pressure of the jumps at the LMAF to PM and corresponding HO to PM transitions. The common origin of both phases may in fact be related to excitations seen in neutron scattering. Notably, excitations at (1,0,0) only appear in the HO phase and may be its salient property Villaume et al. (2008); Elgazzar et al. (2009). However, excitations at (1.4,0,0) in the PM state become gapped in both the HO and LMAF state and have been quantitatively linked to the specific heat jump at zero pressure Wiebe et al. (2007).

Finally, Fig. 4 suggests a new route to the HO. It shows a summary of the pressure evolution of features in the resistivity and magnetization, which suggest the existence of an AF quantum critical point (QCP) at an extrapolated negative pressure. Remarkably, these features, which are usually denoted as Kondo or coherence temperature, all seem to extrapolate to the same critical pressure. The HO in URuSi could be understood as emerging from quantum criticality, possibly even masking an AF QCP (case I in Fig. 4). However, considering the remoteness of the proposed QCP, the balance between LMAF and HO might rather be tipped by pressure induced changes of the properties of URuSi. This has for example been suggested in a recent proposal, where HO and LMAF are believed to be variants of the same underlying complex order parameter hau (). In such a scenario, the HO is more likely to collapse at the proposed QCP as denoted by the dashed line (case II in Fig. 4). The pressure dependence of sets constraints on any theory of the HO involving quantum criticality.

In conclusion, using Larmor diffraction to determine the lattice constants and their distribution at high pressures and with very high precision, we were able to show that the SMAF in URuSi is purely parasitic. Moreover, the HO and LMAF are separated by a line of first-order transitions ending in a bicritical point. This is the behavior expected for the HO being, e.g., incommensurate orbital currents, helicity order, or multipolar order.

We are grateful to P. Böni, A. Rosch, A. de Visser, K. Buchner, F. M. Grosche and G. G. Lonzarich for support and stimulating discussions. We thank FRMII for general support. CP and MV acknowledge support through DFG FOR 960 (Quantum phase transitions) and MV also acknowledges support through DFG SFB 608.


  • Palstra et al. (1985) T. T. M. Palstra, et al., Phys. Rev. Lett. 55, 2727 (1985).
  • Maple et al. (1986) M. B. Maple, et al., Phys. Rev. Lett. 56, 185 (1986).
  • Schlabitz et al. (1986) W. Schlabitz, et al., Z. Phys. B 62, 171 (1986).
  • Broholm et al. (1987) C. Broholm, et al., Phys. Rev. Lett. 58, 1467 (1987).
  • Amitsuka et al. (1999) H. Amitsuka, et al., Phys. Rev. Lett. 83, 5114 (1999).
  • Gor’kov and Sokol (1992) L. P. Gor’kov and A. Sokol, Phys. Rev. Lett. 69, 2586 (1992).
  • Agterberg and Walker (1994) D. F. Agterberg and M. B. Walker, Phys. Rev. B 50, 563 (1994).
  • Shah et al. (2000) N. Shah, et al., Phys. Rev. B 61, 564 (2000).
  • Mineev and Zhitomirsky (2005) V. P. Mineev, M. E. Zhitomirsky, Phys. Rev. B 72, 014432 (2005).
  • Chandra et al. (2002) P. Chandra, et al., Nature 417, 831 (2002).
  • Kiss and Fazekas (2005) A. Kiss, P. Fazekas, Phys. Rev. B 71, 054415 (2005).
  • Varma and Zhu (2006) C. M. Varma, L. Zhu, Phys. Rev. Lett. 96, 036405 (2006).
  • Bourdarot et al. (2005) F. Bourdarot, et al., Physica B 359-361, 986 (2005).
  • Motoyama et al. (2003) G. Motoyama, et al., Phys. Rev. Lett. 90, 166402 (2003).
  • Uemura et al. (2005) S. Uemura, et al., J. Phys. Soc. Japan 74, 2667 (2005).
  • Hassinger et al. (2008) E. Hassinger, et al., Phys.Rev.B 77, 115117 (2008).
  • Motoyama et al. (2008) G. Motoyama, et al., J. Phys. Soc. Japan 77, 123710 (2008).
  • Amitsuka et al. (2007) H. Amitsuka, et al., J. Magn. Magn. Mat. 310, 214 (2007).
  • Matsuda et al. (2003) K. Matsuda, et al., J. Phys.: Condens. Matter 15, 2363 (2003).
  • Yokoyama et al. (2005) M. Yokoyama, et al., Phys. Rev. B 72, 214419 (2005).
  • (21) P. G. Niklowitz, et al., Proceed. SCES 2008.
  • Rekveldt et al. (2001) M. T. Rekveldt, et al., Eur. Phys. Lett. 54, 342 (2001).
  • Keller et al. (2002) T. Keller, et al., Appl. Phys. A (Suppl.) 74, 332 (2002).
  • Pfleiderer et al. (2005) C. Pfleiderer, et al., J. Phys. Conden. Matter 17, S3111 (2005).
  • Pfleiderer et al. (2006) C. Pfleiderer, et al., Phys. Rev. B 74, 104412 (2006).
  • Pfleiderer et al. (2007) C. Pfleiderer, et al., Science 316, 1871 (2007).
  • de Visser et al. (1986) A. de Visser, et al., Phys. Rev. B 34, 8168 (1986).
  • Kagayama et al. (1994) T. Kagayama, et al., J. Alloy. Compd. 213, 387 (1994).
  • Villaume et al. (2008) A. Villaume, et al., Phys. Rev. B 78, 012504 (2008).
  • Elgazzar et al. (2009) S. Elgazzar, et al., Nat. Mater. 8, 337 (2009).
  • Wiebe et al. (2007) C. R. Wiebe, et al., Nature Phys. 3, 96 (2007).
  • (32) K. Haule and G. Kotliar, arXiv:0907.3889 and 0907.3892.
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