Two-magnon scattering in the 5d all-in-all-out pyrochlore magnet Cd2Os2O7

5d pyrochlore oxides with all-in-all-out magnetic order are prime candidates for realizing strongly correlated, topological phases of matter. Despite significant effort, a full understanding of all-in-all-out magnetism remains elusive as the associated magnetic excitations have proven difficult to access with conventional techniques. Here we report a Raman spectroscopy study of spin dynamics in the all-in-all-out magnetic state of the 5d pyrochlore Cd2Os2O7. Through a comparison between the two-magnon scattering and spin-wave theory, we confirm the large single ion anisotropy in this material and show that the Dzyaloshinskii–Moriya and exchange interactions play a significant role in the spin-wave dispersions. The Raman data also reveal complex spin–charge–lattice coupling and indicate that the metal–insulator transition in Cd2Os2O7 is Lifshitz-type. Our work establishes Raman scattering as a simple and powerful method for exploring the spin dynamics in 5d pyrochlore magnets.

P yrochlore lattice magnets feature a network of cornersharing tetrahedra, whose triangle-based lattice geometries can result in geometrically frustrated magnetism 1 . A number of 5d transition metal-oxide pyrochlores, including Cd 2 Os 2 O 7 2-7 and R 2 Ir 2 O 7 (R = Sm 8 , Nd 9 , Y 10 , Eu 11 , etc) are believed to host all-in-all-out (AIAO) antiferromagnetic ground states. A schematic of the AIAO ordered state in Cd 2 Os 2 O 7 is shown in Fig. 1b. The Os spins in a given Os-O tetrahedron point inward (all-in), while those in the neighboring tetrahedra point outward (all-out). In the 5d transition metal-oxide pyrochlores, AIAO order is often accompanied by a continuous metal-insulator transition (MIT). The close relationship between AIAO order and electronic structure is especially intriguing since AIAO order breaks time-reversal symmetry while retaining the crystalline symmetry of the pyrochlore lattice. Based on such symmetry breaking, numerous theoretical works have proposed that these systems may realize strongly correlated and topologically nontrivial states, in particular the Weyl semimetallic state 12,13 . These proposals have in turn stimulated a large experimental effort 5,8,14 .
The pyrochlore osmate Cd 2 Os 2 O 7 is a prototype system in which to investigate AIAO magnetism. The AIAO magnetic ordering at the Os sites has been firmly established by resonant X-ray and neutron diffraction below T N = 227 K 4,5 , and the material is available in high-quality single crystalline form 4 . The AIAO order drives an MIT which has recently been classified as Lifshitz-type 4,6,10 . Due to the 5d 3 (t 2g 3 ) configuration, the Os 5+ ion is in a L = 0, S = 3/2 state 5,7 . Since this state is an orbital singlet, spin-orbit coupling (SOC) does not, to first order, play a dominant role. Instead, the strong SOC manifests itself as a large single-ion anisotropy (SIA), which is in turn thought to stabilize the AIAO state 2,7,15 . This is in contrast with the Ir-based pyrochlores where the SOC leads to the formation of relativistic j eff = ½ orbitals and the AIAO order depends crucially on the antisymmetric Dzyaloshinskii-Moriya interaction (DMI) 16 . The Cd 2+ ion is non-magnetic, in contrast to most Ir-based pyrochlores R 2 Ir 2 O 7 8,9 , where the rare-earth ions may also order magnetically. These two pyrochlore sublattices (Ir and R) may be magnetically coupled, which complicates investigations of the Ir-site AIAO magnetism. 40 80 120 160 200 T 2g (1) T 2g (2) T 2g (4) T 2g ( While a number of studies have investigated the magnetic excitations in 5d pyrochlores, a full understanding of the AIAO magnetism remains elusive. This is partly due to the fact that the magnetic excitations in these systems have proven difficult to study with conventional techniques such as inelastic neutron scattering or resonant inelastic X-ray scattering (RIXS). Cd and Ir are strong neutron absorbers 17,18 , making inelastic neutron scattering challenging. Several RIXS studies have examined the spin excitations in AIAO magnets. Donnerer et al. 8 recently reported evidence for a dispersive spin-wave excitation in Sm 2 Ir 2 O 7 , while Clancy et al. 14 found evidence for a dispersive and heavily damped magnetic excitation in Eu 2 Ir 2 O 7 and Pr 2 Ir 2 O 7 . However, the resolution of state-of-the-art RIXS is still only 25 meV for Ir 8 and above 40 meV for Os 14 , so fine details of the magnetic excitation spectrum, including the dispersions and energy splitting between distinct magnetic excitations are difficult to resolve. In the case of Cd 2 Os 2 O 7, a recent RIXS experiment observed a dispersionless magnetic excitation that was interpreted as a superposition of single-site spin-flip excitations 15 . The magnetic excitation in Cd 2 Os 2 O 7 was found to be broad and featureless, so a detailed determination of the spin Hamiltonian from the experimental data was not attempted. As a result, the nature of the magnetic excitations of the AIAO state in Cd 2 Os 2 O 7 , their relationship with other degrees of freedom, and a quantitative understanding of the underlying microscopic spin Hamiltonian have not been clarified to date.
In this article, we report a combined Raman spectroscopic and theoretical investigation of the magnetic excitations in Cd 2 Os 2 O 7 . The fine energy resolution (~0.25 meV) of the Raman technique 19 allows us to observe two well-separated two-magnon peaks that were not detected with other spectroscopies. Our results constitute the first detection of two-magnon excitations in a 5d pyrochlore oxide using Raman scattering. Through a comparison with linear spin-wave theory (LSWT), we make quantitative estimates of the magnetic couplings that are in good agreement with recent many-body quantum-chemical calculations 7 and clarify the impact of the DMI, SIA, and Heisenbergexchange interaction on the magnetic excitation spectrum. Understanding the nature of the magnetic excitations and the role of the microscopic magnetic interactions provides a foundation for deeper and fundamental discussion regarding the magnetic properties. Our measurements also reveal signatures of nontrivial coupling between spin, charge and lattice degrees of freedom across the magnetically-driven MIT which indicates that this transition may be classified as Lifshitz-type. These results provide insight into the interplay between electronic structure and magnetism in 5d pyrochlore magnets and highlight the utility of Raman scattering for exploring the spin dynamics of other 5d AIAO pyrochlore magnets, such as the closely related pyrochlore iridates.

Results
Two-magnon Raman scattering. Below 100 meV, the Raman spectra of Cd 2 Os 2 O 7 show six phonon modes (see Fig. 1a). The spectra of Fig. 1a were obtained at 15 K using a 2.33 eV excitation laser in an unpolarized configuration. Six phonon modes may be discerned around 28, 32, 43, 57, 60, and 96 meV. These modes are consistent with a factor group analysis, which predicts six Ramanactive Γ-point phonon modes with A 1g + E g + 4T 2g symmetries for the cubic pyrochlore lattice with space group Fd3m 20 . By comparison with previous reports 20, 21 , the four peaks at 28, 43, 57, and 96 meV can be assigned to T 2g , the peak at 32 meV to E g , and the peak at 60 meV to A 1g . No change in the number of phonon modes was observed between 100 and 270 K, confirming the absence of a structural transition across T N . Further discussion of the phonon spectra and a comparison with firstprinciples calculations may be found in the Supplementary Note 1 and Supplementary Table 1.
Above 100 meV, the Raman spectra in Fig. 1 reveal two intriguing broad peaks. These are located at~127 meV and 152 meV and marked as M 1 and M 2 , respectively. The M 1 peak also possesses a low-energy shoulder, which we label M 1 ′. These features are shown in more detail in the inset of Fig. 1. The widths and energies of M 1 and M 2 are much larger than the optical phonon modes located below 100 meV. The polarization properties of M 1 and M 2 were investigated in three input-output polarization geometries: collinear, crossed, and unpolarized. We found that the lineshape and Raman shift of M 1 and M 2 are independent of polarization geometry ( Supplementary Fig. 2). For the remainder of our discussion, we focus on the unpolarized case, as the overall intensity is larger in this geometry. We also measured the Raman scattered intensity under 1.96 eV excitation at 100 K and verified that the Raman shifts of M 1 and M 2 are unchanged (Fig. 1c). This confirms that M 1 and M 2 are true Raman features and not from photoluminescence.
In order to elucidate the nature of M 1 and M 2 , we measured the Raman scattered signal at various temperatures (T). A 1.96 eV excitation was used for the T-dependent measurements because it produces stronger intensity of the M 1 and M 2 peaks. The results are presented in Fig. 2a, where the spectra are displayed with a vertical offset for clarity. We find that M 1 and M 2 are strongly T-dependent compared to the narrow phonon peaks, suggesting a different origin of these features. As T increases, M 1 and M 2 rapidly lose intensity and vanish near T N . In addition, both features soften and broaden considerably as T increases. These trends may be better appreciated by considering the difference spectra shown in Fig. 2b. Here we show I(ω,T) -I(ω, 230 K) with the T 2g (4) phonon subtracted. The reference temperature of 230 K is just above T N . As T increases, the M 1 and M 2 peaks become indistinguishable while the overall distribution of scattered intensity broadens and shifts to lower energy. Above T N , no T-dependent scattering is observed. This temperature dependence indicates that M 1 and M 2 have a magnetic origin.
To confirm the connection with magnetism, we compare the Raman intensity with the magnetic susceptibility χ. In Fig. 2c, we show the integrated intensity of the I(ω,T) − I(ω, 230 K) spectra in the energy region between 75 and 165 meV (open black circles) and compare these with the literature values of χ (filled blue triangles) 4 . Note that both quantities show clear anomalies at T N . The integrated intensity is relatively constant below 0.6 T N before rapidly dropping to a minimum at T N , while χ peaks at T N . Above T N , the magnetic scattering is negligible (we only observe a temperature-independent, flat background) and the susceptibility is slowly varying. Figure 2d displays the T-dependence of the normalized frequency (ω M ), intensity (I M ) and linewidth (Γ M ) of the M 2 peak which was fitted with a Lorentzian function. Above 180 K, M 2 becomes too broad and weak to analyze in this way. The abrupt decrease in intensity of M 1 and M 2 , as well as the rapid changes in the lineshapes and peak locations ( Fig. 2a and Fig. 2d), suggests that these features have a magnetic origin. A recent RIXS study of Cd 2 Os 2 O 7 also identified a feature near 160 meV of magnetic origin that emerges near T N , similar to our findings 5 . Furthermore, the T-dependent Raman scattering of AIAO-ordered Cd 2 Os 2 O 7 is similar to the two-magnon scattering reported in a number of well-studied magnetic systems [22][23][24][25][26] . These observations suggest that the M 1 and M 2 features originate from two-magnon Raman scattering. momentum q = 0 27 . Ignoring magnon-magnon interaction effects, the scattered intensity is therefore related, within a matrix element, to the two-magnon density of states (DOS). To quantitatively connect the observed magnetic signal with the spin wave dispersion, we computed the magnon DOS within LSWT. The magnon dispersions were calculated for the AIAO magnetic ground state, assuming the following Hamiltonian: The terms are the nearest-neighbor exchange coupling (J), the nearest-neighbor DMI (D), and the SIA (A). S i is a spin operator at site i with S = 3/2. For J, D, and A, we used values of 5.1 meV, 1.7 meV, and −5.3 meV, respectively. As discussed in detail later, these values yield good agreement with the Raman data and also closely agree with the results of many-body quantum-chemical calculations 7 . The sign of the DM vector was assumed to be of the direct type (D > 0) since it stabilizes the AIAO state 7,8 . The spin easy axis is denoted by a unit vector n i , which points along the line connecting the centers of the two tetrahedra that adjoin site i.
The LSWT calculations confirm that the broad Raman peaks arise from two-magnon Raman scattering in the AIAO state. As displayed in Fig. 3a, our model calculation shows three spin-wave branches along the high-symmetry Γ-X line. From the dispersions, we evaluated the magnon DOS, displayed in Fig. 3b. Note that the DOS is usually dominated by states near the Brillioun zone boundary. Figure 3c shows a comparison between the energy of the M 1 and M 2 Raman peaks and the magnon DOS with energy scaled by factor of two, which approximates the two-magnon DOS. We find excellent agreement between the experimental spectrum and the calculated result. The overall lineshape and width is satisfactorily reproduced. In particular, a two-peak (T 1 and T 2 ) structure is observed at similar energies to the experimental M 1 and M 2 peaks, while the shoulder M 1 ′ near 121 meV in experiment is also apparent in the calculated DOS (T 1 ′).
With reference to the magnon dispersions in Fig. 3a, M 1 and M 2 may be associated with two-magnon scattering involving the two highest energy branches at the Brillouin zone boundary, respectively. Meanwhile, the shoulder of M 1 at~121 meV likely originates from two-magnon scattering involving the lowest energy branch at the Brillouin zone boundary. It should also be noted that the spin-wave interpretation given here differs from the discussion of the RIXS data presented in ref. 5 , where the magnetic scattering was interpreted as a superposition of single site excitations.
Each term in the spin Hamiltonian (J, D and A) affects the magnon DOS in a distinct manner, as shown in Supplementary  Fig. 3. In combination with the high energy resolution of the Raman technique, these distinct effects allow us to accurately estimate the J, D, and A parameters experimentally from the spectra. An increase of the J parameter increases the overall separations and widths of the DOS peaks, reflecting changes in the bandwidths of the individual magnon branches, while leaving the onset in the DOS unchanged ( Supplementary Fig. 3a, d). An increase in D is observed to shift the peak positions and also reduce their separations ( Supplementary Fig. 3b, e). Finally, an increase in A is seen to increase the energies of T 1 ′, T 1 and T 2 equally, with the splitting between them remaining approximately constant ( Supplementary Fig. 3c, f).Therefore, by comparing the calculated result to the dominant peak positions and onset in the data (Fig. 3c) The discrepancy between our LSWT estimates and the quantumchemical results may be due to the neglect of final-state magnon-magnon interactions in our calculations.
Evidence for spin-charge-lattice coupling. 5d transition metaloxides are characterized by a close coupling between spin, charge, and lattice degrees of freedom 26,28 . To determine whether the spin excitations interact with other degrees of freedom in Cd 2 Os 2 O 7 , we now turn to the phonon features present in the Raman data (Fig. 1a). All Raman modes reveal anomalies near T N . However, we focus on the T 2g (4) phonon near 96 meV, which shows the most pronounced anomalies as well as a distinct asymmetric (Fano) lineshape. Such a spectral lineshape can arise from the coupling of the phonon with a continuum of excitations and is often encountered in the Raman spectra of metals 29 . The ionic motion associated with this mode mostly involves O(1), the oxygen atom at the apex of the OsO 6 octahedron, and is illustrated in Supplementary Fig. 1f. As shown in Fig. 4a, the T 2g (4) mode displays a pronounced Fano asymmetry at T > T N (i.e., 240 K), but becomes comparably symmetric at T < T N (i.e., 115 K). To quantify the observed changes, we have fitted the T-dependent spectra with the Breit-Wigner-Fano (BWF) profile 30 : here I 0 , ω 0 , Γ, and 1/|q| are the intensity, phonon frequency, width, and dimensionless asymmetry parameter of the BWF mode, respectively. As can be seen in Fig. 4a, the Fano fitting adequately describes the T 2g (4) phonon both below and above T N .
The T-dependence of the Fano parameters reveals anomalies near T N (i.e. at T*~0.9T N ). Figure 4b shows that 1/|q| has a complex non-monotonic T-dependence. Above T*, 1/|q| is relatively constant before dropping rapidly to a minimum near 0.8 T N . It then grows as T is reduced further. As shown in Fig. 4 (c), the ω and Γ parameters show related anomalies near T*: Γ drops rapidly while ω 0 reveals a rapid rise. Phonon modes usually show a smooth increase (decrease) in the frequency (width) at low temperatures due to lattice anharmonicity. The T-induced changes of ω 0 and Γ expected from anharmonicity can be evaluated from the anharmonic decay model 31 and are shown as the dashed lines in Fig. 4c. At low temperatures, the ω data show a clear kink at T* while the slope of Γ changes abruptly below T*, clearly deviating from the anharmonic model. Note that the occurrence of the phonon anomalies below T N is not an artifact due to local laser heating: the magnetic scattering intensity introduced in Fig. 2c clearly onsets at T N .
The complex non-monotonic T-dependence of 1/|q| and the anomalies of Γ below T N indicate coupling of the T 2g (4) phonons to both charge and spin degrees of freedom. In the metallic region above T N , 1/|q| remains constant and quite large, indicating that the T 2g (4) phonon is strongly coupled with free carriers. At T < T* (~0.9T N ), 1/|q| is approximately proportional to (T N -T), implying the coupling to spin degrees of freedom as well. At T* < T < T N , the value of 1/|q| may be understood by combining these two coupling contributions. As shown in Fig. 4c, both the ω 0 and Γ parameters reveal anomalies at T*, not at T N . Such behavior suggests that there is a temperature region (i.e. T* < T < T N ) where free carriers coexist with magnetism in Cd 2 Os 2 O 7 , in agreement with a recent optical study 6 .

Discussion
The important features of the magnetic scattering in Cd 2 Os 2 O 7 at T≪T N can be explained using LSWT, implying the existence of well-defined dispersive magnons. Despite its overall success, however, the T-dependence and detailed lineshape of the two- magnon scattering reveal several unusual features that cannot be captured within LSWT. In terms of lineshape, we note that the M 2 peak has a clear tail extending to higher energies than expected from LSWT, which predicts a cutoff at~160 meV (Fig. 3b, c). The discrepancies between the experimental and theoretical curves is probably due to the neglect of final-state magnon-magnon interactions in our calculations 32,33 , which are expected to be strong in the non-collinear AIAO magnetic state. In particular, the asymmetric DOS singularities seen in the calculation are expected to broaden, become more symmetric, and shift to lower energies once magnon-magnon interactions are properly considered. As can be seen in Fig. 2d, the frequency is renormalized by more than 15% at 180 K and the ratios Γ M (180 K)/Γ M (100 K) is about 2.5. At T N , we expect these values to reach 25% and 4, respectively. This behavior may also be attributed to magnon-magnon interaction effects, as these are expected to become more pronounced at elevated T due to thermally-excited magnons. The strong T-dependence of the two-magnon peak energies and linewidths are in accord with the earlier reports of two-magnon scattering for three-dimensional antiferromagnets, and much stronger than the two-dimensional (2D) case (where the frequency of the zone-boundary magnons are renormalized by less than 5% and Γ becomes broadened by about a factor of 1.5 only) 22,34 . An additional factor that may contribute to the above anomalies is Landau damping 8 , which has been suggested in previous reports to be relevant to the AIAO state in the intermediate correlation regime 8,11 . We note that the optical gap in our Cd 2 Os 2 O 7 crystals is only~155 meV at low temperatures 6 , slightly above the energy of the two-magnon scattering. The magnetic excitations may therefore overlap with the electron-hole continuum and Landau damping (electron-magnon interaction) can occur. As a result, the magnetic excitations may decay into electron-hole pair excitations, so the magnon lifetimes and energies may be renormalized. Consequently, Landau damping may contribute to the broadening and renormalization of the two-magnon peaks. As T is increased towards T N , the optical gap softens considerably 6 . Coupling with low-lying charge excitations, as well as magnon-magnon interaction effects, may therefore contribute to The T-dependence of the Fano asymmetry parameter. The experimental data are plotted as black circles. The solid and the dashed lines are guides for the eye. The dashed lines express the contribution of magnetic (green dashed line) and charge (blue dashed line) coupling to 1/|q|, while the red solid line represents the total. c The frequency (ω 0 -black triangles) and the width (Γ-white circles) at various temperatures. The fitted anharmonic decay model is shown in dotted lines. Error bars in b, c represent the standard deviation in the data fitting procedure. d A schematic of the Liftshitz-type MIT, which present simplified band structures expected for the paramagnetic semimetal (P-SM), AIAO ordered semimetal (AIAO-SM), and AIAO ordered insulating (AIAO-I) states. Above T N , the system is a P-SM with the same number of electrons and holes due to the even number of electrons in the unit cell. The filled green and violet regions represent the electron and hole pockets. The electron and hole bands overlap in energy, resulting in a semimetallic state. When T decreases through T N , the emergence of AIAO ordering shifts the electron and hole bands upwards and downwards respectively, gradually annihilating the Fermi surface. With a further decrease in T, the electron and hole pockets disappear and their overlap in energy eventually becomes zero at T*. Below T*, a true energy gap develops between the electron and hole bands, resulting in a robust insulating phase the strong T-dependent damping and softening of M 1 and M 2 that is evident in Fig. 2a, as well as to the high-energy tail of the magnetic scattering discussed above.
The complete disappearance of the magnetic scattering above T N in Cd 2 Os 2 O 7 is also unusual (Figs 2a and 2c). This behavior should be contrasted with the T evolution reported previously for two-magnon scattering in canonical insulating magnets. In threedimensional systems, such as MnF 2 and FeF 2 , the well-defined two-magnon scattering present at T ≪ T N progressively softens, evolving into an intense quasi-elastic response at T ≫ T N [35][36][37] . Persistent scattering at T > T N is also observed in 2D systems, such as HoMnO 3 24 , Sr 2 IrO 4 26 , and K 2 NiF 4 22 , although in these cases the magnetic scattering remains peaked at finite energies due to the presence of short-range 2D spin-spin correlations at experimental temperatures. Above T N , Cd 2 Os 2 O 7 enters a metallic state, as evidenced by direct current transport and optical conductivity studies 4,6,38 . The disappearance of the magnetic scattering at T N may therefore be attributed to strong longitudinal spin fluctuations in the metallic state (in other words, the Os local moment itself is completely washed out) 39 , in line with the exchange-enhanced Pauli-like susceptibility (e.g., non-Curie-Weiss susceptibility) reported by Mandrus et al. above T N 38 .The complete suppression of magnetic scattering above T N , as well as the comparable energies of the magnetic and charge excitations, is suggestive of itinerant magnetism which is valid in the limit of weakly interacting band electrons 40 . This should be contrasted with the success of LSWT, which presupposes welldefined local moments (and localized electrons), in describing the magnetic scattering at T ≪ T N . Taken together, these findings suggest that Cd 2 Os 2 O 7 manifests aspects of both localized and itinerant magnetism, and may therefore be placed in the intermediate electron correlation regime in the sense of ref. 11 . This is broadly consistent with the extended, and hence weaklycorrelated, nature of the 5d Os orbitals 41 .
Having described the magnetic excitations, we now focus on the anomalous temperature dependence of the T 2g (4) phonon. The unusual T-dependence of the T 2g (4) phonon in Fig. 4 can be understood in terms of the Lifshitz-type MIT, recently proposed for Cd 2 Os 2 O 7 2, 42 . It is depicted schematically in Fig. 4d. At T > T N , the system is a paramagnetic semimetal with both electrons and hole bands at the Fermi level (E F ), leading to a large 1/|q| due to electron-phonon coupling. Below T N , the system enters an AIAO-ordered semimetallic state. As the magnetic order develops, the electron and hole bands are repelled from E F and the electronic contribution to 1/|q| (the dashed line in Fig. 4b) is gradually reduced. At the crossover temperature T*~0.9T N , the Fermi surface is entirely removed and 1/|q| rapidly drops towards its minimum value. Concurrently, Γ is reduced and ω 0 is renormalized due to the loss of the electron-hole decay channel (Fig. 4c). At still lower temperatures, the AIAO order continues to develop and the two-magnon scattering intensity (the tail of M 1 and M 2 ) increases (Fig. 2a). The magnetic continuum also couples to the T 2g (4) phonon, causing 1/|q| to rise. Indeed, a linear approximation to the magnetic contribution to 1/|q| (dashed-dot) line in Fig. 4b extrapolates to zero near T N , pointing to the magnetic origin of this component. Our estimate of T*~0.9T N2 04 K agrees well with the 210 K value estimated from the optical conductivity data 6 . Note that the coexistence of free carriers with AIAO magnetism also is predicted to occur in the pyrochlore iridate system, such as in the Weyl semimetal state 12,43 .
Our study has revealed that, in addition to the phonon modes reported in the literature 19 , there exist broad peaks in the Raman response of Cd 2 Os 2 O 7 at higher energy. These broad peaks exhibit an anomalous behavior near the magnetic transition temperature and our analysis indicates that they originate from two-magnon scattering. The good agreement between the observed two-magnon scattering peaks and the calculated spectral shape from LSWT establishes the existence of well-defined spin waves in the AIAO magnetic state of Cd 2 Os 2 O 7 and allows for a quantitative estimation of the effective spin Hamiltonian parameters. We explained certain differences between the magnetic scattering in Cd 2 Os 2 O 7 and in canonical insulating magnets by arguing that Cd 2 Os 2 O 7 should be placed in the intermediatelycorrelated regime.
Our results establish magnetic Raman scattering as a simple and powerful method for exploring the spin dynamics in 5d AIAO pyrochlore magnets, a task that has proven challenging with other techniques. For these systems, Raman scattering has two advantages. First, the high energy resolution of the Raman technique facilitates detecting fine structure in the magnetic excitation spectrum. Second, only a small sample mass is required (useful when only small single crystals or thin films are available). Indeed, pyrochlore iridate thin films are predicted to host topological phenomena and a significantly reduced local moment 44 . Raman scattering is well-positioned to provide insight into such emergent behavior by directly probing the associated magnetic excitations.

Methods
Synthesis and magnetization. Single crystal Cd 2 Os 2 O 7 was grown by the chemical transport method. First, a polycrystalline pellet was prepared from a mixture including 5-10% excess CdO and Os in a sealed quartz tube, under supply of an appropriate amount of AgO as the oxygen source at 1073 K; addition of too much AgO should be avoided, as highly toxic OsO 4 might be produced. Second, the tube was kept in a furnace with a temperature gradient of 1040-1200 K for a week with the pellet at the high temperature side. Single crystals were then grown via a chemical vapor transport process. Magnetization was measured in a Quantum Design MPMS.
Raman scattering. The Raman scattering spectra of the Cd 2 Os 2 O 7 samples were obtained in the backscattering configuration with microprobe LabRAM HR Evolution (Horiba Co.) and NANOBASE XperRam 200 Raman spectrometers. For detection, we used a high-throughput single-stage spectrometer with a grating of 1800 lines per mm. The spectral resolutions are about 2 cm −1 for the LabRAM and about 3 cm −1 for the XperRam. Solid state lasers operating at 633 nm (1.96 eV) and 532 nm (2.33 eV) were used as the excitation sources. The excitation power and beam diameter on the sample surface were~1 mW and~50 µm, respectively. The sample was mounted in a compact temperature stage (THMS600, Linkam) for the T-dependent measurements from 100 to 270 K and a helium closed-cycle cryostat for 15 to 100 K.
Linear spin wave theory. The calculations of the magnon spectra have been performed using LSWT for the AIAO magnetic ground state assuming the Hamiltonian in Eq. (1).
In order to obtain the spin wave expansion about the noncollinear AIAO state, we first rewrite the Hamiltonian in Eq. (1) in terms of local spin variables Here R i is the rotation operator that takes the direction of magnetic ordering at site i and rotates it to the z axis of the global coordinate system. Next, the Hamiltonian is expressed in terms of bosonic operators b i and b þ i using the Holfstein-Primakoff transformation: whereS ± i ¼S x i ± iS y i . Only the terms up to quadratic order in the bosonic operators are retained. Then, we Fourier transform the bosonic operators and obtain the excitation spectrum via a Bogoliubov transformation.
Data availability. The data that support the findings of this study are available from the corresponding author upon request.