France



Conversion of heat into spin current has recently drawn a lot of attention due to its potential usage on heat recovery via the spin Seebeck effect (SSE) [1] as well as fundamental interests including generation of spin super currents [2] and Bose-Einstein condensation of magnons [3]. The underlying mechansim for SSE is understood as a combination of interfacial and bulk (intrinsic) contriubtion. The interfacial SSE is driven by the tempearture drop at the interface between metal and magnetic layer while the bulk SSE is driven by diffusive thermal magnons. In the nonlocal spin transport measurements, the long range exponential decay of thermally generated spin signal was explained solely by the intrinsic SSE [4] while there are several studies showing that there is another decay mechanism in subhundred nanometer scale [5-7]. Here, we study the spatial decay of thermally excited magnon currents inside a thin magnetic insulator by focusing on the short-range behavior in the nonlocal geometry. We compare SSE signal (Δ&lt;sub&gt;1,2&lt;/sub&gt;) on the same device before and after adding a nonmagnetic Al capping layer. The Al capping alters the thermal profile significantly near the heat source, which results in that the nonequilibrium thermal magnon profile deviates from an exponential decay and shows two sign reversals within 1 μm from the heat source. From simulated temperature profiles, we find the vertical temperature gradient also reverses twice within the same length scale in the Al deposited case. The correlation suggests that thermal magnons behave locally at this length scale. Using a phenomenological spin transport model, we calculate the spatial profile of nonequilibrium spin density. The observed short-range behavior can be accounted if the relavant decay length is on the order of subhundred nanometers. Our result shows the existance of the shorter decay length in the nonlocal magnon transport experiments. This suggests that the long-range SSE signal in previous measurements should be attributed to magnons with lower energy.

**References:**

[1] S. R. Boona, R. C. Myers, and J. P. Heremans, Energy &amp; Environmental Science, 7, 885 (2014).&lt;br/&gt;[2] D. A. Bozhko, A. A. Serga, P. Clausen, et. al., Nature Physics, 12, 1057 (2016).&lt;br/&gt;[3] Y. Tserkovnyak,S. A. Bender, R. A. Duine, et. al., Physical Review B, 93, 100402. (2016).&lt;br/&gt;[4] L. J. Cornelissen, J. Liu, R. A. Duine, et. al., Nature Physics, 11, 1022 (2015).&lt;br/&gt;[5] A. Kehlberger, U. Ritzmann, D. Hinzke, et. al., Physical Review Letters, 115, 096602. (2015).&lt;br/&gt;[6] A. Prakash, B. Flebus, J. Brangham, et. al., Physical Review B, 97, 020408. (2018).&lt;br/&gt;[7] J. S. Jamison, Z. Yang, B. L. Giles, et. al., Physical Review B, 100, 134402. (2019).

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/71fcbac32cc3cda92f6d18b1228e05ae.jpg)
Fig.1: Comparison of the experimentally measured local and non-local SSE signals (Δ&lt;sub&gt;1,2&lt;/sub&gt;) at 1 and 2 mA injection and the numerically calculated chemical potential profiles with different input values of decay length λ for YIG/Pt/Si&lt;sub&gt;3&lt;/sub&gt;N&lt;sub&gt;4&lt;/sub&gt; (case A) on a symmetric log scale. The insets show the schematic of the sample structure (bottom left) and temperature profile (top right).

![](https://assets.underline.io/uploads/markdown_image/1/image/898460b298a266d784aeaeab1dbbca16.jpg)
Fig.2: Same plots as Fig.1 for YIG/Pt/Si&lt;sub&gt;3&lt;/sub&gt;N&lt;sub&gt;4&lt;/sub&gt;/Al (case B). The result with λ = 0.1 µm reproduces the measured double crossing as shown, revealing the short range thermal magnon diffusion. The second crossing does not appear anymore when increasing λ to 0.5 or 1 µm. The insets show the schematic of the sample structure (bottom left) and temperature profile (top right).

INTERMAG 2021

 Short-range Thermal Magnon Diffusion in Magnetic Garnet

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Conversion of heat into spin current has recently drawn a lot of attention due to its potential usage on heat recovery via the spin Seebeck effect (SSE) [1] as well as fundamental interests including generation of spin super currents [2] and Bose-Einstein condensation of magnons [3]. The underlying mechansim for SSE is understood as a combination of interfacial and bulk (intrinsic) contriubtion. The interfacial SSE is driven by the tempearture drop at the interface between metal and magnetic layer while the bulk SSE is driven by diffusive thermal magnons. In the nonlocal spin transport measurements, the long range exponential decay of thermally generated spin signal was explained solely by the intrinsic SSE [4] while there are several studies showing that there is another decay mechanism in subhundred nanometer scale [5-7]. Here, we study the spatial decay of thermally excited magnon currents inside a thin magnetic insulator by focusing on the short-range behavior in the nonlocal geometry. We compare SSE signal (Δ1,2) on the same device before and after adding a nonmagnetic Al capping layer. The Al capping alters the thermal profile significantly near the heat source, which results in that the nonequilibrium thermal magnon profile deviates from an exponential decay and shows two sign reversals within 1 μm from the heat source. From simulated temperature profiles, we find the vertical temperature gradient also reverses twice within the same length scale in the Al deposited case. The correlation suggests that thermal magnons behave locally at this length scale. Using a phenomenological spin transport model, we calculate the spatial profile of nonequilibrium spin density. The observed short-range behavior can be accounted if the relavant decay length is on the order of subhundred nanometers. Our result shows the existance of the shorter decay length in the nonlocal magnon transport experiments. This suggests that the long-range SSE signal in previous measurements should be attributed to magnons with lower energy.

**References:**

[1] S. R. Boona, R. C. Myers, and J. P. Heremans, Energy & Environmental Science, 7, 885 (2014). [2] D. A. Bozhko, A. A. Serga, P. Clausen, et. al., Nature Physics, 12, 1057 (2016). [3] Y. Tserkovnyak,S. A. Bender, R. A. Duine, et. al., Physical Review B, 93, 100402. (2016). [4] L. J. Cornelissen, J. Liu, R. A. Duine, et. al., Nature Physics, 11, 1022 (2015). [5] A. Kehlberger, U. Ritzmann, D. Hinzke, et. al., Physical Review Letters, 115, 096602. (2015). [6] A. Prakash, B. Flebus, J. Brangham, et. al., Physical Review B, 97, 020408. (2018). [7] J. S. Jamison, Z. Yang, B. L. Giles, et. al., Physical Review B, 100, 134402. (2019).

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/71fcbac32cc3cda92f6d18b1228e05ae.jpg)
Fig.1: Comparison of the experimentally measured local and non-local SSE signals (Δ1,2) at 1 and 2 mA injection and the numerically calculated chemical potential profiles with different input values of decay length λ for YIG/Pt/Si3N4 (case A) on a symmetric log scale. The insets show the schematic of the sample structure (bottom left) and temperature profile (top right).

![](https://assets.underline.io/uploads/markdown_image/1/image/898460b298a266d784aeaeab1dbbca16.jpg)
Fig.2: Same plots as Fig.1 for YIG/Pt/Si3N4/Al (case B). The result with λ = 0.1 µm reproduces the measured double crossing as shown, revealing the short range thermal magnon diffusion. The second crossing does not appear anymore when increasing λ to 0.5 or 1 µm. The insets show the schematic of the sample structure (bottom left) and temperature profile (top right).

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Einstein-de Haas (EdH) effect is the fundamental phenomenon that the microscopic spin angular momentum is converted to the angular momentum of mechanical rotation. A mechanical torque due to the EdH effect, the magnitude of which is proportional to the time derivative of the magnetization, is difficult to be detected, which keeps its practical application away. However, recent development of microfabrication technology has enabled to sensitively detect the tiny EdH torque using micro-fabricated mechanical resonators [1,2]. These findings show that the EdH effect can be utilized for the new principle of the mechanical torque generation in sub-micron scale device. Moreover, it was demonstrated that the ultrafast demagnetization due to the laser heating excited the transverse strain wave in a Fe film due to the EdH effect, where the timescale and conversion efficiency of the angular momentum transfer were quantitatively estimated [3]. Rayleigh-type surface acoustic waves (RSAWs), the displacement of which oscillates elliptically, have been widely used to excite the spin waves in a ferromagnetic thin film via the magnetoelastic interaction [4]. Recently, as the phenomena based on the angular momentum conversion from the lattice rotation to the magnetization or electron spin, the gyromagnetic spin-wave excitation [5] and the spin current generation in a nonmagnetic metal with a weak spin-orbit coupling [6] were demonstrated. In this study, we demonstrate both acceleration and deceleration of RSAW velocity in the ferromagnetic (FM) film based on the EdH effect. When the spin-wave is gyromagnetically excited by RSAW propagation through the FM film, the EdH torque is generated in the FM lattice as the back action of the spin-wave resonance (SWR) (Fig. 1(a)). As shown in Fig. 1(a), the direction of EdH torque is opposite to the time derivative of the magnetization. We theoretically expect that the transverse velocity of RSAW can be modulated by the EdH torque, resulting in the phase change of RSAW propagation. In the experiment, we successfully observed the phase change of RSAW propagation, whose magnitude and variation were consistent with our analytical prediction. Figure 1(b) shows the schematical experimental setup for measuring the phase change of RSAW. A pair of inter-digital transduces (IDTs) consisting of Ti(3)/Au(30) is fabricated on a piezoelectric LiNbO3 substrate by the electron beam evaporation. The numbers in the parentheses indicate the layer thickness in nanometers. The width and space of the electrode of IDT are 550 nm. The Ni81Fe19 (NiFe) film with a lateral size of 400×400 μm2 is sputtered between a pair of IDTs. By applying a microwave with the fundamental frequency of RSAW excitation into one of IDTs, RSAWs are excited via the piezoelectric effect. The RSAWs propagating through the NiFe film are electrically detected by the other of IDTs using a vector network analyzer (VNA) as the inverse process of the RSAW excitation. Figures 2(a) and 2(b) show the reduced RSAW energy dissipation ΔPnorm and phase difference Δθ, respectively, as a function of external magnetic field swept in the direction parallel to the RSAW wave vector at the RSAW frequency of 1.75 GHz. Steep peaks appear at 4.6 and -4.0 mT in Fig. 2(a), showing that the spin-wave is excited because the values of the resonant field and resonant frequency are matched with the spin wave dispersion of a 20-nm-thick NiFe film. A bipolar change of Δθ is observed in the vicinity of the resonance field of spin-waves. From the angle between the applied external field and RSAW wave vector, it can be seen that the spin-wave is excited via gyromagnetic effect, not the magnetoelastic coupling [5]. The increase and decrease in Δθ can be explained by our analytical model consisting of the elastic motion equation with the EdH torque term. The maximum value of phase change Δθmax is -0.035 rad at 5.0 mT. This value is as large as that in case using the magnetoelastic coupling in a single Ni film [7]. In addition, the order of Δθmax is comparative to the value analytically obtained by assuming a loss-less conversion of the angular momentum. The consistency in Δθmax suggests that the EdH effect is robust in the angular translation from the magnetization to the lattice in the gigahertz regime.

**References:**

[1] K. Harii, et. al., Nat. Commun. 10, 2616 (2019). [2] K. Mori, et. al., Phys. Rev. B 102, 054415 (2020). [3] C. Dornes, et. al., Nature 565, 209 (2019). [4] M. Weiler, et. al., Phys. Rev. Lett. 106, 117601 (2011). [5] Y. Kurimune, et. al., Phys. Rev. Lett. 124, 217205 (2020). [6] D. Kobayashi, et. al., Phys. Rev. Lett. 119, 077202 (2017). [7] R. Sasaki, et. al., Phys. Rev. B 95, 020407 (R) (2017). [8] S. Tateno, et.al., submitted.

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/95a80b47499a8efb662564ebc84f2325.jpg)
Fig. 1 (a) Schematic of the stress based on EdH effect σEdHzx and the EdH torque τEdH in the Ni-Fe lattice. The direction of the EdH torque is opposite to the time derivative of the magnetization. (b) Experimental setup for measuring the phase changeΔθ of RSAW using a VNA. The external field is applied along the RSAW propagation direction.

![](https://assets.underline.io/uploads/markdown_image/1/image/6d3a013484d0f414781f2f3ebf4436f3.jpg)
Fig. 2 The field dependence of (a) ΔPnorm and (b) Δθ at the fundamental frequency of RSAW excitation, respectively. The red solid line in (b) shows the result of the best fit using our analytical model.

 Velocity Modulation of Surface Acoustic Waves via Einstein-de Haas Effect

In recent years, the coupling between the elastic and magnetic domain in magnetostrictive materials has gained strong interest [1]. The magnetoelastic coupling in these materials results in elastic response originating from magnetic excitations and vice versa. At microwave frequencies, this mutual interaction leads to coupling between elastic and magnetic waves, forming magnetoelastic waves. Whereas plane magnetoelastic waves are already studied in bulk materials some decades ago [2-4], the magnetoelastic waves in thin magnetostrictive films gained attention only recently [5,6]. By contrast, many recent spin-wave-based information processing applications employ nanoscale waveguides for information transfer and computation [7]. At these nanoscales, confinement of both the elastic and magnetic waves leads to multiple modes each of which with a specific mode profile and consequently also to confined magnetoelastic waves. The shape of the magnetoelastic field depends on the displacement profile and the shape of the magnetoelastic body force depends on the magnetization profile. As a consequence, it is expected that every mode experiences different magnetoelastic coupling strength. This presents a rather complex multiphysics problem where analytical methods are hard or even impossible, and thus numerical approaches are preferred. Therefore, in this work, we present the development of a novel mumax3 extension that allows the numerical calculation of magnetoelastic waves in scaled waveguides [8]. Furthermore, we present results of magnetoelastic waves in a nanoscale waveguide with static magnetization along the wave propagation direction. The studied system consists of a thin CoFeB waveguide with width of 200 nm and thickness of 20 nm. A weak external field of 5 mT is applied in the longitudinal direction of the waveguide to initiate the static magnetization along this direction. The resonant modes in the structure are numerically found by applying a 5 ps excitation pulses and performing a two-dimensional fast Fourier transform. By comparing the numerical result with the analytical uncoupled dispersion relations of confined elastic and magnetic waves, all modes were identified. The uncoupled resonant waves of this structure consist of confined magnetic spin waves, antisymmetric and symmetric lamb waves and out-of-plane shear elastic waves. Fig. 1a shows the numerically obtained dispersion relations and Fig. 1b shows the overlay with the analytically calculated dispersion relations for uncoupled elastic and magnetic waves. The magnetoelastic coupling leads to the formation of anti-crossings near the reciprocal point where the uncoupled elastic and magnetic dispersion relations would intersect with each other. These anti-crossings identify regions of strong interaction between the elastic and magnetic domain and correspond to pure magnetoelastic waves. The magnetoelastic waves are shown to have different behavior as compared to the pure elastic or magnetic waves. The magnetoelastic wave group velocity is rather unaffected in the quasi-magnetic or quasi-elastic regime whereas it strongly differs close to the anti-crossing. Furthermore, the magnetization and displacement value are shown to take both high values close to the anti-crossing. However, when approaching the quasi-elastic regime there is a very strong decay of the magnetization component of the magnetoelastic wave and vice versa for the displacement component and the quasi-magnetic regime. Lastly, careful analysis of the dispersion relations also shows reciprocal points with weak or even without anti-crossing. The frequency gap formed by the anti-crossing is a good measure of the magnetoelastic coupling strength and thus provides much information. The variation in amplitude of this frequency gap is attributed to the wave confinement and their mode profiles. Every elastic and magnetic mode has its own mode profile and thus also its own magnetoelastic body force and field. Considering these mode dependent body forces and fields together with the mode’s overlap integral allows to identify the strength of the coupling between the different elastic and magnetic waves. The strongest coupling is shown to exist between the odd magnetic modes and symmetric lamb modes and even magnetic modes and anti-symmetric lamb modes. This work has been partially funded by the European Union’s Horizon 2020 research and innovation programme within the FET-OPEN project CHIRON under grant agreement No. 801055. FV acknowledge the financial support from Fonds voor Wetenschappelijk Onderzoek (FWO) under the grant No. 1S05719N.

**References:**

[1] A. D. Kent and D. C. Worledge, Nature Nanotechnol. Vol. 10, p. 187 (2015) [2] C. Kittel, Phys. Rev. Vol. 110, p. 836 (1958). [3] E. Schlomann and R. I. Joseph, J. Appl. Phys. Vol. 35, p. 2382 (1964). [4] P. A. Fedders, Phys. Rev. B. Vol. 9, p. 3835 (1974). [5] Y. Nozaki and S. Yanagisawa, Electr. Eng. Jpn. Vol. 204, p. 3 (2018). [6] S. Bhuktare, A. Bose, H. Singh, and A. A. Tulapurkar, Sci. Rep. Vol. 7, p. 840 (2017). [7] A. Khitun and K. L. Wang, J. Appl. Phys. Vol. 110, p. 34306 (2011). [8] F. Vanderveken, et al., https://github.com/Fredericvdv/Magnetoelasticity_MuMax3.

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/c4a42e298a703a137c4d16ff97d65c5e.jpg)
Figure 1: Dispersion relations of magnetoelastic waves in a 200 nm wide and 20 nm thick CoFeB waveguide. (a) Numerically calculated dispersion relations. The inset shows a magnification of a region near a magnetoelastic gap. (b) Analytically calculated dispersion relations of uncoupled elastic and spin waves superimposed to the numerically obtained results.

 Confined magnetoelastic waves in thin waveguides

The interaction between different types of wave excitation in hybrid systems is usually anisotropic. Magnetoelastic coupling between surface acoustic waves and spin waves strongly depends on the direction of the external magnetic field. However, in the present study we observe that even if the orientation of the field is supportive for the coupling, the magnetoelastic interaction can be significantly reduced for surface acoustic waves with a particular profile in the dirR/S-SAWection normal to the surface at distances much smaller than the wavelength. We use Brillouin light scattering to investigate thermally excited phonons and magnons in a magnetostrictive CoFeB/Au multilayer deposited on a Si substrate – see Fig.1. The experimental data interpretation is based on a linearized model of interaction and finite element method computations[1]. For propagating waves, the coupling requires matching both the frequencies and the wavelengths[2]. This condition can be fulfilled for spin waves (SWs) and surface acoustic waves (SAWs) existing in the same range of frequencies and wave vectors. However, the strength of the magnetoelastic interaction depends on the orientation of the wave vector with respect to the direction of the static magnetic field[3]. Moreover, this interaction is different for different types of SAWs, specifically, Rayleigh-SAWs (R-SAW) and Love-SAWs (L-SAW)[1,4] – see Fig.2. Thus, the coupling is strongly anisotropic and cannot be observed for arbitrary SAWs and SWs, even if their frequencies and wave vectors match. Our study reveals an additional factor limiting the interaction between SAWs and SWs. The SAW/SW coupling proves to require an appropriate profile of the elastic wave near the surface of the magnetostrictve structure, at distances much smaller than the wavelength. For R-SAWs the tangential component of displacement ux can have nodes within the magnetic layer, resulting in a reduction of the net strength of magnetoelastic interaction even if the strain εxx is locally significant. In an L-SAW the displacement uy does not have any nodes (uy changes monotonously in the normal direction). The location of R-SAW nodes depends on elastic properties of the system, specifically, the elastic material parameters of the multilayer and the substrate, and the thickness of the multilayer. We have shown that this additional factor plays a role for some types of surface acoustic waves (R-SAW), while other types (L-SAW) are insensitive to it. We believe that the studies on magnon-phonon interaction in confined geometries (surfaces, cavities) are very promising and can reveal unusual interaction mechanisms. Sample We used naturally oxidized (001) silicon as a substrate supporting the studied [Co20Fe60B20/Au]20 multilayers deposited on top of a 4 nm titanium (Ti) and a 15 nm gold (Au) buffer layers. The multilayers were deposited by magnetron sputtering in argon atmosphere. Method We studied the dispersion relations of thermally excited SAWs and magnetostatic SWs using a six-pass tandem Brillouin spectrometer (Scientific Instrumentsc©TFP2-HC),which ensures a contrast of 1015. A frequency-stabilized diode-pumped solid-state laser (Coherentc©VERDI V5) operating at λ0= 532 nm was used as a source of incident light. The measurements were performed in the 180o backscattering geometry with crossed (p-s)polarization of incident and scattered light for SWs and non-crossed (p-p) polarization for SAWs. Using the finite element method in COMSOL Multiphysics©, we solve numerically the coupled equations of motion for mechanic displacement and magnetization. The CoFeB/Au multilayer is treated as a 60-nm-thick effective magnetic layer, and the CoFeB/Au multilayer together with the Ti/Au buffer as an 80-nm-thick effective acoustic layer on a Si substrate. Acknowledgement The research leading to these results has received funding, hereby gratefully acknowledged, from the National Science Centre, Poland, project No. UMO-2016/21/B/ST3/00452. S. Mies. would like to additionally acknowledge the financial support from the National Science Centre, Poland, project No. UMO-2020/36/T/ST3/00542.

**References:**

 [1] N. K. P. Babu, A. Trzaskowska, P. Graczyk, et al., Nano Lett. (2020) https://doi.org/10.1021/acs.nanolett.0c03692 [2] Y. Hashimoto, D. Bossini, T. H. Johansen, et al., Phys. Rev., Vol. 97, 14040 (2016) [3] L. Dreher, M. Weiler, M. Pernpeintner, et al., Phys. Rev. B 86, 134415 (2012) [4] M. Geilen, F. Kohl, A. Nicoloiu, et al., Appl. Phys. Lett. Vol. 117, 213501 (2020) [5] N.E. Khokhlov, P.I. Gerevenkov, L.A. Shelukhin, et al., Phys. Rev. Applied Vol. 12, 044044 (2019)

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/052c823eb22ae084daf2c19fe75deaf0.jpg)
Fig.1 In the studied system acoustic waves propagate along the surface of the silicon substrate and are mostly concentrated in the CoFeB/Au multilayer cover. The multilayer can be regarded as an effective magnetostrictive medium where surface acoustic waves can interact with spin waves. The anisotropy of magnetoelastic interaction (i.e. the dependence on the orientation f of magnetic field) is different for Love and Rayleigh/Sezawa acoustic waves (L-SAW, R/S-SAW); presented on the left are the respective polar plots of the in-plane component of magneto elastic field.

![](https://assets.underline.io/uploads/markdown_image/1/image/bc1badb1dc20cc3a670ea3ed7a09b463.jpg)
Fig.2 The BLS experimental magnetoelastic dispersion relation measured for magnons (redlines) and phonons (blue lines) with an in-plane applied magnetic field of (a) 30 mT and (b) 50 mT for Φ=0 deg . The dashed shows the regions where the frequencies of fundamental spin wave fundamental mode (F-SW) and L-SAW or R-SAW are agreed. The interactions is seen for L-SAW only. (c) For Φ=45 deg observe the lack of R-SAW/F-SW interaction, which cannot be explained based on the interaction anisotropy (see hme,‖(Φ) for R-SAW in Fig.1). The R-SAW/F-SW interaction is suppressed to zero due to the presence of a nodal line for the εxx component of the strain tensor, which averages to zero the magnetoelastic coupling.

 The interaction between surface acoustic waves and spin waves: the role of anisotropy and spatial profiles of the modes

Modern quantum computing architectures are built to provide low-error environments within which to perform the unitary operations that form the bases of quantum computations. These low-error environments necessary for successful quantum computation require use of complex structures that make large-scale implementation difficult, leading to the investigation of coupled magnon-photon systems [1-6] that can achieve strong coupling rates (&gt; 100 MHz) as a potential platform for hybrid quantum computing architectures. Such coupled magnon-photon systems benefit from the magnetic field tunability of the resonant magnon frequency, where dynamic tuning of resonant magnon frequencies with a pulsed magnetic field at rates comparable to or less than the order of the magnon-photon energy exchange time can realize unique operations not possible with static tuning [7-8]. Previously, we analyzed this problem numerically and found that a parabolically shaped pulsed magnetic field profile can realize the coherent exchange of quantum data and the generation of entanglement by changing the curvature λ and maximum frequency Δ of the parabolic profile [8]. That is, in the same physical structure, depending on the shape of the pulsed magnetic field, different unitary magnon-mediated quantum gates can be realized [8]. Here, we consider an analytical approach to study this system. Namely, we consider a hybrid magnon-photon system, consisting of two photonic resonators having degenerate frequencies ωp and one magnonic resonator with a dynamically-tuned resonance frequency ωm(t). The photonic resonators are not directly coupled with each other but are both coupled with the magnonic mode with the coupling rate κ. We consider a simple analytically-solvable interaction protocol in this hybrid system, which can be experimentally realized with rectangular magnetic field pulses of sufficiently large magnitude. We assume that initially (t&lt;0) the frequency difference │ωm–ωp│&gt;&gt;κ and interaction between the subsystems can be ignored. At t=0 the magnonic mode frequency ωm(t) is brought within the efficient interaction interval Δ=ωm–ωp∼κ and is held constant for the duration T. After t=T, the magnonic frequency is once again moved out of the photonic resonance region and any interaction between the subsystems stops. Depending on the control pulse parameters Δ and T, different behaviors of the hybrid system can be realized. Of particular interest is the situation, in which the magnonic and photonic subsystems stay completely decoupled after the action of the control pulse. Such a case corresponds to a unitary operation on the photonic modes, realized through the indirect magnon-mediated coupling, and is of great importance for practical applications of magnonic resonators in quantum computing systems. Using our model, we derived a simple analytical condition of realizing unitary magnon-mediated operations, namely, for each detuning Δ there exist an infinite series of pulse durations Tn(Δ)=2nπ/(8κ2+Δ2)½ providing unitary conditions (here, n is a positive integer). The resulting effect of the magnon interaction on the photonic subsystem, in this case, can be described by 2×2 unitary matrix Un=Uei(nπ/2–Tn(Δ)Δ/4) relating photonic states before and after the pulse, which has components: U11=ei2πcos(θn), U12=eiπ/2sin(θn), U21=–e–iπ/2sin(θn), U22=e–i2πcos(θn) Here θn=nπ/2–Tn(Δ)Δ/4 has the meaning of inter-mode energy exchange angle. For example, for θn=π/2+mπ (m is an integer number) a complete exchange of two photonic states is achieved, while θn=π/4+mπ describes 50% mixing behavior that allows one to entangle the two photonic modes. The obtained results allow one to select pulse parameters realizing the desired unitary operation and, also, to analyze the limitations on the performance of the proposed magnon-mediated gates. Thus, it is clear that the simple rectangular pulse cannot realize all possible unitary gates since the matrix Un depends only on one continuous parameter (θn), while the general 2×2 unitary matrix has 4 independent parameters. On the other hand, this pulse profile is sufficient to achieve an arbitrary exchange angle θn. The shortest pulse duration for which a complete exchange (θn=π/2) is possible is Tmin=π/(κ√2)and is realized at exact resonance Δ=0. Our results, also, show a possibility to realize magnon-mediated unitary gates working in off-resonance conditions │Δ│≥κ. For example, θn=π/2 gate can be realized with Δ=18(2/19)½κ and T10=(19/2)½π/κ. While such off-resonance operations require longer interaction times, their advantage in comparison to resonance-type operations is that the magnonic and photonic subsystems remain only weakly coupled throughout the whole process. This may lead to weaker decoherence of the quantum photonic subsystem caused by spin-lattice relaxation processes in the magnonic resonator. In general, n-th unitary branch Tn(Δ) has n different detuning values Δ, for which a given exchange angle θn (up to multiplies of π) is achieved, which leaves a lot of space for optimization of practical magnon-mediated unitary gates. In summary, we proposed a simple model of magnon-mediated interaction in dynamically-tuned hybrid magnon-photon quantum systems. We derived analytically the conditions under which such interaction results in a unitary operation on the photonic subsystem and obtained expressions for the parameters of the control pulse necessary for achieving the desired operation. Our results can be used for estimation and optimization of performance parameters of practical hybrid magnon-photon systems.

**References:**

[1] H. Huebl, C. W. Zollitsch, J. Lotze, et al., Phys. Rev. Lett., vol. 111, no. 127003, 2013. [2] Y. Tabuchi, S. lshino, T. Ishikawa, et al., Phys. Rev. Lett, vol. 113, no. 083603, 2014. [3] X. Zhang, C.-L. Zou, L. Jiang, et al., Phys. Rev. Lett., vol. 113, no. 156401, 2014. [4] Y. Tabuchi, S. lshino, A. Noguchi, et al., Science, vol. 349, no. 6246, pp. 405-408, 2015. [5] Y. Li, T. Polakovic, Y.-L. Wang, et al., Phys. Rev. Lett., vol. 123, no. 107701, 2019. [6] J. Hou and L. Liu, Phys. Rev. Lett., vol. 123, no. 107702, 2019. [7] C. Trevillian and V. Tyberkevych, FE-09, Digests of the Intermag Conference, 2020. [8] C. Trevillian and V. Tyberkevych, Q2-07, Abstracts of the 65th Annual Conference on Magnetism and Magnetic Materials, 2020.

**Images:**

 Analytical Model for Unitary Magnon-Mediated Quantum Gates in Hybrid Magnon-Photon Systems

We theoretically investigate the topological aspects of the magnon-phonon hybrid excitation in a simple two-dimensional (2D) square-lattice ferromagnet with perpendicular magnetic anisotropy [1]. Several distinguishing features of our model are as follows. Our model is optimized for atomically thin magnetic crystals, i.e., 2D magnets. The recent discovery of magnetism in 2D van der Waals materials opens huge opportunities for investigating unexplored rich physics and future spintronic devices in reduced dimensions [2,3]. In our 2D model, we ignore the nonlocal dipolar interaction, which is not a precondition for a finite Berry curvature in 2D magnets. Moreover, the Berry curvature we find requires neither a special spin asymmetry such as the Dzyaloshinskii-Moriya interaction (DMI) nor a special lattice symmetry: Our 2D model description is applicable for general thin-film ferromagnets. Therefore, we show that even without such long-range dipolar interaction, DMI, or special lattice symmetry, the nontrivial topology of a magnon-phonon hybrid can emerge by taking account of the well-known magnetoelastic interaction originates from the magnetocrystalline anisotropy. Because the magnetocrystalline anisotropy is ubiquitous in ferromagnetic thin-film structures, our result does not rely on specific preconditions and thus is quite generic. Furthermore, we show that the topological structures of the magnon-polaron bands can be manipulated by effective magnetic fields via topological phase transition. We uncover the origin of the nontrivial topological bands by mapping our model to the well-known two-band model for topological insulators [4], where the Chern numbers are read by counting the number of topological textures, called skyrmions, of a certain vector in momentum space. In this picture, the magnon-phonon hybridization induces the chiral texture of the momentum space vector. As an experimental probe for our theory, we propose the thermal Hall conductivity [Fig. 2].

**References:**

[1] G. Go et al., Topological Magnon-Phonon Hybrid Excitations in Two-Dimensional Ferromagnets with Tunable Chern Numbers, Phys. Rev. Lett. 123, 237207 (2019). [2] C. Gong et al., Discovery of intrinsic ferromagnetism in two-dimensional van der Waals crystals, Nature (London) 546, 265 (2017). [3] B. Huang et al., Layer-dependent ferromagnetism in a van der Waals crystal down to the monolayer limit, Nature (London) 546, 270 (2017). [4] B. A. Bernevig, T. L. Hughes, and S.-C. Zhang, Quantum spin Hall effect and topological phase transition in HgTe quantum wells, Science 314, 1757 (2006).

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/436ed988646e642bcb99ed25391293f6.jpg)
Fig. 1. (a) The schematic illustration of the magnon and phonon system. The ground state of the magnetization is given by the uniform spin state along the z-axis (red arrow). (b) The Chern number of our magnon-phonon hybrid system. H represents the effective magnetic field including the anisotropy field and the external magnetic field. Band dispersion (c) without the magnon-phonon interaction and (d) with the magnon-phonon interaction.

![](https://assets.underline.io/uploads/markdown_image/1/image/2bc284e0ccbc6784cc3e8d6d0786fed4.jpg)
FIG. 2. (a) Dependence of thermal Hall conductivity on the effective magnetic field Heff and with different temperatures T using the parameters in the main text. (b) Dependence of the Chern number on the effective magnetic field Heff using the parameters in the main text.

 Topological magnon-polaron in a two-dimensional ferromagnet

Acoustically-driven ferromagnetic resonance (ADFMR) gained interest in 2012 as Dreher et al. (1) developed it as a powerful and versatile method of examining complex magnetoacoustic interactions. While initial studies established the technique, the physical mechanisms behind the coupling must be thoroughly understood if ADFMR is to be exploited in next-generation microwave communications devices. In particular, the nonlinearity of ADFMR driven at high powers (2) is not well characterized, which may result in unwanted or unpredicted behavior when devices become optimized. To address this aspect, we produce ADFMR devices using curved interdigitated transducers (IDTs), in contrast to the straight IDTs that are typically used. Like an optical lens, these IDTs are engineered to focus acoustic energy towards a region smaller than the IDTs themselves. In this way, acoustic and magnetic amplitudes in a small region in the center of the device may be driven much higher than was previously possible, allowing examination of nonlinear processes such as Suhl instabilities. This may also produce an avenue for improved magnetoacoustic coupling, as well as further device miniaturization. Our devices are produced in much the same way as previously described (2), using aluminum split-finger IDTs and a 20-nm thin-film nickel layer grown on a y-cut lithium niobate (LiNbO3) substrate. We examine a device using a scanning acoustic-wave imaging interferometer similar to that used in Ref. (3). A 785-nm laser is split into signal and reference paths using an acousto-optic modulator operated at 40 MHz. The signal component is focused onto the device with a 10X objective lens. The beams are then recombined and the interference between them is recorded using a lock-in amplifier. Meanwhile, the ADFMR device is driven at its fundamental frequency 284 MHz or a higher odd harmonic. The DC photodiode signal is simultaneously recorded as a reference image (Fig. 1a), and follows the reflectivity of the scanned spot, showing the exact positions of the metallic nickel and aluminum surfaces. The vibration of the probed spot, downmixed to the range of the lock-in, is shown in Fig. 1b. Here, the gaussian-like curve of the focused SAWs is clearly visible as they converge to a high-amplitude region near the center of the device. Extracting a longitudinal segment of this signal allows us to see the oscillatory behavior in Fig. 1c. These oscillations indicate a standing wave with wavelength v/f = 12 µm (v = 3488 m/s is the Rayleigh velocity of SAWs in the LiNbO3 and f = 284 MHz is the driving frequency), as the output of the device is reflected back towards the input. To quantify the power convergence, transverse slices were taken near the center and fitted with the lorentzians shown in Fig. 1d, using the fitting parameters in Fig. 1e. Near the center (X ≈ 20.7 mm), the amplitude reaches a value of nearly 5 times greater than it is near the IDTs, as the width shrinks to a minimum of 22 µm, demonstrating that the focused IDTs significantly increase the energy density in a small region. ADFMR measurements on a focused IDT device show extremely power-dependent behavior. The linear regime is accessed with a -15 dBm driving field (Fig. 2a), where the shape is independent of power. However, with only +15 dBm of input power (Fig. 2b) the absorption lobes begin to shift towards lower field, and with a weaker maximum absorption. At +25 dBm of input power (Fig. 2c) the lobes shift even further and are much weaker in comparison. These results are a clear indication that a nonlinear power regime is accessed with modest input powers with the assistance of the curved IDTs, dramatically concentrating acoustic energy density. *This material is based on work supported by the Air Force Office of Scientific Research under project number FA9550-20RXCOR074

**References:**

1. L. Dreher, M. Weiler, M. Pernpeintner, H. Huebl, R. Gross, M. S. Brandt, and S. T. B. Goennenwein, “Surface acoustic wave driven ferromagnetic resonance in nickel thin films: Theory and experiment,” Physical Review B, vol. 86, no. 13, p. 134415, 2012. 2. D. Bas, P. Shah, M. McConney and M. Page, “Optimization of acoustically-driven ferromagnetic resonance devices,” Journal of Applied Physics, vol. 126, no. 11, p. 114501, 2019. 3. Z. Shen, X. Han, C. L. Zou, and H. X. Tang “Phase sensitive imaging of 10 GHz vibrations in an AlN microdisk resonator,” Review of Scientific Instruments, vol. 88, No. 12, p. 123709, 2017.

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/cf30be12a3755d154f36adeba3fe0211.jpg)
Figure 1. Interferometric imaging of microwave surface acoustic waves on a device. (a) Reflectivity map of the device in arbitrary units, scanned with 5-µm steps, highlighting the curved interdigitated transducers (IDTs), thin film of nickel (Ni), and substrate of lithium niobate (LiNbO3). (b) Interferometric acoustic wave imaging showing the amplitude of surface vibrations in arbitrary units, demodulated at the fundamental frequency of the IDTs (284 MHz) after downmixing. (c) Line scan indicated by the blue dashed line in (b), fitted with a sinusoid of period 12 µm, which corresponds to the period of standing waves in LiNbO3 at 284 MHz. (d) A series of lorentzian fits along the Y-direction for the data indicated by the dashed orange box in (b). (e) Fitting parameters width and height for the curves in (d).

![](https://assets.underline.io/uploads/markdown_image/1/image/43305569f2e8ce46063c1c55933a4975.jpg)
Figure 2. Normalized ADFMR signal in a focused IDT device. Driving field is (a) -15 dBm, (b) +15 dBm, and (c) +25 dBm at 864 MHz.

 Focused SAWs enhance nonlinearity in ADFMR

Magnetoelectric multiferroics, which simultaneously stabilize magnetic and polar static orders, have been predicted to present unusual dynamical magnetoelectric effects (ME). The relatively large magnitude of this dynamical ME response as well as its strong interac-tion with light is extremely attractive for potential applications among others are multifunctional spin-based memories or optical switches. The dynamical ME effects under consideration in this presentation, are characterized by the existence of an electro-active magnetic excitation called electromagnon. The electroactivity of electromagnons was first observed in type II multiferroics, where ferroelectricity is magnetically induced. In orthorhombic RMnO3 and RMn2O5(R=Tb, Y) families, both THz [1] and Raman [2] spectroscopies showed that this mode can be excited by means of the electric field of the light. The demonstration of the complementary magnetic nature of this excitation has been the prerogative of inelastic neutron scattering (INS) [3]. Sincethen, electromagnons have also been reported in Type I multiferroics hexagonal RMnO3 [4], in BiFeO3 and even in a paraelectric compound Ba2Mg2Fe12O22. To describe this unusual property, different mechanisms were proposed, in particular for the manganites families. These models basically rely on the very same magnetoelectric coupling which accounts for the static properties: lattice vibrations alter the exchange couplings or anisotropies which in turn affect the magnon spectrum. In helical magnetic systems for instance, where the multiferroicity originates from Dzyaloshinskii-Moriya Interac-tion (DMI), the same DMI has been proposed to explainthe origin of the electromagnon [5]. Although later refuted in DyMnO3, such DMI based scenario seems to be at play in CuO. Other propositions are based on Exchange-Striction (ES) [6], and couple a polarlattice mode to the magnon spectrum [1]. So far, these models have been consistent with experimental results in TbMn2O5 [3]. These interpretations tend to reduce the definition of the electromagnon to a hybrid magnon-phonon mode, or, as proposed in ErMnO3, to a mixing between a magnon and an electro-active rareearth crystal field transition [4]. In this presentation we question this issue and support the idea that electroactivity can be a purely electronic phenomenon. The RMn2O5 multiferroic compounds crystallize in the polar Pm space group [7] but present quasi-symmetries of the paraelectric Pbam space group. Along the c direction, the structure is composed of chains of Mn4+O6 octahedra, separated by layers of R3+ or Mn3+ ions. In the (a,b) plane, zig-zag chains of Mn4+O6 octahedra and Mn3+O5 square-pyramids run along the a axis and are stacked along b. GdMn2O5, like the other members of the family, shows an Incommensurate Magnetic ordering (ICM) belowTN=38 K, with a magnetic propagation wave vector k1= (½,0,0.28). Then, below Tc=32 K, the magnetic order becomes commensurate with a propagation wave vector k2= (½,0,0), accompanied by the largest electric polarization known in type II multiferroics [8]. This strong electric polarization has been ascribed to two cooperative ES mechanisms [6]. As all members of the series, the electric polarization is mainly oriented along the b axis [8] even if few studies have recently suggested the existence of small additional components along the a and even the c directions. The dynamical properties of this compound have been studied by means of IR and INS on high quality single crystals. In this presentation, we will mainly focus on the demonstration and characterization of an electromagnon present in the compound GdMn2O5. More precisely, the IR measurements allowed us to demonstrate the existence of an excitation below the TN, at an energy of 35cm-1 at 5K, which is electroactive because it is sensitive to the direction of the electric field of light (see fig. 1). The temperature tracking shows that this excitation disappears above the TN, which shows the magnetic origin of this excitation. Moreover, INS measurements have allowed us to measure the excitation in the center of the magnetic zone (½,0,0) (see fig. 2), but also to measure its dispersion, which we have been able to interpret through simulations based on the «Holstein-Primakov» representation, which shows that this excitation is an electroactive spin wave, and thus an electromagnon. Polarized INS measurements (see fig. 2) allowed us to discriminate between the nuclear and magnetic contributions, and to show that this excitation is purely magnetic, thus excluding the hypothesis of a coupling with a phonon. Finally, the presence of a crystalline field level was excluded by both INS and IR measurements, and by ab-initio calculations. Consequently, the electroactivity of this electromagnon is of a different nature than those observed in the past, and seems to have a purely electronic origin.

**References:**

a[1] A. B. Sushkov, R. V. Aguilar and S. W. Cheong, Phys. Rev. L 98, 3 (2007) [2] P. Rovillain, Cazayous and A. Sacuto, Phys. Rev. B 86, 014437 (2012) [3] S. Petit, V. Balédent and P. Foury-Leylekian, Phys. Rev. B 87, 1 (2013) [4] L. Chaix P. Roy and V. Simonet, Phys. Rev. L 112, 1 (2014) [5] H. Katsura, A. V. Balatsky and N. Nagaosa, Phys. Rev. L 98, 1 (2007) [6] V. Balédent, M. B. Lepetit, and P. Foury-Leylekian, Phys. Rev. B 97, 5 (2018) [7] V. Balédent, S. Chattopadhyay and P. Foury-Leylekian, Phys. Rev. L 114, 117601 (2015) [8] B. Khannanov, E. I. Golovenchits and V. A. Sanina, J.Phys.: Conf. Series 572, 12046 (2014)

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/bd2e503f7f47b740d4f6a1478408d52f.jpg)
Inelastic polarized neutron scattering at Q=(3/2,0,0) performed at THALES@ILL for 15 K. NSFx, SFx SFy and SFz stands for Non-Spin-Flip, Spin-flip with polarisation parallel to a, c and b crystallographic axis respectively.

![](https://assets.underline.io/uploads/markdown_image/1/image/bd2ea5b97909165cb1bda30c587ddab0.jpg)
Absorbance at 5 K with a reference at 40 K in Gd for e//a h//b & e//b & h//a (electric and magnetic field of the light) with respect to crystallographic axis.

 Study of a new type of excitation in the multiferroic magnetoelectric compound GdMn2O5, the electromagnon

Integrated magnetic devices show great potential for applications of radiofrequency and microwave integrated circuits, such as chip-scale magnetic inductors, bandpass filters, phase shifters, etc. [1, 2]. Recently, many researchers have been vastly concentrating on ferromagnetic/insulator sandwich structure for high-frequency applications. This thin film stack reduces the eddy-current as well as the out-of-plane anisotropy [3, 4], reducing the energy dissipation in form of heat. The FeGaB has soft magnetic nature, a large magnetostriction coefficient, and saturated at lower magnetic fields. Due to the low loss property of Al2O3 in microwave frequency, we have attempted to obtain low damping (α) and narrow linewidth through the FeGaB/Al2O3 thin film stack and characterize the ferromagnetic resonance (FMR) by utilizing Cryo-FMR. In this article, Ta (5)/ [FeGaB (15)/ Al2O3 (3)] n/Ta (3) / Al2O3 (2) thin-film stack are deposited by DC and RF sputtering on Si substrate, where n indicates the number of multilayer (n=1, 5, and 10) and parenthesis indicates thickness in nanometers. Fig.1 (a) shows normalized magnetic loop of the thin film stack, which reveals that the magnetic saturation moment has increased for increasing layer thickness. The coercive filed (Hc) has a low value below 3 Oe as indicated in Fig.1 (b). The dynamical magnetic properties have been studied using NanOsc Instruments Cryo-FMR in VersaLab system with temperature variation 300-100 K and exciting frequency from 2 to 20 GHz. The ferromagnetic absorption spectrum is shown in Fig.2 (a). The absorption spectrum contains the perpendicular standing spin wave (PSSW) modes for n=5 and n=10 in addition to FMR mode. The linewidth of absorption spectrum is fitted with dH= dH0 + αf/γ, (d=delta) to obtain damping factor (α), and inhomogeneous line width (dH0)[5]. The thin film stack with n=1 has a narrow linewidth and a low damping factor compared to other two thin film stacks, as shown in Fig.2 (b). When the temperature decreases, the damping factor has decreased for n=1, but increased for n=5 and n=10 due to defects arise for lowering the temperature. The Fig.2 (c) shows temperature dependent inhomogeneous linewidth for thin film stacks. As the temperature lowering to 100 K, the dH0 has increased for n=1 and n=10 thin film stacks, whereas decreased for n=5. The dH0 is lower for n=1 and larger value for n=5. The frequency dependence of FMR fields (Hres) plot provides effective magnetization (Meff) and magnetic anisotropy, when the plot has fitted to the Kittle equation. The Meff has a lower value for n=10 than other two stacks. The Meff has increased in all thin film stack as the temperature decreases. Since the absorption of the spectrum shows the PSSW modes in additional to FMR mode, the exchange magnetic fields (Hex) have been calculated by the subtraction method [6]. The plot of Hex and number of PSSW mode has provided the spin-wave exchange stiffness (D). The D values are 13.6615 and 10.7371 x10-18 Tm-2 for n=5, and n=10, respectively at 300 K. As the temperature decreases to100 K, the D has decreased for n= 5 thin film stack whereas increased for n=10. The temperature-dependent stiffness is following the T2 model in a linear form, and it suggests the existence of the electron–magnon interaction in this thin film stack. In order to calculate the constant of spin-wave exchange stiffness (A), saturation magnetization of thin film stack has multiplied with the exchange stiffness. At 300K, the A values are 7.1108, and 5.3213 pJ/m, respectively. In summary, we have deposited multilayer film stack of Ta (5)/ [FeGaB (15)/ Al2O3 (3)] n/Ta (3) / Al2O3 (2) onto Si substrates, and studied magnetodynamic (ferromagnetic resonance) properties with multilayer thickness and temperature dependence. The magnetic properties of thin film stack reveal that saturation magnetic moment has enhanced for increasing thickness of thin film stack, and Hc has obtained below 3 Oe. Therefore, the multilayer thin film stacks have the most significant for microwave applications. The dynamic magnetic properties suggest that the lowest damping and narrow linewidth are obtained for n=1 thin film stack compared to other thin film stacks. The FMR absorption spectrum of thin film stack with n=5, and n=10 show the PSSW modes in addition to the FMR mode. Consequently, the spin-wave exchange stiffness has been extracted. The temperature-dependent stiffness has followed the T2 model, which provides the strong presence of electron–magnon interaction in materials. The constant of spin-wave exchange stiffness has calculated with help of saturation magnetic moment and the exchange stiffness. Hence, the multilayer thin film stacks can be employed for microwave device applications.

**References:**

[1] Y. He, et.al,” IEEE Trans. on Magn., vol. 54, no. 9, pp. 1-4, 2018. [2] T. Wu, et.al, IEEE Magn. Lett., vol. 2, pp. 6000104-6000104, 2011. [3] X. Xing, et.al, IEEE Trans. on Magn., vol. 47, no. 10, pp. 3104-3107, 2011. [4] T. Wu, et.al, Appl. Phys. Lett., vol. 98, no. 1, pp. 012504, 2011. [5] K. Yadagiri, & T. Wu,J. Magn. Magn Mater., vol. 515, pp. 167277, 2020/12/01/, 2020. [6] K. Yadagiri, et.al, IEEE Trans. on Magn., vol. 57, no. 1, pp. 1-7, 2021.

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/958b8bb25594b09daba2dc26ecee751d.jpg)
Fig.1 (a) Normalized M-H loop for Ta (5)/ [FeGaB (15)/ Al2O3 (3)] n/Ta (3) / Al2O3 (2); n=1, n=5 and n=10, inset of Fig.1 (a) shows the Hc of thin film stacks, (b) coercive field HC (Oe) and Mr/Ms as a function of number of multilayer (n).

![](https://assets.underline.io/uploads/markdown_image/1/image/f01c6f6422c349af3f382d094dd43e8f.jpg)
Fig.2 (a) The absorption spectra of Ta (5)/ [FeGaB (15)/ Al2O3 (3)] n/Ta (3) / Al2O3 (2); n=10 at 300 K with exciting frequencies 2-20 GHz; inset of figure shows absorption spectra at 15 GHz with FMR mode and PSSW modes, (b) the damping factor (α) versus termeapture for thin film stack, and (c) the inhomogeneous linewidth (deltaH0) as a function of temperature for Ta (5)/ [FeGaB (15)/ Al2O3 (3)] n/Ta (3) / Al2O3 (2).

 Magnetodynamic properties of FeGaB/Al2O3 multilayer thin film stack for microwave applications

Magnetic materials are at the hearts of billions of high frequency communication devices and on-chip integration of magnetic microwave devices is of paramount importance for efficient utilization of the huge electromagnetic (EM) spectrum beyond 5G. Magnonics – a sub-field of spintronics – employs magnetic waves and oscillations in magnetic thin films and patterned nanostructures for processing GHz to sub-THz EM signal [1-2]. Magnetic ferrites are conventionally used in such magnetic microwave devices. However, due to the need for external bias magnetic field and incompatibility with complementary metal oxide semiconductor (CMOS) process, ferrites are not suitable for miniaturized microwave components. On the other hand, metallic magnetic thin films and nanostructures have great potential for efficient engineering of microwaves. Although, the need for bias field remains a bottleneck. We have been working on solutions where the requirement of the bias-field is absent. We have successfully demonstrated several strategies for achieving such device architecture by utilizing self-biased nanomagnets with reprogrammable remanent states which are associated with distinct magnetization dynamics [2-11]. To illustrate reconfigurable microwave properties, we have shown in Fig 1 as an example, a pair of dipolarly coupled rhomboid nanomagnets (RNMs). Two different remanent states (↑↑ and ↑↓) are obtained by utilizing a simple field initialization (HI) scheme: applying a saturating field along short and long axes of the RNMs with subsequent removal of the field (Fig. 1(a)). Due to different distributions of the stray fields for the two remanent states, the effective fields (Fig. 1(b)) are different which manifest in the shift of the microwave spectra for the two remanent states. Measurement of microwave properties from a single isolated nanomagnetic pair was obtained by using micro-focused Brillouin light scattering (micro-BLS) experiment (Fig. 1(c)) and the micro-BLS spectra are shown in Fig. 1(d). This strategy for reconfigurable magnonic responses is expanded to 2D arrays of the RNMs for different magnetic configurations: antiferromagnetic-type and ferrimagnetic-type artificial magnonic crystals. The maximum amount of the shift in the microwave responses is achieved by using multilayer isolated as well as dipolar-coupled networks of RNMs. Beyond, RNM shape, we have also demonstrated reconfigurable microwave operation based on other strategic shapes with multiple remanent states, such as arrow-, C-, L- and S-type nanomagnets and zigzag nanowires. Furthermore, we emphasize that such self-biased nanomagnets are also suitable for magnonic device applications where the propagation and gating of magnons – quanta for spin waves – are of primary interest. Conventionally, a large bias magnetic field is used in order to satisfy an orthogonal orientation between spin wave propagation and magnetization direction for efficient transmission characteristics (known as surface geometry or Damon-Eshbach mode). The need of such bias field hinders device integration on-chip for magnonic waveguides. Therefore, we have proposed and demonstrated a self-biased magnonic waveguide based on dipolar-coupled but physically separated chain of RNMs (Fig. 2). A prototype of such magnonic devices is shown in Fig. 2(a) where a microwave antenna (input) excites the spin waves and the spin waves are detected using micro-BLS technique with a focused laser spot (output). In order to gate the spin wave propagation, we have flipped a RNM in the waveguide and it is marked as ‘gate’ in the scanning electron microscopy (SEM) image (Fig. 2(b)). Such waveguide design enables one to have two different remanent states: ferromagnetically ordered (FO) and FO with a defect (FO*) when field initialized (same scheme as mentioned above) along the width and the length of the waveguide, respectively. FO and FO* remanent magnetic states are shown in Fig. 2(b) using magnetic force microscopy (MFM) images. Gating of the spin wave propagation has been shown by plotting 2D spatial profiles of the spin wave intensities using micro-BLS technique which clearly indicate gated magnon flow for the FO* state in comparison to the FO state. Thus, one can also achieve binary gating of output signal amplitude using such self-biased nanomagnetic waveguide which is remarkable as it also eliminates the need for bias field. In this presentation, we would like to emphasize the need for bias-free reconfigurable magnonics along with recent developments and future roadmap.

**References:**

[1] A. Haldar, C. Tian and A. O. Adeyeye, Sci. Adv. 3, e1700638 (2017). [2] A. Haldar, D. Kumar and A. O. Adeyeye, Nat. Nanotech. 11, 437 (2016). [3] A. Haldar and A. O. Adeyeye, ACS Nano. 10, 1690 (2016). [4] A. Haldar and A. O. Adeyeye, Appl. Phys. Lett. 108, 192404 (2016). [5] A. Haldar and A. O. Adeyeye, Appl. Phys. Lett. 108, 022405 (2016). [6] A. Haldar and A. O. Adeyeye, J. Appl. Phys. 123, 243901 (2018). [7] K. Begari and A. Haldar, J. Phys. D: Appl. Phys. 51, 275004 (2018). [8] K. Begari and A. Haldar, J. Phys. D: Appl. Phys. 52, 335003 (2019). [9] K. Begari and A. Haldar, J. Phys. D: Appl. Phys. 53, 455005 (2020). [10] A. Haldar and A.O. Adeyeye, Appl. Phys. Lett. 116, 162403 (2020). [11] A. Haldar and A. O. Adeyeye, J Appl. Phys. 128, 240902 (2020).

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/d84bb5df54b8e122952d84e6e7237690.jpg)
Figure 1: (a) Reprogrammable remanent states (X- and Y-state) of a RNM network. (b) Stray field distributions showing difference in the effective field for the two remanent states. (c) Measurement scheme from a single RNM network using micro-BLS technique. (d) Reconfigurable microwave responses for the two different remanent states.

![](https://assets.underline.io/uploads/markdown_image/1/image/408cd838fb91485f6c26689a83c74bc1.jpg)
Figure 2: (a) Propagating spin wave measurement scheme from a RNM chain using micro-BLS technique. (b) Logic device based on dipolar coupled RNM chain is shown in the SEM image. MFM images show the two different magnetic states (FO and FO*). Logic operation is demonstrated by using 2D spatial maps of the spin wave propagation for the FO and FO* states.

 Reconfigurable magnonics using self-biased reprogrammable nanomagnetic structures INVITED

Magnonics where magnons, the associated quasiparticles of spin waves are used to perform advanced logical or analogue functions represents a promising paradigm for new means of information processing for beyond complementary metal oxide semiconductor (CMOS) based architectures. Furthermore, in view of the emerging nano-magnonics which can eventually lead to a large-scale integration of magnonic devices new approaches for a compact, reconfigurable operation of magnonic device are required. Although such a reconfigurability is key to any efficient application such as magnonic filters, it has hitherto only theoretically [1] but not experimentally been shown on a sub-micron scale. On the other hand, multiferroics inherently offer compact means to implement voltage-control and reconfigurability in such microscopic magnonic systems [2]. In this work, we combine multiferroics with ferromagnets by employing a fully epitaxial heterostructure to achieve such voltage-controlled and reconfigurable magnonic system. Frequency filtering is most often based on magnonic crystals (MC) where a periodic modulation of the spin wave’s energy landscape results in frequency bandgaps in the magnon spectrum [3,4]. Here, we employ a thin-film multiferroic bismuth ferrite BiFeO3 (BFO)- lanthanum strontium manganite La2/3Sr1/3MnO3 (LSMO) heterostructure with a low Gilbert damping ~6x10-3 for the LSMO layer. Instead of modulating the sample shape, we create a MC by imprinting a periodic remnant electrical polarization in the multiferroic BFO layer which modulates the effective magnetic field in the ferromagnetic layer. We characterize the spin wave propagation spectra in this artificial, voltage-induced magnonic crystal and demonstrate the occurrence of a robust magnonic bandgap with &gt;20 dB rejection, i.e. filtering. The imprinted ferroelectric domains can be reconfigured repeatedly and are long-lived. Our results open a new path for the transduction and configurable filtering of spin waves within a single magnonic device. In general, bridging between between the scientific fields of functional oxides and magnonics, it opens new perspectives for the development of beyond CMOS based technologies [5].

**References:**

[1] Q. Wang , A. V. Chumak, L. Jin et al., Phys. Rev. B. 95, 134433 (2017) [2] N. Spaldin and R. Ramesh, Nat. Mat. 18, 203-212 (2019) [3] P. Frey , A.A. Nikitin, D. Bozhko et al., Commun Phys 3, 17 (2020) [4] A. V. Chumak, A. A. Serga and B. Hillebrands, J. Phys. D: Appl. Phys. 50, 244001 (2017) [5] H. Merbouche, I. Boventer, V. Haspot et al., submitted

**Images:**

![](https://assets.underline.io/uploads/markdown_image/1/image/243806faa5791ce2503db35d16d621e6.jpg)
Schematics of the experimental setup shown for the periodic ferroelectric domain state for the BFO layer.

![](https://assets.underline.io/uploads/markdown_image/1/image/4e0581eb0df6af24b4bcc64b618bde47.jpg)
Evidence for the bandgap for the BFO/LSMO heterostructure with periodic domains in the BFO in the amplitude representation in logarithmic scale. The data is normalized by the mean amplitude. At the bandgap frequency, the amplitude is dropping by >20 dB. A reconfiguration of the periodic domain state to the uniform down state erases the gap and reconstitutes the initial uniform state's response. Pn,m label the different domain states where n is the cycle number (1 cycle : down (virgin)-> up-> periodic-> ) and m the direction of the ferroelectric polarization.

Short-range Thermal Magnon Diffusion in Magnetic Garnet

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Short-range Thermal Magnon Diffusion in Magnetic Garnet

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