A distributed active patch antenna model of a Josephson oscillator

  1. Vladimir M. KrasnovORCID Logo

Department of Physics, Stockholm University, AlbaNova University Center, SE-10691 Stockholm, Sweden

  1. Corresponding author email

This article is part of the thematic issue "Intrinsic Josephson effect and prospects of superconducting spintronics".

Associate Editor: J. M. van Ruitenbeek
Beilstein J. Nanotechnol. 2023, 14, 151–164. https://doi.org/10.3762/bjnano.14.16
Received 11 Nov 2022, Accepted 13 Jan 2023, Published 26 Jan 2023

A non-peer-reviewed version of this article has been posted as a preprint https://doi.org/10.3762/bxiv.2022.86.v1


Optimization of Josephson oscillators requires a quantitative understanding of their microwave properties. A Josephson junction has a geometry similar to a microstrip patch antenna. However, it is biased by a dc current distributed over the whole area of the junction. The oscillating electric field is generated internally via the ac-Josephson effect. In this work, I present a distributed, active patch antenna model of a Josephson oscillator. It takes into account the internal Josephson electrodynamics and allows for the determination of the effective input resistance, which couples the Josephson current to cavity modes in the transmission line formed by the junction. The model provides full characterization of Josephson oscillators and explains the origin of the low radiative power efficiency. Finally, I discuss the design of an optimized Josephson patch oscillator capable of reaching high efficiency and radiation power for emission into free space.

Keywords: antenna theory; cavity modes; Josephson effect; terahertz radiation


A flux-flow oscillator (FFO) is the most extensively studied Josephson source of high-frequency electromagnetic waves (EMW) [1-12]. A FFO was used in the first direct demonstration of Josephson emission by Yanson et al., back in 1965 [13,14]. State of the art FFOs, developed by Koshelets and co-workers show a remarkable performance in terms of tunability and linewidth [6,9,12]. However, they emit very little power into free space [11,13,15,16]. The low radiation power efficiency, that is, the ratio of radiated to dissipated power, is commonly attributed to a large impedance mismatch between a Josephson junction (JJ) and free space [10,16,17]. But there is no consensus about the value of the junction impedance: Is it very small [16] or, in contrast, very large [10]? At present, there is no clear understanding about what causes the impedance mismatch and which geometrical parameters should be changed for solving the problem. The discovery of significant terahertz emission from stacked intrinsic JJs in layered high-Tc cuprates [18-27] further emphasizes the necessity of a quantitative understanding of microwave emission from Josephson oscillators.

Figure 1a shows a sketch of a typical FFO. It is based on a sandwich-type (overlap) JJ with the length, a ≫ λJ, much larger than the Josephson penetration depth, and both in-plane sizes much larger than the thickness of the junction interface, dba. The in-plane magnetic field, Hy, introduces a chain of Josephson vortices (fluxons) in the JJ. The dc bias current, Ib, exerts a Lorentz force, FL, and causes a unidirectional fluxon motion. Upon collision with the junction edge, the fluxons annihilate. The released energy produces an EMW pulse, which is partially emitted but mostly reflected backwards in the JJ. Propagation and reflection of FFO pulses in the transmission line (TL) formed by the JJ leads to the formation of standing waves. The corresponding cavity mode resonances are manifested by Fiske steps in the current–voltage (IV) characteristics [16,28-32]. FFOs exhibit sharp emission maxima at the Fiske steps [9,12,13]. Such a conditional emission indicates that several additional and equally important phenomena (apart from the ac-Josephson effect) are involved in FFO operation [10]. The excitation of high-quality factor, Q ≫ 1, cavity modes is one of them.


Figure 1: (a) A sketch of the Josephson flux-flow oscillator. It is based on a sandwich-type junction with two superconducting electrodes (light blue) separated by a dielectric interlayer (yellow). Red ovals represent Josephson vortices that are driven by the Lorentz force, FL, exerted by the dc bias current, Ib. From the outside, the junction has a patch antenna geometry. However, inside it is driven by a distributed dc current, and the oscillating voltage is generated internally by a combination of the ac-Josephson effect and the flux-flow phenomenon. (b) Clarification of spatial and angular coordinates. (c) An equivalent circuit of the Josephson junction. The ac-Josephson effect provides a source of the high-frequency alternating current with the fixed amplitude of current density, Jc0. The oscillating voltage at the junction edges is generated by means of the input junction impedance, Zin, and is distributed between the internal dissipative resistance, Rdis, and the external radiative impedence, Zrad, connected by the transmission line impedance ZTL.

Geometry is playing a decisive role for characteristics of microwave devices. Although calculations of radiative impedances of JJs do exist [33], they were not made for the FFO geometry. From the outside, the overlap JJ looks like a well-known microstrip patch antenna [34-36]. The difference, however, is inside. A standard patch antenna has a point-like feed-in port, while in a JJ the bias current is distributed over the whole area of the JJ. Furthermore, the oscillating component of the current is actively generated inside the JJ by means of the ac-Josephson effect and the flux-flow phenomenon. Therefore, a JJ can be considered as an actively pumped patch antenna with a distributed feed-in current.

In this work, I present a distributed, active patch antenna model of a Josephson oscillator. It expands the TL model of a patch antenna [36], taking into account the spatial distribution of the input current density in a JJ, described by the perturbed sine-Gordon equation. In the presence of a magnetic field and fluxons, the oscillating current is distributed nonuniformly within the junction. This nonuniformity is essential for the FFO operation. It determines the variable input resistance, which enables the coupling of the Josephson current to cavity mode resonances in the junction. The presented model allows for the application of many of patch antenna results and facilitates full characterization of Josephson oscillators, including the emission power, directivity, and power efficiency. The model explains the origin of the low power efficiency for emission in free space and clarifies which parameters can be changed to improve the FFO characteristics. Finally, I discuss the design of a Josephson patch oscillator that can reach high power for emission in free space with the optimal power efficiency of approx. 50%.


The spatial-temporal distribution of voltage in a JJ is described by the equation (see chapter 9 in [31]):


where c0 is the (Swihart) velocity of EMWs in the TL formed by the JJ and L is the inductance of JJ per square. Jz is the current density through the JJ, which has Cooper pair and quasiparticle (QP) components,


Here, Jc0 is the Josephson critical current density, η is the Josephson phase difference, and rQP = RQPab is the QP resistance per unit area.

Active patch antenna model of a junction

Equation 1 is the equation for an active TL [37] with a distributed feed-in current density Jz. Therefore, a JJ has many similarities with the microstrip patch antenna. However, there are three main differences:

(i) The feed-in geometry. A patch antenna has a point-like feed-in port, through which the oscillating current is applied [34-36]. The FFO is biased by a dc current distributed over the whole JJ area.

(ii) The excitation scheme. A patch antenna is a linear oscillator pumped by a harmonic signal. In contrast, a JJ is biased by a dc-current and the oscillatory component is generated inside the JJ via the ac-Josephson effect and the flux-flow phenomenon.

(iii) The slow propagation speed of EMWs inside the JJ, c0c. This is caused by a large kinetic inductance of superconducting electrodes. For Nb-based JJs, c/c0 ≈ 40 (see the estimation in section Discussion). For atomic-scale intrinsic JJs in layered cuprates, c0 can be almost 1000 times slower than c [32]. Because of that, the wavelength inside the JJ is much smaller than in free space, λ ≪ λ0. Therefore, a JJ corresponds to a patch antenna with an extraordinary large effective permittivity, [Graphic 1] = (c/c0)2.

The dynamics of a JJ is described by a nonlinear perturbed sine-Gordon equation,


It follows from Equation 1 and Equation 2, taking into account the ac-Josephson relation, V = (Φ0/2π)∂η/∂t. Equation 3 is written in a dimensionless form with space, [Graphic 2] = xJ, normalized by λJ,and time, [Graphic 3] = ωpt, by the Josephson plasma frequency, ωp. Here α is the QP damping factor, and [Graphic 4] = Jb/Jc0 is the normalized bias current density, which originates from the ∂2V/∂y2 term in Equation 1 [38]. In what follows, “tilde” will indicate dimensionless variables, [Graphic 5] = ω/ωp and [Graphic 6] = λJk. The definition of and the interconnection between different variables are clarified in the Appendix section.

Radiative resistance of a patch antenna

A rectangular patch antenna has two radiating slots, which correspond to the left and right edges of the JJ in Figure 1a. The slots can be considered as magnetic current lines (magnetic dipoles) [39]. Radiation from the antenna is determined by the radiative impedance, Zrad. For a patch with a very thin insulator (as is the case for a tunnel JJ), the radiative admittance of one slot, 1/Zrad1 = G1 + iB1, contains a large imaginary part B1, caused by the large capacitance. However, at the cavity mode resonance the imaginary contributions from the two slots cancel out [34,36,39] and the radiative impedance becomes real. Therefore, at the resonance the radiation power from one slot is


where |v(0,a)| is the amplitude of voltage oscillations at the slot (x = 0,a) and G1 is the radiative conductance of the single slot. Low-Tc JJs are operating at sub-terahertz frequencies, for which the wavelength in free space is large, λ0bd. In this limit [36,39],


where Z0 = [Graphic 7] ≃ 376.73 (Ω) is the impedance of free space.

To calculate the total radiation power from both slots one has to take into account the mutual radiative conductance, G12, and the array factor AF [36]. G12 is originating from a cross product of electric and magnetic fields generated by different slots. For λ0bd it is equal to [36,40]


Here, J0 is the zeroth-order Bessel function, k0 = 2π/λ0 is the wave number in free space, and the angle Θ is defined in Figure 1b. For the n-th cavity mode,


the argument of J0 becomes (c0/cnsinΘ. Since c0c, k0a is small. Expanding in Equation 6, J0(x) ≃ 1 − x2/4 (for x ≪ 1), we obtain:


It is seen that the mutual conductance for a JJ with thin electrodes (slow c0) is not negligible and can be as big as the single-slot conductance G1, Equation 5.

The array factor takes into account the interference of electromagnetic fields from the two slots in the far field. It depends on the separation between the slots, a, the relative phase shift, β, and the direction (φ,Θ). Since radiation from a patch antenna is induced by magnetic current lines, it is more intuitive to consider the interference of magnetic fields, H1 + H2 = AFH1. For the geometry of Figure 1a and Figure 1b, it can be written as [36,40]


Odd-number cavity modes have antisymmetric voltage oscillations but symmetric magnetic currents, β = 0. This leads to a constructive interference with the maximum AF = 2 perpendicular to the patch along the z-axis. For even modes its vice versa, β = π, and a destructive interference leads to a node, AF = 0, along the z-axis.

The total emission power is


where the plus/minus signs are for odd/even modes, respectively. For equal amplitudes, |v(0)| = |v(a)|,


with the effective radiative resistance


Determination of voltage amplitudes

To calculate Prad, we need voltage amplitudes at the JJ edges. Within the TL model of patch antennas, v(x) is obtained by decomposition into a sum of cavity eigenmodes [34]. For JJs, a similar approach is used for the analysis of Fiske steps [16,29-31]. To separate dc and ac components, we write


Here, k = 2π(Φ/Φ0)/a is the phase gradient induced by the external field, where Φ is the flux in the JJ. ω = 2πΦ0Vdc is the angular Josephson frequency proportional to the dc voltage Vdc. The last term, ϕ, represents the oscillatory component induced by cavity modes and fluxons. This term generates the ac voltage, which we aim to determine:


Small-amplitude, multimode analysis

In the small-amplitude limit, ϕ ≪ 1, a perturbation approach can be used. A linear expansion of Equation 3 yields [16,29,31],


Here, [Graphic 8] is the excess dc current with respect to the ohmic QP line. It is caused by the second term on the right-hand side, which enables nonlinear rectification of the Josephson current. The excess dc current is defined as


The oscillatory part is described by the equation


A comparison with Equation 1 shows that this is the active TL equation in which the supercurrent wave, sin(kx + ωt), acts as a distributed (x,t)-dependent drive.

To obtain ϕ, a decomposition into cavity eigenmodes is made [15,16,29,31], similar to the TL analysis of patch antennas [34-36]:


Note that Equation 18 does not include the dc term, n = 0, which is accounted for in [Graphic 9] instead, so that ϕ generates solely ac voltage, as described by Equation 14. Substituting Equation 18 in Equation 17 and taking into account the orthogonality of eigenfunctions, one obtains


From Equation 14, voltage amplitudes at radiating slots are:


Excess current

Without geometrical resonances, the dc current, well above the field-dependent critical current, IIc(H), is determined by the QP resistance, I = V/RQP. In dimensionless units, I/Ic0 = αV/Vp, where Vp = Φ0ωp/2π is the voltage at plasma frequency. At resonances, a partial rectification of the oscillating supercurrent occurs, leading to the appearance of Fiske steps in the IV curves. The excess dc current, obtained from Equation 16, is [16,29,31]


Figure 2a shows calculated IV characteristics of a JJ with a = 5λJ, α = 0.1 and at a magnetic field corresponding to Φ = 5Φ0 in the JJ. Blue symbols represent the direct numerical simulation of the sine-Gordon Equation 3 for up and down current sweep. The red line shows the analytic solution with the excess current given by Equation 24. The agreement between exact (without linearization) numeric and (approximate) analytic solutions is quite good. It is seen that a series of Fiske steps appear in the IV. Vertical grid lines mark positions of cavity mode resonances, ω/c0 = kn. Fiske steps appear at this condition because of the vanishing of [Graphic 10] term in the denominator of gn, Equation 19. The main step occurs at the double resonance condition, ω/c0 = kn = k. It happens at n = 2Φ/Φ0 and leads to the vanishing of (kkn) in the denominators of Equation 20 and Equation 21. The condition, ω/c0 = k, is referred to as the velocity matching because at this point the velocity of the fluxon chain (or phase velocity of the current wave in Equation 17) reaches c0 [16].


Figure 2: (a) Simulated current–voltage characteristics of a junction with L = 5λJ, Φ/Φ0 = 5 and α = 0.1. Blue symbols represent the full numeric solution of the sine-Gordon equation (up and down current sweep). The red line represents the approximate (perturbative) analytic solution, I = V/RQP + ΔI. (b) Excess dc current, ΔI(V), at Fiske steps. The thick red line represents the multimode analytic solution, Equation 24. Thin blue, black, and olive lines show single-mode solutions for n = 9, 10, and 11, respectively. Vertical grid lines in (a) and (b) mark Fiske step voltages. Voltages are normalized by (a) the plasma frequency voltage, Vp, and (b) the lowest Fiske step voltage, V1.

Single-mode analysis

Figure 2b shows the excess current, ΔI/Ic0 versus V, normalized by the n = 1 Fiske step voltage, V1 = Φ0c0/2a. Such normalization clearly shows that the main resonance occurs at n = 2Φ/Φ0 = 10. The thick red line represents the full multimode solution, Equation 24. Thin blue, black, and olive lines represent a single eigenmode contribution for n = 9, 10, and 11, respectively. A perfect coincidence with the red line indicates that for underdamped JJs, α ≪ 1, it is sufficient to consider just a single mode. This greatly simplifies the analysis.

For a resonance at mode n,






Large-amplitude case

The described above perturbative approach is valid only for small amplitudes. Simulations in Figure 2a are made for an underdamped JJ, α = 0.1. In this case the quality factor of high-order cavity modes is large,

[Graphic 11]

and |gn| is not small. Since ϕ appears within the sin η term in Equation 3, the maximum possible amplitude of |gn| is π. This reflects one of the key differences between FFO and patch antenna. The patch antenna is a linear element in which the voltage amplitude is directly proportional to the feed current. A FFO is essentially nonlinear. The amplitude of Josephson phase oscillations will not grow beyond |gn| = π. Instead, higher harmonic generation will occur.

Full numerical simulations of the sine-Gordon equation (Equation 3), shown by blue symbols in Figure 2a, reveal that the amplitude of oscillations reach π at the end of the velocity-matching step. This causes a premature switching out of the resonance before reaching the resonant frequency. It is somewhat miraculous that the agreement with the perturbative solution (red line in Figure 2a) is so good. Apparently, it works remarkably well far beyond the range of its formal applicability, |gn| ≪ 1.

A general single-mode solution for an arbitrary amplitude was obtained by Kulik [30]. The amplitude at the resonance, [Graphic 12], is given by the first solution of the implicit equation [31],


where J0 is the zeroth-order Bessel function. This equation can be easily solved numerically. It is also possible to obtain an approximate analytic solution by expanding J0(x) ≃ 1 − x2/4 for small x. With such expansion, Equation 29 is reduced to a quadratic equation with the solution


For overdamped JJs, α ≫ 1, it reduces to the small-amplitude result of Equation 25, |gn| = [Graphic 13]. For underdamped JJs, it qualitatively correctly predicts saturation of the amplitude for α→0, although at a value of 4 instead of π. Thus, Equation 30 provides a simple and sufficiently good approximation for a significantly broader range of damping parameters than Equation 25.

Input resistance

For the practically most important velocity matching mode, kn = k, from Equations 19–21 it follows, Bn = 1, Cn = 0, Fn = 1, leading to a remarkably simple result,


This equation has a straightforward meaning illustrated by the equivalent circuit in Figure 1c. A JJ is a source of a spatially distributed oscillating current, Jz = Jc0sin(ωt + kx), with a fixed amplitude, Jc0, but spatially dependent phase, kx. It couples to the cavity mode via some effective input impedance Zin. Zin depends on ω, kn and k and is, in general, complex. However, since the phase of the current wave is strongly varying along the junction, it is hard to define the phase shift between current and voltage. Therefore, in what follows, I will be talking about the input resistance, Rin = |Zin|, defined via the relation


From Equation 26 it follows,


Figure 3a–c shows, respectively, Bn, Cn, and Rin/RQP = Fn versus n for the case from Figure 2. Lines are obtained for continuous variation of n in Equation 20 and Equation 21, and circles represent the actual cavity modes with integer n. From Figure 3c, it is seen that Rin has a distinct maximum at the velocity matching condition n = 2Φ/Φ0 = 10. At this point, [Graphic 14], the wave numbers of the cavity mode and the current wave coincide, leading to a perfect coupling along the whole length of the JJ. Therefore, Rin = RQP and v = Ic0RQP. For other modes, knk, the coupling with Josephson current oscillations is much weaker. As seen from Figure 3c, it is oscillating with n. For the particular case with integer Φ/Φ0, Rin vanishes for all even modes. This leads to the absence of corresponding Fiske steps in Figure 2a.


Figure 3: Panels (a) and (b) show mode-number dependence of coefficients Bn and Cn, given by Equation 20 and Equation 21, for the case from Figure 2 with Φ/Φ0 = 5. Panel (c) shows the corresponding oscillatory dependence of the input resistance, Equation 28 and Equation 33. (d) Input resistance for Φ/Φ0 = 5 (olive), 5.25 (blue) and 5.5 (red). The large Rin enables good coupling of the cavity mode to the Josephson current.

The coupling of a cavity mode to the current wave in the JJ depends on magnetic field and flux in the JJ (via the parameter k). This is illustrated in Figure 3d for Φ/Φ0 = 5 (olive line, the same as in Figure 3c), 5.25 (blue), and 5.5 (red). Although the oscillatory behavior of Fiske step amplitudes is well known [16,29,31], the interpretation of such behavior in terms of the input resistance makes a clear connection to the analysis of patch antennas, for which Rin is one of the most important parameters. From this point of view, geometrical resonances with large voltage amplitudes appear only for modes coupled to the current source (Josephson oscillations) via a large input resistance, Equation 32. As seen from Figure 3d, the best coupling with maximum, Rin = RQP, occurs for the velocity-matching step, n = 2Φ/Φ0. Modes with Rin = 0 are not coupled to Josephson oscillations and, therefore, are not excited at all. In particular, there is no coupling to any mode in the absence of an applied field, Rin(H = 0) = 0. This is why Fiske steps do not appear at zero field.

Inclusion of radiative losses in a cavity mode analysis

Finally, in order to calculate radiative characteristics, we need to take into consideration radiative losses. In the previous section, only QP losses in a pure cavity eigenmode were considered. Yet, pure eigenmodes, En ∝ cos(knx), Hn ∝ sin(knx), do not emit any radiation because they do not produce ac magnetic fields at the edges Hn(0,L) = 0 [36]. Consequently, the Pointing vector is zero. In other words, eigenmodes have infinite radiative impedance, Zrad(0,L) = E(0,L)/H(0,L) = ∞. Therefore, despite large electric fields, the radiated power PradE2/Zrad is zero [10].

Radiative losses can be included using the equivalent circuit sketched in Figure 1c. Voltage oscillations at the JJ edges are produced by the oscillating supercurrent via the input resistance, Equation 32. The generated electromagnetic power is distributed between internal losses, characterized by the dissipative resistance, Rdis, and radiative losses to free space, characterized by the radiative resistance Rrad. They are connected by the transmission line impedance,


Here Zsurf is the surface impedance of the electrodes, GQP = 1/RQP is the quasiparticle conductance, L is the inductance, and C is the capacitance of the JJ. The bars indicate that the quantities are taken per unit length. For not very high frequencies and temperatures, the surface resistance of Nb electrodes is small (as will be discussed below). For tunnel JJs, GQP is also small. In this case,


It is very small because b ≫ Λ ≫ d and can be neglected for all practical cases. Therefore, in Figure 1c we may consider that the dissipative and radiative resistances are connected in parallel. Analysis of patch antennas [36] and numerical calculations for JJs with radiative boundary conditions [10] show that radiative losses can be simply included in the cavity mode analysis by introducing the total quality factor, Qtot, of the cavity mode with parallel dissipative and radiative channels,


Here, Qdis is associated with all possible dissipative losses, such as QP resistance in the JJ as well as surface resistance in electrodes and dielectric losses while Qrad represents radiative losses,


Using definitions of α and Q, we can introduce a total damping factor


where the total resistance is


Thus, to include radiative losses, α and RQP in the equations above should be replaced by αtot and Rtot. For the n-th cavity mode resonance we obtain,


For the most important velocity matching resonance from Equation 31, we obtain


with Rrad and Rtot defined in Equation 12 and Equation 39.

Power efficiency

The total power dissipated in a JJ is given by the product of dc voltage and dc current,


Here, the left factor is the dc voltage, and the right one is the total dc current. It contains the QP current (first term) and the rectified excess current, ΔI, (second term). The latter is written using Equation 27 at the resonance condition [Graphic 15]. It is important to note that the nonlinear rectification occurs only inside the JJ. Therefore, the damping parameter αdis within the JJ is used for both terms. The first term in Equation 42 describes dissipative dc losses, which generate only heat, Pheat = V2/2Rdis. The second term in Equation 42 describes the total power consumed by the cavity mode, Pcav = VΔI. Only this term is participating in radiation. From Equation 39 and Equation 40, we obtain a well-known connection between the radiated power and the power consumed solely by the cavity mode,


As usual, the maximum emission power is achieved at the matching condition Rrad = Rdis. In this case, exactly one half of the cavity mode power is emitted and another half is dissipated. This is typical for antennas [36] and is consistent with direct simulations for JJs with radiative boundary conditions [10]. Yet, the overall power efficiency is reduced by the “leakage” QP current in Equation 42, which just produces heat. For the IV curves in Figure 2a, the ohmic QP current is more than twice ΔI at the velocity matching step. Therefore, the total power efficiency, Prad/Ptot, for such moderately underdamped JJ will not exceed 50/3 ≃ 17%. Since the leakage current decreases with increasing RQP, strongly underdamped JJs are necessary for reaching a power efficiency of approx. 50%. This is the case for Nb tunnel JJs [9] and for high-quality intrinsic JJs in Bi-2212 high-Tc cuprates, for which the quality factor may exceed several hundreds [32] and ΔI can be several times larger than the leakage QP current [9,32].


Estimation of parameters

Let us estimate characteristic impedances for the case of Nb/AlOx/Nb tunnel JJs, which are used in state-of-the-art FFOs [9,11]. I assume that a = 100 μm, b = 10 μm, d = 2 nm, εr = 10, d1 = d2 = 100 nm, the zero-temperature London penetration depth λL0 = 100 nm, Jc0 = 5 × 103 (A/cm2), Ic0 = Jc0ab = 50 mA, and the characteristic voltage Ic0Rn = 1 mV. This yields, Rn = 20 mΩ, C = 44.25 pF, Λ = 272.6 nm, inductance L* = μ0Λa/b = 3.43 pH, and c0/c = 2.71 × 10−2.

Surface resistance

Within the two-fluid model, the surface resistance of two superconducting electrodes can be written as [41]:


Here, σn is the normal state conductivity. This approximation is valid for not very high temperatures, T/Tc < 0.8. Using typical parameters for sputtered Nb films, σn ≃ 1.75 × 105 (Ω·cm)−1 [42], frequency f = 400 GHz, and T/Tc = 0.5, we obtain: Rsurf ≃ 0.12 Ω.

Transmission line impedance

The TL impedance is given by Equation 34 where GQP = 1/RQP. For tunnel JJs, RQPRn at sub-gap voltages. I will assume RQP = 25Rn, typical for Nb tunnel JJs [9,11]. This gives RQP = 0.5 Ω and GQP = 2 Ω−1. At f = 400 GHz, ωL* = 8.61 Ω, ωC = 111.2 Ω−1, and ZTL ≃ 0.278 + i0.0015 Ω. It practically coincides with the resistance of an ideal TL, Equation 35. The value of ZTL is only slightly affected by an ill-defined QP resistance and remains practically the same even if we use the upper limit, GQP = 1/Rn. Importantly, ZTL is small because of very small d.

Dissipative resistance

The effective dissipative resistance is affected by all sources of dissipation, including QP and dielectric losses in the junction barrier and surface resistance in electrodes. According to Equation 37, Rdis is defined via the effective quality factor, Qdis, which can be written as:


where QQP, Qsurf and Qdiel are determined by QP, surface, and dielectric losses, respectively. QP and surface resistance contribution can be accounted for using the TL analysis. The quality factor of a TL is determined by the relation

[Graphic 16]

where k1 and k2 are real and imaginary parts of the wave number in the TL, k = k1ik2. They are obtained from the TL dispersion relation,

[Graphic 17]

Taking into account that GQP = 1/RQP ≪ ωC, Rsurf ≪ ωL*, and [Graphic 18], we obtain


Dielectric losses in the AlOx barrier of a JJ were estimated in [43]. At f ≃ 10 GHz, Qdiel ≈ 104. Although it should decrease at f = 400 GHz, we anticipate that it is still in the range of ca. 103. Therefore, dielectric losses are negligible, compared to QP and surface loses. Assuming Qdiel = 500, we obtain, from Equations 45–47, Qdis = 29.48 and Rdis ≃ 0.265 Ω. It is close to the effective dissipative resistance of the TL,


Radiative and total resistances

From Equation 12 and Equation 8, taking into account the smallness of c0/c, we can write,


Substituting λ0 = 750 μm for f = 400 GHz, we obtain a very large value, Rrad ≃ 126.5 kΩ. Since RradRdis, the total resistance, Equation 39, is Rtot = 0.265 Ω ≃ Rdis.

Table 1 summarizes characteristic resistances.

Table 1: Estimation of characteristic resistances (in ohms) for a Nb/AlOx/Nb tunnel junction with sizes a = 100 μm, b = 10 μm, d = 2 nm, d1 = d2 = 100 nm, Jc0 = 5000 (A/cm2), at T/Tc = 0.5 and f = 400 GHz.

Rn RQP Rsurf RTL ωL* C)−1 Rdis Rrad Rtot
0.02 0.5 0.12 0.28 8.6 0.009 0.265 126.5k 0.265

Radiation power

From Equation 41, we get the maximum radiation power at the velocity matching condition, Prad,k ≃ 0.7 nW. It is much smaller than the total dc power at the velocity matching step, approx. Φ0fIc0 ≃ 40 μW. The corresponding power efficiency of approx. 10−5 reflects the key problem for using FFO as a free-space oscillator.

Whom to blame?

The very low radiation power efficiency of a JJ is colloquially attributed to “impedance mismatch”. However, so far, there was no clear understanding of what mismatches with what. A long-living misconception is that the mismatch is between the TL and free-space impedances, ZTLZ0 [16]. However, this is not the source of the poor performance. On the contrary, it is beneficial to have a small TL impedance, connecting two radiating slots in a patch antenna [36]. The small ZTL does not affect antenna performance and can be neglected.

The real source of the problem becomes apparent from Equation 41. It is associated with the more than five orders of magnitude mismatch between the total and radiative resistances, RtotRrad, see Table 1. There are two main reasons for the mismatch: (i) The smallness of the junction width with respect to the free-space wavelength. The factor (λ0/b)2 in Equation 12 and Equation 49 leads to a very large RradZ0. (ii) The smallness of the junction resistance, RQPZ0. The huge mismatch indicates that a JJ alone does not work as a free-space oscillator.

What to do?

Accurate matching between radiative and junction resistances is necessary for efficient emission into free space. Therefore, RQP should be increased and Rrad decreased to a fraction of Z0. However, this is not possible for the standard FFO geometry as sketched in Figure 1a. Indeed, increasing RQP would require the reduction of junction sizes, which would lead to even faster increase of Rrad. Alternatively, RQP can be increased by decreasing Jc0, but this will not reduce Rrad. Therefore, the impedance matching requires modification of the oscillator geometry.

There are many ways of coupling a Josephson oscillator to free space. First, I note that biasing electrodes that are attached to the junction, significantly affect the net impedance. Since the total length of the electrodes (few millimeters) is larger than λ0, the electrodes will reduce the net impedance and, thus, improve impedance matching with free space [17]. Analysis of large JJ arrays demonstrated that long electrodes may act as a traveling wave antenna, facilitating a power efficiency of several percent at f = 0.1–0.2 THz [44,45], which is much better than approx. 10−5 estimated above for the bare junction without electrodes. In [11], a free-space oscillator based on an FFO, coupled to a double-slot antenna, was demonstrated. Although the power efficiency was not specified, a detected off-chip signal up to 55 dB higher than the background noise was reported at f = 0.5 THz. In [27], a mesa structure containing several hundreds of stacked Bi2Sr2CaCu2O8+δ intrinsic JJs was implemented in a turnstile antenna. A radiation power efficiency up to 12% at f ≃ 4 THz was reported. The record high efficiency was attributed to a good impedance matching with free space [17]. In [24], a Bi2Sr2CaCu2O8+δ mesa was implemented into a patch antenna and far-field emission at f = 1.5 THz was reported.

Common for all mentioned approaches is that the junctions, which are small compared to λ0 and, according to Equation 49, have poor coupling to free space, are coupled to large passive elements, comparable with λ0. These elements act as microwave antennas, enabling good impedance matching and enhancing the power efficiency for emission in free space. The target parameters for such oscillators are f ≈ 1–10 THz, a high power-efficiency of approx. 50% and a sufficiently high off-cryostat power above 1 mW.

Josephson patch oscillator

Since in this work I consider patch antennas, below I will dwell on the patch antenna approach, discussed by Ono and co-workers [24]. Figure 4 shows a design of a Josephson patch oscillator (JPO). Here, small junctions (red) are acting as an excitation source for a superconducting patch antenna. The bottom junction electrode (blue) forms the ground plane, and the top electrode (cyan) creates the patch antenna with sizes (a, b), comparable to λ0. In principle, the JPO can be driven by a single JJ. However, as follows from the estimation above (see Table 1), raising the junction resistance to the desired Z0 level would require a drastic (100 times) reduction of the junction area. This will also lead to a proportional reduction of Ic0 and the net available power. Therefore, a better strategy is to use a stack of JJs with large-enough area, enabling high-enough Ic0. The number of JJs, N, is an additional controllable parameter, allowing for fine-tuning of Rn and Rtot. Furthermore, in-phase synchronization of N JJs would provide the N-fold increment of the oscillating voltage v(0,L), leading to a superradiant amplification of the emission power, PradN2 [10].


Figure 4: A proposed design of the impedance-matched free-space Josephson oscillator. Here, a small stack of Josephson junctions (red) is sandwiched between two large superconducting electrodes, namely the ground plane (blue) and the top electrode (light blue). The stack is acting as a source of microwave current (feed-in) for the patch antenna formed by the electrodes.

Moderate-size (approx. 10 μm) Bi2Sr2CaCu2O8+δ mesa structures are optimal for JPOs. The Rn of such mesas can be easily raised to several hundred ohms, while maintaining Ic0 of a few milliamperes. This facilitates the optimal net power level ≈I2Rn of several milliwatts [24,27]. It is small enough for obviation of catastrophic self-heating, which is one of the major limiting factors for superconducting devices [17,27]. Simultaneously, it is large enough to enable emission above 1 mW, provided the radiation power efficiency is close to the optimal approx. 50%.

The operation frequency should be aligned with the Josephson frequency at the characteristics voltage, Ic0Rn, of JJs. For operation at the primary [Graphic 19] mode, one side of the patch should be a ≃ λ/2, where λ = λ0/[Graphic 20] is the wavelength inside the patch and εr is the relative dielectric permittivity of the insulation layer between the patch electrodes. The other size, b, is adjustable and strongly affects the patch antenna performance. For b ≪ λ0, the radiative conductance per slot is given by Equation 5. In the opposite limit, it becomes [36]


One of the most important parameters of the emitting antenna is the directivity, D, of the radiation pattern. A rectangular patch at the [Graphic 21] mode has the main lobe directed perpendicular to the patch (in the z-axis direction) with [36]

[Graphic 22]

A good free-space emitter should have a value for D as large as possible. From this point of view, it is preferable to have fairly wide antennas b ∼ λ0.

Finally, the position (x, y) of the stack plays an important role in the selection of the excited cavity mode. To excite solely the [Graphic 23] mode, the stack should be placed at x close to one of the radiating slots, that is, xa and y = b/2. The position x of the stack affects the effective input resistance of the antenna and provides another adjustable parameter for patch antenna operation, along with the shape of the top electrode [35,36,46]. The FFO input resistance, Equation 33, is not relevant for JPOs, because it describes coupling to an internal cavity mode within the JJ. In JPOs, the Josephson current is coupled to an external cavity mode in the patch. Since the patch is much larger than the JJ, the feed-in of the JPO is not distributed (in contrast to a FFO). Consequently, there is no need for a magnetic field. The best coupling occurs at H = 0, corresponding to the homogeneous distribution of the Josephson current. Generally, operation of JPOs is described by the standard patch antenna theory [36]. The only interesting physics is associated with synchronization of JJs in the stack [10], which can be forced by the high-quality cavity mode in the antenna [47].


I described a distributed, active patch antenna model of a Josephson oscillator. It expands the standard transmission line model of a patch antenna, taking into account the spatial-temporal distribution of the input Josephson current density in a Josephson junction. In the presence of a magnetic field and fluxons, the distribution of the oscillatory component of current is nonuniform. This nonuniformity is essential for operation of a Josephson flux-flow oscillator and determines the effective input resistance, which enables the coupling between the Josephson current and the cavity modes in the junction. The presented model allows for the explicit application of many patch antenna results and facilitates full characterization of the device, including emission power, directivity, and power efficiency. The model explains the low power efficiency for emission in free space. It is primarily caused by the smallness of the junction width compared to the free-space wavelength and the corresponding mismatch between very large radiative and small junction resistances. The model clarifies which parameters can be changed to improve FFO characteristics. Finally, I discussed the design of a Josephson patch oscillator that can reach high power for emission in free space with the optimal power efficiency of approx. 50%.


Definition of variables (Table 2).

Table 2: Definition of variables.

Variable Definition Properties
a, b junction length and width in (x, y) plane a ≫ λJ, b ∼ λJ
α quasiparticle damping factor α = 1/ωpRQPC = 1/QQPp)
C junction capacitance C = ε0εrab/d
c0 Swihart velocity [Graphic 24]
d, d1,2 thicknesses of JJ interlayer and the two electrodes dba
Φ flux in the junction Φ = HyΛ*a
Φ0 flux quantum Φ0 = h/2e
Jc0, Ic0 maximum critical current density and critical current Ic0 = Jc0ab
k field-induced phase gradient k = 2πΦ/Φ0a
kn wave number of a cavity mode kn = (π/a)n
L*, L inductance of JJ and inductance per square L* = μ0Λa/b, L = μ0Λ
λL1,2 London penetration depths of the two JJ electrodes
λ0 wavelength in free space
λ wavelength in the patch antenna λ = λ0/[Graphic 25]
λJ Josephson penetration depth λJ = [Φ0/2πμ0Jc0Λ]1/2 = c0p
Λ characteristic length associated with JJ inductance Λ = d + λL1coth(d1L1) + λL2coth(d2L2)
Λ* effective magnetic thickness of the JJ Λ* = d + λL1tanh(d1/2λL1) + λL2tanh(d2/2λL2)
η Josephson phase difference
ωp Josephson plasma frequency ωp = [2πIc00C]1/2
ωJ angular Josephson frequency ωJ = ∂η/∂t = 2πVdc0
ωn cavity mode angular frequency ωn = c0kn
RQP, (rQP) subgap quasiparticle resistance, (per unit area) rQP = RQPab
Rdis net dissipative resistance
Rsurf surface resistance of electrodes
Rn normal state resistance of the JJ
RTL transmission line resistance
Rrad radiative resistance
Rin effective input resistance of the JJ
Rtot total load resistance of the JJ


  1. Soerensen, M. P.; Parmentier, R. D.; Christiansen, P. L.; Skovgaard, O.; Dueholm, B.; Joergensen, E.; Koshelets, V. P.; Levring, O. A.; Monaco, R.; Mygind, J.; Pedersen, N. F.; Samuelsen, M. R. Phys. Rev. B 1984, 30, 2640–2648. doi:10.1103/physrevb.30.2640
    Return to citation in text: [1]
  2. Nagatsuma, T.; Enpuku, K.; Sueoka, K.; Yoshida, K.; Irie, F. J. Appl. Phys. 1985, 58, 441–449. doi:10.1063/1.335643
    Return to citation in text: [1]
  3. Qin, J.; Enpuku, K.; Yoshida, K. J. Appl. Phys. 1988, 63, 1130–1135. doi:10.1063/1.340019
    Return to citation in text: [1]
  4. Zhang, Y. M.; Winkler, D.; Claeson, T. Appl. Phys. Lett. 1993, 62, 3195–3197. doi:10.1063/1.109127
    Return to citation in text: [1]
  5. Golubov, A. A.; Malomed, B. A.; Ustinov, A. V. Phys. Rev. B 1996, 54, 3047–3050. doi:10.1103/physrevb.54.3047
    Return to citation in text: [1]
  6. Koshelets, V. P.; Shitov, S. V.; Shchukin, A. V.; Filippenko, L. V.; Mygind, J.; Ustinov, A. V. Phys. Rev. B 1997, 56, 5572–5577. doi:10.1103/physrevb.56.5572
    Return to citation in text: [1] [2]
  7. Ustinov, A. V. Phys. D (Amsterdam, Neth.) 1998, 123, 315–329. doi:10.1016/s0167-2789(98)00131-6
    Return to citation in text: [1]
  8. Cirillo, M.; Grønbech-Jensen, N.; Samuelsen, M. R.; Salerno, M.; Rinati, G. V. Phys. Rev. B 1998, 58, 12377–12384. doi:10.1103/physrevb.58.12377
    Return to citation in text: [1]
  9. Koshelets, V. P.; Shitov, S. V. Supercond. Sci. Technol. 2000, 13, R53–R69. doi:10.1088/0953-2048/13/5/201
    Return to citation in text: [1] [2] [3] [4] [5] [6] [7]
  10. Krasnov, V. M. Phys. Rev. B 2010, 82, 134524. doi:10.1103/physrevb.82.134524
    Return to citation in text: [1] [2] [3] [4] [5] [6] [7] [8] [9]
  11. Kinev, N. V.; Rudakov, K. I.; Filippenko, L. V.; Baryshev, A. M.; Koshelets, V. P. IEEE Trans. Terahertz Sci. Technol. 2019, 9, 557–564. doi:10.1109/tthz.2019.2941401
    Return to citation in text: [1] [2] [3] [4] [5]
  12. Paramonov, M. E.; Filippenko, L. V.; Khan, F. V.; Kiselev, O. S.; Koshelets, V. P. Appl. Sci. 2022, 12, 8904. doi:10.3390/app12178904
    Return to citation in text: [1] [2] [3]
  13. Yanson, I. K.; Svistunov, V. M.; Dmitrenko, I. M. Sov. Phys. - JETP 1965, 21, 650.
    Return to citation in text: [1] [2] [3]
  14. Yanson, I. K. Low Temp. Phys. 2004, 30, 515–521. doi:10.1063/1.1789911
    Return to citation in text: [1]
  15. Langenberg, D. N.; Scalapino, D. J.; Taylor, B. N.; Eck, R. E. Phys. Rev. Lett. 1965, 15, 294–297. doi:10.1103/physrevlett.15.294
    Return to citation in text: [1] [2]
  16. Langenberg, D. N.; Scalapino, D. J.; Taylor, B. N. Proc. IEEE 1966, 54, 560–575. doi:10.1109/proc.1966.4776
    Return to citation in text: [1] [2] [3] [4] [5] [6] [7] [8] [9] [10] [11]
  17. Krasnov, M. M.; Novikova, N. D.; Cattaneo, R.; Kalenyuk, A. A.; Krasnov, V. M. Beilstein J. Nanotechnol. 2021, 12, 1392–1403. doi:10.3762/bjnano.12.103
    Return to citation in text: [1] [2] [3] [4]
  18. Ozyuzer, L.; Koshelev, A. E.; Kurter, C.; Gopalsami, N.; Li, Q.; Tachiki, M.; Kadowaki, K.; Yamamoto, T.; Minami, H.; Yamaguchi, H.; Tachiki, T.; Gray, K. E.; Kwok, W.-K.; Welp, U. Science 2007, 318, 1291–1293. doi:10.1126/science.1149802
    Return to citation in text: [1]
  19. Wang, H. B.; Guénon, S.; Yuan, J.; Iishi, A.; Arisawa, S.; Hatano, T.; Yamashita, T.; Koelle, D.; Kleiner, R. Phys. Rev. Lett. 2009, 102, 017006. doi:10.1103/physrevlett.102.017006
    Return to citation in text: [1]
  20. Kakeya, I.; Omukai, Y.; Yamamoto, T.; Kadowaki, K.; Suzuki, M. Appl. Phys. Lett. 2012, 100, 242603. doi:10.1063/1.4727899
    Return to citation in text: [1]
  21. Benseman, T. M.; Gray, K. E.; Koshelev, A. E.; Kwok, W.-K.; Welp, U.; Minami, H.; Kadowaki, K.; Yamamoto, T. Appl. Phys. Lett. 2013, 103, 022602. doi:10.1063/1.4813536
    Return to citation in text: [1]
  22. Zhang, H.; Wieland, R.; Chen, W.; Kizilaslan, O.; Ishida, S.; Han, C.; Tian, W.; Xu, Z.; Qi, Z.; Qing, T.; Lv, Y.; Zhou, X.; Kinev, N.; Ermakov, A. B.; Dorsch, E.; Ziegele, M.; Koelle, D.; Eisaki, H.; Yoshida, Y.; Koshelets, V. P.; Kleiner, R.; Wang, H.; Wu, P. Phys. Rev. Appl. 2019, 11, 044004. doi:10.1103/physrevapplied.11.044004
    Return to citation in text: [1]
  23. Borodianskyi, E. A.; Krasnov, V. M. Nat. Commun. 2017, 8, 1742. doi:10.1038/s41467-017-01888-4
    Return to citation in text: [1]
  24. Ono, Y.; Minami, H.; Kuwano, G.; Kashiwagi, T.; Tsujimoto, M.; Kadowaki, K.; Klemm, R. A. Phys. Rev. Appl. 2020, 13, 064026. doi:10.1103/physrevapplied.13.064026
    Return to citation in text: [1] [2] [3] [4]
  25. Delfanazari, K.; Klemm, R. A.; Joyce, H. J.; Ritchie, D. A.; Kadowaki, K. Proc. IEEE 2020, 108, 721–734. doi:10.1109/jproc.2019.2958810
    Return to citation in text: [1]
  26. Tsujimoto, M.; Fujita, S.; Kuwano, G.; Maeda, K.; Elarabi, A.; Hawecker, J.; Tignon, J.; Mangeney, J.; Dhillon, S. S.; Kakeya, I. Phys. Rev. Appl. 2020, 13, 051001. doi:10.1103/physrevapplied.13.051001
    Return to citation in text: [1]
  27. Cattaneo, R.; Borodianskyi, E. A.; Kalenyuk, A. A.; Krasnov, V. M. Phys. Rev. Appl. 2021, 16, L061001. doi:10.1103/physrevapplied.16.l061001
    Return to citation in text: [1] [2] [3] [4]
  28. Coon, D. D.; Fiske, M. D. Phys. Rev. 1965, 138, A744–A746. doi:10.1103/physrev.138.a744
    Return to citation in text: [1]
  29. Kulik, I. O. JETP Lett. 1965, 2, 84.
    Return to citation in text: [1] [2] [3] [4] [5] [6]
  30. Kulik, I. O. Sov. Phys. Tech. Phys. 1967, 12, 111.
    Return to citation in text: [1] [2] [3]
  31. Barone, A.; Paternò, C. Physics and Applications of the Josephson Effect; John Wiley & Sons, Inc.: New York, USA, 1982.
    Return to citation in text: [1] [2] [3] [4] [5] [6] [7] [8]
  32. Katterwe, S. O.; Rydh, A.; Motzkau, H.; Kulakov, A. B.; Krasnov, V. M. Phys. Rev. B 2010, 82, 024517. doi:10.1103/physrevb.82.024517
    Return to citation in text: [1] [2] [3] [4]
  33. Bulaevskii, L. N.; Koshelev, A. E. J. Supercond. Novel Magn. 2006, 19, 349–367. doi:10.1007/s10948-006-0176-5
    Return to citation in text: [1]
  34. Carver, K. R.; Mink, J. W. IEEE Trans. Antennas Propag. 1981, 29, 2–24. doi:10.1109/tap.1981.1142523
    Return to citation in text: [1] [2] [3] [4] [5]
  35. Okoshi, T. Planar Circuits for Microwaves and Lightwaves; Springer-Verlag: Berlin Heidelberg New York Tokyo, 1985. doi:10.1007/978-3-642-70083-5
    Return to citation in text: [1] [2] [3] [4]
  36. Balanis, C. A. Antenna Theory: Analysis and Design, 3rd ed.; John Wiley & Sons, Inc., Publ.: Hoboken, New Jersey, 2005.
    Return to citation in text: [1] [2] [3] [4] [5] [6] [7] [8] [9] [10] [11] [12] [13] [14] [15] [16] [17]
  37. Lindquist, C. S. J. Franklin Inst. 1971, 291, 1–17. doi:10.1016/0016-0032(71)90258-4
    Return to citation in text: [1]
  38. Krasnov, V. M. Phys. Rev. B 2020, 101, 144507. doi:10.1103/physrevb.101.144507
    Return to citation in text: [1]
  39. Derneryd, A. IEEE Trans. Antennas Propag. 1976, 24, 846–851. doi:10.1109/tap.1976.1141445
    Return to citation in text: [1] [2] [3]
  40. Derneryd, A. IEEE Trans. Antennas Propag. 1978, 26, 532–535. doi:10.1109/tap.1978.1141890
    Return to citation in text: [1] [2]
  41. Schmidt, V. V.; Müller, P.; Ustinov, A. V. The Physics of Superconductors: Introduction to Fundamentals and Applications, 3rd ed.; Springer Berlin: Berlin, Germany, 1997. doi:10.1007/978-3-662-03501-6
    Return to citation in text: [1]
  42. Krasnov, V. M.; Oboznov, V. A.; Ryazanov, V. V. Phys. C (Amsterdam, Neth.) 1992, 196, 335–339. doi:10.1016/0921-4534(92)90455-l
    Return to citation in text: [1]
  43. Gunnarsson, D.; Pirkkalainen, J.-M.; Li, J.; Paraoanu, G. S.; Hakonen, P.; Sillanpää, M.; Prunnila, M. Supercond. Sci. Technol. 2013, 26, 085010. doi:10.1088/0953-2048/26/8/085010
    Return to citation in text: [1]
  44. Galin, M. A.; Borodianskyi, E. A.; Kurin, V. V.; Shereshevskiy, I. A.; Vdovicheva, N. K.; Krasnov, V. M.; Klushin, A. M. Phys. Rev. Appl. 2018, 9, 054032. doi:10.1103/physrevapplied.9.054032
    Return to citation in text: [1]
  45. Galin, M. A.; Rudau, F.; Borodianskyi, E. A.; Kurin, V. V.; Koelle, D.; Kleiner, R.; Krasnov, V. M.; Klushin, A. M. Phys. Rev. Appl. 2020, 14, 024051. doi:10.1103/physrevapplied.14.024051
    Return to citation in text: [1]
  46. Delfanazari, K.; Asai, H.; Tsujimoto, M.; Kashiwagi, T.; Kitamura, T.; Yamamoto, T.; Wilson, W.; Klemm, R. A.; Hattori, T.; Kadowaki, K. IEEE Trans. Terahertz Sci. Technol. 2015, 5, 505–511. doi:10.1109/tthz.2015.2409552
    Return to citation in text: [1]
  47. Cattaneo, R.; Galin, M. A.; Krasnov, V. M. Beilstein J. Nanotechnol. 2022, 13, 1578–1588. doi:10.3762/bjnano.13.132
    Return to citation in text: [1]

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