500 microkelvin nanoelectronics

TL;DR

This paper demonstrates a novel nuclear refrigeration technique that cools nanoelectronic devices to an electron temperature of approximately 421 microkelvin, enabling observation of fragile quantum effects at unprecedented low temperatures.

Contribution

It introduces a combined on-chip and off-chip nuclear refrigeration method to achieve sub-millikelvin electron temperatures in nanoelectronic devices.

Findings

Achieved electron temperature of 421 microkelvin.

Maintained sub-millikelvin temperature for over 85 hours.

Demonstrated effective cooling surpassing previous millikelvin barriers.

Abstract

Fragile quantum effects such as single electron charging in quantum dots or macroscopic coherent tunneling in superconducting junctions are the basis of modern quantum technologies. These phenomena can only be observed in devices where the characteristic spacing between energy levels exceeds the thermal energy, $k_\textrm{B}T$, demanding effective refrigeration techniques for nanoscale electronic devices. Commercially available dilution refrigerators have enabled typical electron temperatures in the $10$ to $100\,$mK regime, however indirect cooling of nanodevices becomes inefficient due to stray radiofrequency heating and weak thermal coupling of electrons to the device substrate. Here we report on passing the millikelvin barrier for a nanoelectronic device. Using a combination of on-chip and off-chip nuclear refrigeration, we reach an ultimate electron temperature of $T_\textrm{e}=421\pm35\,\mu$K and a hold time exceeding $85\,$hours below $700\,\mu$K measured by a self-calibrated Coulomb-blockade thermometer.

Figures

a. Our design is accommodated by a commercial dilution refrigerator (MNK126-700, Leiden Cryogenics) with several microwave-tight radiation shields to reduce electronic noise coupling to the nanostructure. The magnetic field required for magnetic cooling was applied by a superconducting solenoid with a rated field of $13\,$T. The device was installed in the field centre, however parts of the off-chip refrigerants were subjected to smaller magnetic fields defined by the field profile of the solenoid, which we account for by listing the effective molar amount of the materials.

a. Our design is accommodated by a commercial dilution refrigerator (MNK126-700, Leiden Cryogenics) with several microwave-tight radiation shields to reduce electronic noise coupling to the nanostructure. The magnetic field required for magnetic cooling was applied by a superconducting solenoid with a rated field of $13\,$T. The device was installed in the field centre, however parts of the off-chip refrigerants were subjected to smaller magnetic fields defined by the field profile of the solenoid, which we account for by listing the effective molar amount of the materials.

c (blue shade), which provides the quoted statistical error of $T_{\textrm{e}}$. We also display the $T_{\textrm{e}}=0.4E_{\textrm{C}}/k_{\textrm{B}}=1.1\,$mK limit of the universal behaviour [[31](#bib.bib31)], where offset charges do not play a role in the device conductance. In addition, we plot (orange curve) the theoretical maximum of $T_{\textrm{e}}(G/G_{\textrm{t}})$, which occurs when all islands are in full Coulomb blockade. For the MCMC calculation, we assumed uniform tunnel junction resistances and island capacitances. Our fabrication process yields a junction resistance variation o

c,d). Remarkably, we find an excellent agreement with the calculated curves, using $T_{\textrm{e}}$ as the single fit parameter (dashed lines). In addition, we observe no distortion of the lineshape due to Joule heating at finite voltage biases, further demonstrating the role of strong electron-nucleus coupling in indium. To demonstrate the wide range of primary thermometry in our regime of interest, we display a set of experimental data taken between $T_{\textrm{e}}=480\,\mu$K and $23.2\,$mK (Fig. 3e) together with the fitted theoretical curves on a logarithmic scale (circles and dashed lines

b, we show a measurement run starting with $B_{\textrm{i}}=1\,$T and $T_{\textrm{e,i}}=1.57\pm 0.01\,$mK. After ramping up the magnetic field up to $8\,$T and back to $B_{\textrm{f}}=1\,$T, we acquire $T_{\textrm{e,f}}=1.57\pm 0.06\,$mK. With $B_{\textrm{f}}=B_{\textrm{i}}$, the adiabatic efficiency [[27](#bib.bib27)] reads $\eta=T_{\textrm{e,i}}/T_{\textrm{e,f}}=1.00\pm 0.04$, unity within error margin. This remarkable result demonstrates the outstanding control of $T_{\textrm{e}}$ by setting the magnetic field, which is unprecedented for nuclear magnetic cooling stages built for nanoelectron

Equations

$$n^{\star }=\frac{1}{V_{\text{m}}}\int {\left(\frac{B(y)}{B_{\text{max}}}\right)}^{2}A(y)\mathrm{d}y=0.32\text{mol},$$

Full text

††thanks: These authors contributed equally to this work.††thanks: These authors contributed equally to this work.

500 microkelvin nanoelectronics

Matthew Sarsby

  

Nikolai Yurttagül

  

Attila Geresdi

geresdi@chalmers.se

QuTech and Kavli Institute of Nanoscience, Delft University of Technology, 2600 GA Delft, The Netherlands.

Fragile quantum effects such as single electron charging in quantum dots or macroscopic coherent tunneling in superconducting junctions are the basis of modern quantum technologies. These phenomena can only be observed in devices where the characteristic spacing between energy levels exceeds the thermal energy, $k_{\textrm{B}}T$, demanding effective refrigeration techniques for nanoscale electronic devices. Commercially available dilution refrigerators have enabled typical electron temperatures in the $10$ to $100\,$mK regime, however indirect cooling of nanodevices becomes inefficient due to stray radiofrequency heating and weak thermal coupling of electrons to the device substrate. Here we report on passing the millikelvin barrier for a nanoelectronic device. Using a combination of on-chip and off-chip nuclear refrigeration, we reach an ultimate electron temperature of $T_{\textrm{e}}=421\pm 35\,\mu$K and a hold time exceeding $85\,$hours below $700\,\mu$K measured by a self-calibrated Coulomb-blockade thermometer.

Introduction

Accessing the microkelvin regime [1] holds the potential of enabling the observation of exotic electronic states, such as topological ordering [2], electron-nuclear ferromagnets [3, 4], p-wave superconductivity [5] or non-Abelian anyons [6] in the fractional quantum Hall regime [7]. In addition, the error rate of various quantum devices, including single electron charge pumps [8] and superconducting quantum circuits [9] could improve by more effective thermalization of the charge carriers.

The conventional means of cooling nanoelectronic devices relies on the heat flow $\dot{Q}$ between the refrigerator and the conduction electrons, mediated by phonon-phonon coupling in the insulating substrate, $\dot{Q}_{\textrm{p-p}}\propto T_{\textrm{p1}}^{4}-T_{\textrm{p2}}^{4}$ with $T_{\textrm{p1}}$ and $T_{\textrm{p2}}$ being the respective phonon temperatures, and electron-phonon coupling in the device $\dot{Q}_{\textrm{e-p}}\propto T_{\textrm{e}}^{5}-T_{\textrm{p}}^{5}$ where $T_{\textrm{e}}$ is the electron temperature [10, 11], both heat flows rapidly diminishing at low temperatures. In a typical dilution refrigerator, $T_{\textrm{p}}$ is larger than $5\,$mK, and specially built systems reach $1.8\,$mK [12], which limits $T_{\textrm{e}}$ larger than $T_{\textrm{p}}$ to be in the millikelvin regime. The lowest static electron temperature reached with this technique was $T_{\textrm{e}}=3.9\,$mK [13] in an all-metallic nanostructure, and other experiments reached similar values [14, 15, 16] in semiconductor heterostructures.

This technological limitation can be bypassed by adiabatic magnetic refrigeration, which relies on the constant occupation probability of the energy levels of a spin system, proportional to $\exp(-g\mu Bm/k_{\textrm{B}}T)$ in the absence of heat exchange with the environment [17]. Here, $k_{\textrm{B}}T$ is the thermal energy at a temperature of $T$, $g\mu B$ is the energy split between adjacent levels at a magnetic field of $B$ and $m$ is the spin index. Thus, the constant ratio $B/T$ allows for controlling the temperature of the spin system by changing the magnetic field. Exploiting the spin of the nuclei [18, 19], this technique has been utilized to cool nuclear spins in bulk metals down to the temperature range of $T$ around $100\,$pK [20]. If only Zeeman splitting is present, which is linear in $B$, the ultimate temperature is limited by the decreasing molar heat capacity, $C_{\textrm{n}}=\alpha B^{2}/T^{2}$ in the presence of finite heat leaks, $\dot{Q}_{\textrm{leak}}$. Here, the prefactor $\alpha=N_{0}I(I+1)\mu_{\textrm{n}}^{2}g_{\textrm{n}}^{2}/3k_{\textrm{B}}$ contains $I$, the size of the spin, $g_{\textrm{n}}$, the g-factor, $N_{0}$, the Avogadro number and $\mu_{\textrm{n}}$, the nuclear magneton.

Bulk nuclear cooling stages have predominantly been built of copper [19], owing to its high thermal conductivity, beneficial metallurgic properties and weakly coupled nuclear spins, which allows for magnetic refrigeration of the nuclear spins down to $50\,$nK [21], however the weak hyperfine interaction results in a decoupling of the electron system at much higher temperatures, around $1\,\mu$K in bulk samples. Another material, a Van Vleck paramagnet, PrNi5, has been used as a bulk nuclear refrigerant exploiting its interaction-enhanced heat capacity in a temperature range above $200\,\mu$K [22] even in dry dilution refrigerators [23].

Integrating the nuclear refrigerant with the nanoelectronic device yields a direct heat transfer between the electrons and nuclei $\dot{Q}_{\textrm{e-n}}=\alpha\kappa^{-1}B^{2}\left(T_{\textrm{e}}/T_{\textrm{n}}-1\right)$ per mole. Here, $\kappa$ is the Korringa constant, and $T_{\textrm{e}}$, $T_{\textrm{n}}$ are the electron and nuclear spin temperatures, respectively. Owing to an $\alpha/\kappa$ ratio $60$ times better than that of copper, indium has recently been demonstrated as a viable on-chip nuclear refrigerant [24]. In addition, indium allows for on-chip integration of patterned thick films by electrodeposition and has been demonstrated as a versatile interconnect material for superconducting quantum circuits [25].

However, on-chip nuclear refrigeration is limited by the large molar heat leaks $\dot{Q}_{\textrm{leak}}$, which thus far limited the attainable electron temperatures above $3\,$mK both for copper ($\dot{Q}_{\textrm{leak}}=0.91\,$pW mol*-1*, [26]) and indium ($\dot{Q}_{\textrm{leak}}=0.69\,$pW mol*-1*,[24]) as on-chip refrigerant, with a total heat leak of approximately $4\,$pW in both of these experiments. Furthermore, only very short hold times were attained with the chips warming up during the magnetic field sweep, limiting the practical applications of these devices. In contrast, encapsulating the chip in a microkelvin environment has led to superior cooling performance using copper, yielding $T_{\textrm{e}}=2.8\,$mK with a hold time of approximately $1\,$hour below $3\,$mK [27].

Here, we report on a combined on- and off-chip nuclear demagnetization approach, which surpasses the $1\,$mK barrier in a nanoelectronic device. We demonstrate an electron temperature below $500\,\mu$K by combining on-chip indium cooling fins with an off-chip parallel network of bulk indium leads attached to a copper frame. By demagnetization cooling of all components together we greatly reduce the heat leak to the nanoscale device, enabling both a record low final electron temperature and long hold times in excess of $85\,$hours, demonstrating the viable utilization for quantum transport experiments in the microkelvin regime.

Results

Setup for on- and off-chip indium nuclear demagnetization

We discuss the experimental setup following the cross-sectional drawing in Fig. 1a. Our design is accommodated by a commercial dilution refrigerator (MNK126-700, Leiden Cryogenics) with several microwave-tight radiation shields to reduce electronic noise coupling to the nanostructure. The magnetic field required for magnetic cooling was applied by a superconducting solenoid with a rated field of $13\,$T. The device was installed in the field centre, however parts of the off-chip refrigerants were subjected to smaller magnetic fields defined by the field profile of the solenoid, which we account for by listing the effective molar amount of the materials.

We attach the copper frame ($1.7\,$mol total, $0.32\,$mol effective amount) to the mixing chamber via an aluminium-foil heat switch [28], which is activated by a small solenoid at $\approx 10\,$mT of applied magnetic field. Crucially for our design, the electrical measurement lines are not connected to the copper stage, rather to the parallel network of nuclear cooled indium wires with a $23\,$mmol total and $17\,$mmol effective amount per line. These wires are attached to the copper frame by an epoxy resin membrane (nominal thickness of $40\mu$m, Fig. 1b) which provides an additional layer of thermal isolation during nuclear cooling. The electrical and thermal contact to the device is made by press welding the indium wires onto electroplated indium bonding pads on the chip (Fig. 1c).

We apply both electronic filtering and microwave shielding in order to reach sub-1 mK electron temperatures. We thermalize all electrical lines by custom-made copper-powder filters [29] at each stage of the dilution refrigerator and a fifth order RC filter with a cutoff frequency of $50\,$kHz at the mixing chamber. To decouple the cold chip below $1\,$mK from the thermal noise of the mixing chamber [30], we install an additional set of copper-powder filters within the copper stage which is demagnetizated together with the indium lines (Fig. 1d,e). Further details on the measurement circuit are listed in Supplementary Figures 1-4, and in the Methods.

Integrated Coulomb blockade thermometry

To directly measure the electron temperature, we utilize a Coulomb-blockade thermometer (CBT) [32]. CBTs rely on the universal suppression of charge fluctuations in small metallic islands enclosed between tunnel barriers at low electron temperatures. With a total capacitance of each island, $C_{\Sigma}$, we define the charging energy for a tunnel junction array of length $N$ to be $E_{\textrm{C}}=e^{2}/C_{\Sigma}\times(N-1)/N$ with $e$ being the charge of a single electron. In the weak charging regime, $k_{\textrm{B}}T_{\textrm{e}}\gg E_{\textrm{C}}$, the full width at half maximum of the charging curve is $eV_{1/2}=5.439Nk_{\textrm{B}}T$, providing the possibility of primary thermometry independent of $E_{\textrm{C}}$ defined by the device geometry [33]. Crucially for temperature measurements during demagnetization cooling, CBTs exhibit no sensitivity to the applied magnetic field [34].

We fabricated a $36\times 15$ array with an ex-situ Al/AlOx/Al tunnel junction process [35, 24] to create junctions of $780\times 780\,$nm2 in size (Fig. 1h). Since the highly resistive tunnel junctions with $R_{\textrm{j}}=35\,\textrm{k}\Omega$ correspond to a high thermal barrier, we electrodeposited indium cooling fins ($50\times 140\times 25.4\,\mu$m3 corresponding to $11.4\,$nmol, see Fig. 1f,g) on each island for local nuclear cooling. We note however that the measured device has only $5$ conducting lines, resulting in an $N\times M=36\times 5$ CBT array. The details of the device fabrication are previously described in [24].

In Fig. 2a, we show the normalised differential conductance $G(V)/G_{\textrm{t}}$ of the CBT at different temperatures obtained by conventional low frequency lock-in technique at $19.3\,$Hz. We use the master equation of single electron tunneling [32, 33] to find the electron temperature of each curve and the charging energy as a global fit parameter, $E_{\textrm{C}}=232.6\pm 0.8\,$neV$=k_{\textrm{B}}\cdot 2.7\,$mK, yielding $C_{\Sigma}=670\pm 2\,$fF. Remarkably, at a small magnetic field of $B=45\,$mT required to suppress superconductivity, we achieve an electron temperature $T_{\textrm{e}}=7.07\pm 0.09\,$mK by phonon cooling, attesting to the well-shielded environment of the device. At this low temperature, we had to account for the Joule heating of the CBT chip [36], see the Supplementary Note 1 and Supplementary Figure 6. Upon calibration, we use the zero bias conductance $G(V=0)$ for continuous thermometry, see the Supplementary Note 1. We note that we observe a temperature-independent $\Delta G_{\textrm{t}}/G_{\textrm{t}}\approx 0.03$ magnetoresistance between zero field and $12\,$T (inset of Fig. 2a), which we account for during the magnetic field ramps. To demonstrate the limitations of phonon cooling, we evaluate $T_{\textrm{e}}$ as a function of the mixing chamber temperature and observe a saturation behavior below $10\,$mK (Fig. 2b).

In the low temperature regime, where $E_{\textrm{C}}$ is larger than $k_{\textrm{B}}T_{\textrm{e}}$, random island charge offsets influence the conductance of the CBT [31], which causes an a statistical uncertainity of the inferred $T_{\textrm{e}}$. To estimate this confidence interval, we use the following numerical procedure. First, we calculate $G/G_{\textrm{t}}$ by a Markov chain electron counting model with a random set of offset charges for each island. Using the Markov chain Monte Carlo (MCMC) approach, we evaluate the conductances of the tunnel junction chain for 1000 gate charge configurations at a given $T_{\textrm{e}}$. Finally, we build a histogram of the total CBT conductance, which is the a sum of $M=5$ randomly selected line conductances. The conclusion of our calculations is that the conductance distribution remains surprisingly narrow for our array consisting of 35 islands in series and 5 rows in parallel and enables a temperature measurement with a $3\sigma$ relative confidence interval of less than $10\%$ for $T_{\textrm{e}}$ above $400\,\mu$K$=0.15E_{\textrm{C}}$. We plot the calculated calibration curve $T_{\textrm{e}}(G/G_{\textrm{t}})$ (blue solid line) together with a $3\sigma$ confidence interval in Fig. 2c (blue shade), which provides the quoted statistical error of $T_{\textrm{e}}$. We also display the $T_{\textrm{e}}=0.4E_{\textrm{C}}/k_{\textrm{B}}=1.1\,$mK limit of the universal behaviour [31], where offset charges do not play a role in the device conductance. In addition, we plot (orange curve) the theoretical maximum of $T_{\textrm{e}}(G/G_{\textrm{t}})$, which occurs when all islands are in full Coulomb blockade. For the MCMC calculation, we assumed uniform tunnel junction resistances and island capacitances. Our fabrication process yields a junction resistance variation of $\delta R/R$ less than $10\%$ [24], which yields an upper bound of systematic temperature error of $\Delta T_{\textrm{e}}/T_{\textrm{e}}=k(\delta R/R)^{2}$ around $1\%$, where $k$ is a geometry-dependent prefactor of the order of unity [37]. The details of our numerical simulations can be found in the Supplementary Note 1.

Electron cooling by nuclear demagnetization

We initialize a nuclear demagnetization experiment by precooling the device with a closed heat switch at $B_{\textrm{i}}=12\,$T and reach $T_{\textrm{e,i}}=13\,$mK after precooling for $164\,$hours. After opening the heat switch, we remove the magnetic field with a decreasing rate of $\dot{B}(B)=[-2\times 10^{-4}\textrm{s}^{-1}]\cdot B$ to $B_{\textrm{f}}=0.1\,$T, which results in a decreasing $T_{\textrm{e}}$ (Fig. 3a). After finishing the ramp, we find the lowest measured electron temperature $T_{\textrm{e}}=421\pm 35\,\mu$K calibrated using our MCMC model, averaged over a period of one hour (see inset of Fig. 3a). The quoted $3\sigma$ confidence interval is based on the conductance variation calculated by the MCMC model (see Fig. 2c). We note that the full blockade limit of the CBT also yields $T_{\textrm{e,min}}$ less than $500\,\mu$K (orange line).

After reaching the minimum temperature, the device gradually warms up. We find a warm-up rate of $\dot{T}_{\textrm{e}}=1.7\,\mu$K h*-1*, and a hold time of $85\,$hours with $T_{\textrm{e}}$ less than $700\,\mu$K. This duration was limited by the periodic cryogenic liquid transfer to the host cryostat, which induced mechanical vibrations and consequently a rapid warmup of the device.

As a proof of concept quantum transport experiment in the microkelvin regime, we measure the finite bias charging curve of the CBT at two different temperatures below $1\,$mK (circles in Fig. 3c,d). Remarkably, we find an excellent agreement with the calculated curves, using $T_{\textrm{e}}$ as the single fit parameter (dashed lines). In addition, we observe no distortion of the lineshape due to Joule heating at finite voltage biases, further demonstrating the role of strong electron-nucleus coupling in indium. To demonstrate the wide range of primary thermometry in our regime of interest, we display a set of experimental data taken between $T_{\textrm{e}}=480\,\mu$K and $23.2\,$mK (Fig. 3e) together with the fitted theoretical curves on a logarithmic scale (circles and dashed lines, respectively).

Internal magnetic field and heat leak calculation

Next, we turn to the refrigeration properties of indium, and display a series of $T_{\textrm{e}}(B)$ curves in Fig. 4. Notably, $T_{\textrm{e}}^{2}(B^{2})$ follows a linear relation with a negative intercept, $-b^{2}=-(295\pm 7\,$mT$)^{2}$ (Fig. 4a), which demonstrates that indium does not follow a constant $B/T$ ratio. We attribute our results to the strong quadrupolar splitting due to the inhomogenuous electric field in the crystalline lattice [38]. A resulting effective magnetic field $b$ then adds to the applied magnetic field, $B_{\textrm{tot}}^{2}=B^{2}+b^{2}$ [38], which limits the lowest attainable temperature, even if $B\ll b$ (Fig. 4b). Our measurements yield similar $b$ values to earlier nuclear demagnetization experiments in bulk indium samples [39]. This correspondence directly confirms that the measured $T_{\textrm{e}}$ and the inferred nuclear spin temperature, $T_{\textrm{n}}$ are close to each other, which is the key requirement for nuclear demagnetization cooling of nanoelectronics.

Based on the obtained internal magnetic field, we estimate the heat leak of the CBT using the warm-up rate $\textrm{d}T_{\textrm{n}}/\textrm{d}t=\dot{Q}_{\textrm{leak}}/C_{\textrm{n}}$, where $C_{\textrm{n}}=n\alpha B_{\textrm{tot}}^{2}/T_{\textrm{n}}^{2}$ is the nuclear spin heat capacity with $n$ being the molar amount of the refrigerant. These equations yield $\dot{Q}_{\textrm{leak}}=-n\alpha B_{\textrm{tot}}^{2}\frac{\textrm{d}(1/T_{\textrm{e}})}{\textrm{d}t}$, where $\textrm{d}(1/T_{\textrm{e}})/\textrm{d}t$ is the inverse warmup rate (Fig. 3b) in the limit of $T_{\textrm{n}}=T_{\textrm{e}}$. At $B=100\,$mT, we find $\dot{Q}_{\textrm{leak}}=26.7\,$aW per island, which is lower than the $\dot{Q}_{\textrm{leak}}=32\,$aW per island obtained earlier using copper [27].

The small heat leak is further attested by the direct demonstration of the adiabaticity of the experiment. In the inset of Fig. 4b, we show a measurement run starting with $B_{\textrm{i}}=1\,$T and $T_{\textrm{e,i}}=1.57\pm 0.01\,$mK. After ramping up the magnetic field up to $8\,$T and back to $B_{\textrm{f}}=1\,$T, we acquire $T_{\textrm{e,f}}=1.57\pm 0.06\,$mK. With $B_{\textrm{f}}=B_{\textrm{i}}$, the adiabatic efficiency [27] reads $\eta=T_{\textrm{e,i}}/T_{\textrm{e,f}}=1.00\pm 0.04$, unity within error margin. This remarkable result demonstrates the outstanding control of $T_{\textrm{e}}$ by setting the magnetic field, which is unprecedented for nuclear magnetic cooling stages built for nanoelectronics.

Discussion

In conclusion, we demonstrated nuclear magnetic cooling of electrons in a nanostructure down to an ultimate temperature of $T_{\textrm{e}}=421\pm 35\,\mu$K. Integrating on- and off-chip refrigeration utilizing the strong electron-nucleus coupling of indium, we achieve $85\,$hours of hold time in the microkelvin range, which opens up this, so far unexplored, temperature regime for nanoelectronic devices and quantum transport experiments in pursuit of topological and interacting electron systems. We note that other transition metals with a large $\alpha/\kappa$ ratio [38] can potentially be used in future experiments to target an ultimate temperature regime of $T_{\textrm{e}}\approx T_{\textrm{n}}\sim\mu_{\textrm{n}}g_{\textrm{n}}b/k_{\textrm{B}}$ determined by the internal magnetic field $b$. However, comparing our results with earlier experiments featuring on-chip-only refrigeration [26, 24] demonstrates the importance of a cold electronic environment provided by off-chip refrigeration [27]. Furthermore, due to the finite heat leaks, on-chip refrigeration is required to effectively cool highly resistive devices, where the thermalization via the leads is inefficient. In addition, we extend the range of primary nanoelectronic thermometry below $1\,$mK, opening avenues for metrological applications and quantum sensing in the ultra-low electron temperature regime. Cooling down electrons to the microkelvin regime also paves the way towards investigating the limits of quantum coherence in solid state devices on the macroscopic scale [40].

Methods

Mechanical design

The copper stage is milled from 5N5 purity copper. It is left unannealed to reduce eddy currents. The connection to the heat switch is a single M4 bolt, with both the mating surfaces gold plated. The single heat switch in this design resides in a field compensated region of the main magnet. It is formed with a welded lamination of aluminium foil, connecting to copper foil at each end. The aluminium foil layers are mechanically deformed removing continuous paths for superconducting vortices. The switch is then encapsulated in epoxy laced with copper powder for stiffness and filtering. A small superconducting solenoid surrounds the heat switch.

The heat switch shows closing behaviour at an applied current of $\pm 90\,$mA through the solenoid, without measurable dependence on the main field. We observe an abrupt change in both the mixing chamber and CBT temperatures when the solenoid is energised. To be confident of a closed switch, even at high fields, we choose a working current of $140\,$mA to close the switch. The superconducting lines to the the switch quenched when operated above approximately $300\,$mA. The heat switch current was sourced from a TTi EL301R Power Supply (PSU) running in constant current mode. The copper magnet leads are filtered and thermalised with winding embedded in copper powder epoxy at the $4\,$kelvin plate before transitioning to superconducting NbTi. The room temperature wiring is wrapped around a ferrite ring for additional filtering. However, when the heat switch power supply is attached, the galvanic isolation to the cryostat from the measurement electronics is broken, so for best noise performance the leads to the PSU are physically unplugged when performing the nuclear cooling experiments.

The molar amount of material in the copper stage is calculated to be $1.7\,$moles. However, as not all of the material is in the field centre, the contribution to the heat capacity and nuclear cooling reduces accordingly. We calculate the effective molar amount using the field profile of the main solenoid along the vertical axes, $B(y)$ and the cross-sectional areas, $A(y)$. The effective molar amount is then

[TABLE]

where $V_{\textrm{m}}$ is the molar volume and $B_{\textrm{max}}$ is the field maximum.

Similarly, we estimate the effective amount of the indium lines to be $17\,$mmol with a total amount of $23\,$mmol per line.

The indium stages are made from 6N $2\,$mm indium wire rolled out with a small non-ferrous metal rolling pin to flatten it onto a thin epoxy membrane on the copper stage. From there, 4N $1\,$mm indium wires are stir welded at room temperature to ensure good low temperature interconnects. Connecting to the chip, we used 4N $0.7\,$mm indium wires, which are welded to the $1\,$mm wires and press fit onto the indium plated bond pads on the chip. We anneal the indium in-situ over 2 days at room temperature using a turbo molecular pump before cooling the experiment down.

The electrical lines for measuring the CBT connect from the mixing chamber to the microkelvin stage through NbTi superconducting lines with the sorrounding copper matrix removed using dilute nitric acid.

Zero bias tracking

During the magnetic field sweeps and warm-up, we infer the electron temperature based on the zero bias conductance of the CBT. However, time-dependent bias voltage drifts can offset the device, resulting in a systematic error in the measured electron temperature. We note that this error source increases as the temperature is lowered due to the increasing curvature of the conductance dip. To mitigate this effect, we continuously tracked the device conductance in a small voltage bias window centered around the conductance minimum, which was monitored on-the-fly. Note the visible drift in Supplementary Figure 5. The quoted temperatures are then extracted from the conductance minima of a rolling second-order polinomial fit. This procedure removes the systematic positive temperature error introduced at finite voltage biases, but allows for the temperature tracking during demagnetization.

Filtering of the electronic lines

We paid attention to condition the RF environment around the chip, installing RF absorbing materials, in the volumes between plates to reduce the resonant quality factor of the chambers, and covered inner surfaces with an infrared absorbing paint. A set of copper grills are added onto the nuclear cooled stage to damp microwave resonances without increasing eddy current heating in the microkelvin stage.

We used copper powder filters at all stages of the dilution refrigerator. The mixture is 1:3 by mass of copper to epoxy, which also matches the thermal expansion of copper. Voids in the epoxy casting were removed in a vacuum chamber. As the epoxy, we used Loctite Stycast 2850FT with catalyst CAT 24LV, chosen for lower viscosity. The copper powder was supplied by ALDRICH Chemistry, and specified as copper powder(spheroidal), $20\pm 10\,\mu$m, 99% purity. We note that we used the same mixture in all stages of the setup.

We used a combined RC and copper powder filter anchored to the mixing chamber plate of the dilution refrigerator. The RC filter component provides a sharp cutoff at $50\,$kHz. The entire board is covered by copper powder epoxy to prevent microwave leakage. The board accommodates 12 lines in arranged in 6 pairs.

The RC filter components are listed below:

SMD multilayer ceramic capacitors, 50603 [1608 Metric] $\pm 5\%$ C0G/NP0.

Parts: C0603C152J5GACTU, C0603C332J5GACTU, C0603C472J5GACTU

SMD Chip Resistor, 0402 [1005 Metric], $1.5\,$k$\Omega$, ERA2A Series, 50 V, Metal film.

Parts: ERA2AEB751X, ERA2AED152X.

In addition, we further thermalize the experiment with home-made filters mounted inside the slots of the copper nuclear cooled stage. These are made from printed circuit boards with a long meandering trace resulting in an effective continuous element filter. We measure $R=4.6\,\Omega$ line resistance and a $C\approx 250\,$pF capacitance to electrical ground defined by the copper stage. The PCBs have four meandering copper traces on each side. The dual copper layers and the $0.8\,$mm board thickness slot into $1\,$mm spaces in the copper stage. The gaps are then filled with copper powder epoxy.

Corresponding author

Correspondence and request of materials should be addressed to Attila Geresdi.

Acknowledgements

The authors thank J. Mensingh, O. Benningshof, N. Alberts, R. N. Schouten and C. R. Lawson for technical assistance. This work has been supported by the Netherlands Organization for Scientific Research (NWO) and Microsoft Corporation Station Q. A. G. acknowledges funding from the European Research Council under the European Union’s Horizon 2020 research and innovation programme, grant number 804988.

Author contributions

A. G. designed and supervised the experiments. N. Y. designed and fabricated the CBT devices with integrated indium fins. M. S. designed and fabricated the off-chip nuclear cooling stages and filters. M. S.  and N. Y. performed the experiments. N. Y. implemented the numerical CBT array simulation. All authors analyzed the data. The manuscript has been prepared with contributions from all the authors.

Competing interests

The authors declare no competing interests.

Data availability

Raw datasets measured and analyzed for this publication are available at the 4TU.ResearchData repository, DOI: 10.4121/uuid:ffaeb9fc-9baf-428e-8a33-7e4b451d8f9e (Ref. [41]).