Abstract
Quantum mechanics and Coulomb interaction dictate the behaviour of small circuits. The thermal implications cover fundamental topics from quantum control of heat to quantum thermodynamics, with prospects of novel thermal machines and an ineluctably growing influence on nanocircuit engineering^{1,2}. Experimentally, the rare observations thus far include the universal thermal conductance quantum^{3,4,5,6,7} and heat interferometry^{8}. However, evidence for manybody thermal effects paving the way to markedly different heat and electrical behaviours in quantum circuits remains wanting. Here we report on the observation of the Coulomb blockade of electronic heat flow from a small metallic circuit node, beyond the widespread Wiedemann–Franz law paradigm. We demonstrate this thermal manybody phenomenon for perfect (ballistic) conduction channels to the node, where it amounts to the universal suppression of precisely one quantum of conductance for the transport of heat, but none for electricity^{9}. The interchannel correlations that give rise to such selective heat current reduction emerge from local charge conservation, in the floating node over the full thermal frequency range (≲temperature × k_{B}/h). This observation establishes the different nature of the quantum laws for thermal transport in nanocircuits.
Main
The noninteracting ‘scattering’ approach to quantum transport describes coherent conductors as a set of independent channels^{10,11}. However, in circuits with small floating nodes, the Coulomb interaction induces interchannel correlations, including among distinct conductors connected to the same node. Consequences are wideranging, from the emblematic ‘Coulomb blockade’ suppression of electrical conduction at low voltages and temperatures^{12,13,14,15} to exotic ‘charge’ Kondo physics^{16,17}. Remarkably, Coulomb effects can be profoundly different in the charge and heat sectors, in violation of the standard Wiedemann–Franz ratio between electronic conductances of heat and electricity (π^{2}k_{B}^{2}T/3e^{2} with e the elementary electron charge, k_{B} the Boltzmann constant, T the temperature). For ballistic conductors, along which electrons are never reflected backward, the electrical conductance G_{elec} is predicted^{18,19,20} and found^{21,22,23} immune against Coulomb blockade, essentially because charge flow is noiseless (G_{elec} = N × G_{Q}^{e}, with N the number of channels, G_{Q}^{e} = e^{2}/h the electrical conductance quantum and h the Planck constant). Nonetheless, theory predicts^{9} a universal suppression of the heat conductance G_{heat} across ballistic conductors connected to a small, floating circuit node by precisely one quantum of thermal conductance G_{Q}^{h} = π^{2}k_{B}^{2}T/3h (G_{heat} = (N − 1) × G_{Q}^{h}), as presently observed experimentally.
This violation of the Wiedemann–Franz relation does not result from an energydependent electronic density of states, or from the highpass energy filtering across single electron transistors^{24,25}. We describe the underlying mechanism in the spirit of ref. 9, specifically focusing on a metallic node connected to large voltagebiased electrodes through a total of N ballistic channels (Fig. 1a, b). Electronic heat currents can be viewed as the propagation of electrical current fluctuations within a broad frequency bandwidth, extending up to the thermal cutoff ∼k_{B}T/h. For voltagebiased electrodes, the emitted fluctuations result from the thermal broadening of the electron Fermi distribution. For a floating circuit node, charge conservation imposes that the thermal emission of a net charge through a current pulse is accompanied by an opposite charge accumulation in the node. Since the node charge relaxes in the characteristic RC time (with R = 1/NG_{Q}^{e} here, and C the node geometrical capacitance), the overall (net) charge fluctuations emitted from the node (thermal plus subsequent relaxation) are suppressed at frequencies below ∼1/RC. At low temperature k_{B}T ≪ h/RC (k_{B}T ≪ NE_{C} here, with E_{C} ≡ e^{2}/2C the node charging energy), where this suppression covers the full thermal frequency range, it can result in an important reduction of the total heat current. Note that the electrical fluctuations emitted from such a floating node were previously explored in the context of using a ‘voltage probe’ to emulate inelastic mechanisms within the scattering theory of quantum transport (see, for example, ref. 26 and references within). An intuitive way to understand why, for ballistic conductors this reduction amounts universally to one heat transport channel, is to note^{9} that N ballistic electronic channels can be mapped onto a single charge mode (for example, identical current fluctuations on all electronic channels) and N − 1 independent neutral modes (for example, opposite current fluctuations on each of N − 1 pairs of electronic channels), as schematically illustrated Fig. 1b. The N − 1 ballistic neutral modes are completely decoupled from the global charge of the island, and therefore contribute each by one (universal) quantum of thermal conductance G_{Q}^{h}. In contrast, the electrical current fluctuations propagating along the single charge mode are directly connected with fluctuations of the node’s charge. Negligible charge accumulation in the node for frequencies ≲k_{B}T/h therefore completely blocks the charge mode and suppresses its contribution to heat transport, resulting in G_{heat} = (N − 1) × G_{Q}^{h}.
The experiment expands on an approach introduced to measure the thermal conductance quantum across electronic channels^{5}. In contrast to previous works^{5,6}, the present implementation down to electronic temperatures of 8 mK (Methods) allows for the direct observation of the heat Coulomb blockade, which requires that energy transfers between electrons and phonons in the node remain negligible with respect to those through one ballistic channel. The device consists of a central metallic island (the circuit node, see Fig. 1a) separately connected to three large electrodes indexed by i ∈ {1,2,3} through, respectively, N_{i} ballistic quantum channels (N = N_{1} + N_{2} + N_{3}). A Joule power P_{J} = V^{2}G_{P}/2 controlled by the d.c. voltage V applied to electrode 1 dissipates into the electronic fluid within the island (the remaining voltage generator power going into the large electrodes, see Methods), with electrodes 2 and 3 being grounded and G_{P} the corresponding conductance across the device (here, G_{P} = G_{Q}^{e}/[N_{1}^{−1} + (N_{2} + N_{3})^{−1}]). As a result, the metallic island heats up to a steadystate electronic temperature T_{Ω} > T (with T the base electronic temperature), such that P_{J} and net outgoing heat flow J_{heat} exactly compensate (P_{J} = J_{heat}). The determination of T_{Ω} through thermal noise measurements therefore directly provides the J_{heat}–(T_{Ω} − T) characteristics. In general, J_{heat} is the sum of different contributions, including mainly the electronic heat current J_{heat}^{el}(N, T_{Ω}, T) and thermal transfers to the substrate phonons J_{heat}^{ph}(T_{Ω}, T): J_{heat} ≃ J_{heat}^{el} + J_{heat}^{ph}. However, at T_{Ω} < 20 mK, the rapidly decreasing energy transfers toward phonons are found to become negligible such that P_{J} = J_{heat} ≃ J_{heat}^{el}.
The ballistic electronic channels are realized in a highmobility Al(Ga)As twodimensional electron gas (2DEG), tuned in the integer quantum Hall regime to the filling factor ν = 2 with an applied perpendicular magnetic field B ≃ 4.1 T. Without loss of generality, we benefit from the topologically protected ballistic character of the chiral quantum Hall channels (lines with arrows in Fig. 1a). With ν channels propagating along each edge, it is possible to adjust separately N_{i} ∈ {0,1,2} using the field effect. The device was tuned to N ∈ {2,3,4,5} with at least one ballistic channel connecting the central island to both the large electrodes 1 and 2 (N_{1} = 1, N_{2} ∈ {1,2} and N_{3} ∈ {0,1,2}, except for tests in Methods). The micrometrescale metallic island, mainly composed of gold, is associated with a continuous electronic density of states and a charging energy E_{C} ≃ k_{B} × 0.3 K (Methods). By thermal annealing, we achieve negligible levels of electron reflection probability at the 2DEG/island interface, as detailed per channel in Methods. This is essential not only to reach the ballistic limit, but also because residual reflections would impede the noise thermometry through additional quantum shot noise. The electron temperature is obtained from electrical current fluctuations, resolved down to a statistical uncertainty of ±5 × 10^{−32} A^{2} Hz^{−1} at frequencies near 1 MHz, using a homemade preamplifier^{27} cooled to 3.9 K. Quantum shotnoise measurements provide the in situ calibrations of the noise amplification chain gain (±0.1%, all uncertainties and displayed error bars are statistical standard errors), and of the base electronic temperature T ≃ 8 mK (±1%, further confirmed by dynamical Coulomb blockade thermometry^{28}, see Methods). At nonzero Joule power, the temperature increase (T_{Ω} − T) of the metallic island electrons is directly connected to a rise in emitted current noise. In the spirit of the robust Johnson–Nyquist thermometry, the excess noise S_{exc} measured on the floating electrode D (Fig. 1a) with respect to the noise at V = 0 reads^{5,26,29}: S_{exc} = 2G_{S}k_{B}(T_{Ω} − T), with G_{S} the electrical conductance across the device from electrode 2 to electrodes 1 and 3 (in absence of electrical Coulomb blockade, G_{S} = G_{Q}^{e}/[N_{2}^{−1} + (N_{1} + N_{3})^{−1}]). Note that further tests made to eliminate possible experimental artefacts are described in Methods.
In Fig. 2a we show measurements of the excess noise spectral density S_{exc} (bottomright inset) and of the conductances G_{S} (left side of topleft inset) and G_{P} (right side of topleft inset), all as a function of the d.c. voltage V applied to electrode 1. Each colour corresponds to one device configuration N [N_{1}, N_{2}, N_{3}] ∈ {2 [1,1,0], 3 [1,1,1], 4 [1,1,2], 5 [1,2,2]}, with a colour code fixed from now on. The island heating is manifested in the increase of S_{exc} at finite V. In contrast, both G_{S} and G_{P} remain indistinguishable from their maximum quantum limit (respectively G_{Q}^{e}/[N_{2}^{−1} + (N_{1} + N_{3})^{−1}] and G_{Q}^{e}/[N_{1}^{−1} + (N_{2} + N_{3})^{−1}], displayed as thick ticks), independently of V. This demonstrates the absence of Coulomb blockade reduction of the electrical conductance across ballistic channels, at an experimental accuracy better than 0.1% (see also refs 21,22,23). Lines in the main panel of Fig. 2a represent, in a log–log scale, the electron temperature in the metallic island, T_{Ω}, versus the injected Joule power P_{J}, with T_{Ω} obtained from S_{exc} and the separately calibrated base temperature T ≃ 8.1 mK. As generally expected, T_{Ω} is higher when there are fewer electronic channels to evacuate the dissipated P_{J}. Figure 2b displays as symbols the same data, as well as a subsequent run at T ≃ 8.0 mK, but now as the net heat flow J_{heat} = P_{J} versus T_{Ω}^{2} − T^{2}, and focusing on low temperatures (T_{Ω} < 25 mK) where the phonon contribution J_{heat}^{ph} is reduced and where a full suppression of one electronic thermal channel is predicted^{9} (Methods). The straight dashed line closest to the data for N ballistic channels is (N − 1) × J_{Q}^{el}, with J_{Q}^{el} = π^{2}k_{B}^{2}(T_{Ω}^{2} − T^{2})/6h the quantum limit of heat flow per electronic channel. The mere observation that J_{heat} is well below predictions for N independent ballistic channels (N × J_{Q}^{el}) directly demonstrates the specific suppression of heat transport from small circuit nodes, whereas electrical transport remains at the maximum quantum limit. Moreover, we find at such low temperatures a highprecision agreement with heat Coulomb blockade predictions for electronic heat flow, both in the quantitative prediction of a universal suppression of exactly one electronic channel whatever N and in the temperature power law ∝(T_{Ω}^{2} − T^{2}). This direct demonstration of heat Coulomb blockade in the absence of electrical Coulomb blockade constitutes the central result of the present work (see Methods for additional tests establishing the robustness of this observation).
Theory^{9} further predicts quantitatively a crossover of the electronic heat flow from (N − 1) × J_{Q}^{el} to N × J_{Q}^{el}, which extends mostly over one temperature decade around NE_{C}/πk_{B} (Methods). However, the relatively important and rapidly increasing thermal transfers between electrons and phonons at these higher temperatures prevent a direct observation from J_{heat}(T_{Ω}). Following ref. 5, we separately consider the electronic heat current by focusing on the difference at the same value of T_{Ω} between two numbers of connected ballistic channels (N ∈ {2,3,5} and N_{ref} = 4). Indeed, any mechanism that does not depend on N cancels out in J_{heat}(N, T, T_{Ω}) − J_{heat}(N_{ref}, T, T_{Ω}), including the electron–phonon contribution and the universal lowtemperature suppression of one ballistic channel. However, signatures of the (N − 1) × J_{Q}^{el} to N × J_{Q}^{el} crossover can be observed since the temperature at which it takes place increases with N (Methods). Measurements of J_{heat}(N ∈ {2,3,5}, T, T_{Ω}) − J_{heat}(N_{ref} = 4, T, T_{Ω}), normalized by the quantum limit of heat flow per channel J_{Q}^{el}(T, T_{Ω}), are shown as symbols versus T_{Ω} in Fig. 3a. In this representation, deviations from N − N_{ref} (N − 4, horizontal dashed lines) are specific signatures of the heat Coulomb blockade crossover. The quantitative prediction, without any fitting parameter, of the full heat Coulomb blockade theory (continuous lines, Methods) closely matches the data. For N − N_{ref} = ±1 (N ∈ {3,5}, N_{ref} = 4) the crossover signal is small, barely discernible at experimental accuracy, although in sign and magnitude agreement with predictions. For N − N_{ref} = − 2 (N = 2, N_{ref} = 4), the larger crossover signal precisely follows the theoretical prediction up to T_{Ω} ≃ 60 mK, while at higher T_{Ω} ≳ 60 mK the scatter of the data points rapidly increases due to the overwhelming (subtracted) electron–phonon contribution J_{heat}^{ph}. These observations further establish experimentally the full heat Coulomb blockade theory for ballistic channels at arbitrary temperatures, beyond the universal lowtemperature suppression of one quantum channel.
We now investigate the additional heat transfer mechanisms at work in our device. The main panel of Fig. 3b shows as symbols, in a log–log scale versus T_{Ω}, the measured J_{heat}(N) reduced by the heat Coulomb blockade prediction for N ballistic electronic channels. We observe that the reduced data collapse for all N onto a single curve, which is closely reproduced by the functional 3.9 × 10^{−8}(T_{Ω}^{5.85} − T^{5.85}) W (continuous line). This compares well with theoretical expectations for the electron–phonon contribution J_{heat}^{ph} in disordered conductors, where a temperature exponent of 4 or 6 is predicted depending on the nature of disorder^{30}. In the inset of Fig. 3b, we directly confront the measured J_{heat}(N ∈ {2,3,4,5}, T_{Ω}) (coloured dashed lines) with the essentially indistinguishable calculations (black continuous lines) obtained by adding up the full heat Coulomb blockade prediction and the above T_{Ω}^{5.85} functional attributed to electron–phonon interactions.
Finally, we point out that the presently observed heat Coulomb blockade of one ballistic channel should be considered when exploiting the total outgoing heat flow from a floating node to investigate elusive exotic states^{6}.
Methods
Sample.
The sample nanostructure is produced by standard ebeam lithography in a Ga(Al)As 2DEG buried 105 nm below the surface, of density 2.5 × 10^{11} cm^{−2} and of mobility 10^{6} cm^{2} V ^{−1} s^{−1}. The central micrometresized island is composed of a metallic multilayer of nickel (30 nm), gold (120 nm) and germanium (60 nm). Its galvanic, Ohmic contact with the 2DEG is realized by thermal annealing (440 °C for 50 s).
The interface quality between the metallic island and the 2DEG is fully characterized, through the individual determination of the electron reflection probability at the interface for each connected quantum Hall channel, with the selfcalibrated experimental procedure detailed in the Methods of ref. 17. We find a reflection probability below ≲0.001% (the statistical uncertainty) for the three channels closest to the edge (the outer edge channel of each of the three 2DEG branches), 0.08% for the inner edge channel toward electrode 3 used only for N ∈ {4,5}, and 0.5% for the inner edge channel toward electrode 2 used only for N = 5.
The typical electronic level spacing in the metallic island is estimated to be negligibly small (δ ≍ k_{B} × 0.2 μK), based on the electronic density of states of gold (ν_{F} ≍ 1.14 × 10^{47} J^{−1} m^{−3}) and the metallic island volume (≍3 μm^{3}).
Finally, an important device parameter is the charging energy E_{C} ≡ e^{2}/2C. The value E_{C} ≃ k_{B} × 0.3 K is obtained by standard Coulomb diamond characterization, from the d.c. voltage height V_{diam} of the observed diamonds (E_{C} = eV_{diam}/2). These measurements are performed in the same cooldown, at the same magnetic field (data not shown, see, for example, Figure 1c of ref. 28 for a similar characterization of this sample at a higher quantum Hall filling factor).
Experimental setup.
The device is fixed to the mixing chamber plate of a cryofree dilution refrigerator. Electrical measurement lines connected to the sample include several filters and thermalization stages. Two shields at base temperature screen spurious highfrequency radiations. Conductances are measured by standard lowfrequency lockin techniques, below 200 Hz. Further details, including on the noise measurement setup used for the electronic thermometry, are provided in the Supplementary Information of ref. 28.
Electronic temperature.
The electronic temperature in the device is extracted from onchip quantum shotnoise measurements^{28}. For this purpose, we effectively shortcircuit the central metallic island (equivalent circuit schematic shown bottomleft of Supplementary Fig. 1a) using the lateral continuous gate in the 2DEG branch #2 (gate closest to the bottom in Fig. 1a). The quantum point contact used to set N_{2} (bottomright split gate in Fig. 1a) is here tuned to transmit a single channel with a transmission probability τ ≃ 0.5. Supplementary Fig. 1a shows as symbols the measured excess noise versus d.c. bias voltage V, and as a red continuous line the theoretical prediction at T = 7.97 mK for the simultaneously measured value τ ≃ 0.515 (variations of τ with V remain below 0.003 and are ignored). The very low statistical uncertainty of the data shown in the main panel (±5 × 10^{−32} A^{2} Hz^{−1}, below one tenth of the symbols size) is obtained by averaging 153 sweeps. In practice, we fit each of the individual sweeps separately and extract from the statistical analysis of this ensemble of distinct measurements (shown as symbols in inset) the mean value of the temperature and the standard error (here T = 7.97 ± 0.06 mK). The same shotnoise thermometry is performed both just before and just after each run of the full experiment (two runs shown in the manuscript, the first one at T ≃ 8.1 mK and the second at T ≃ 8.0 mK).
In addition, we consolidate the device electronic temperature T with a different onchip thermometry method based on dynamical Coulomb blockade, following ref. 28. For this purpose, the same quantum point contact (2DEG branch #2) is set to the tunnel regime τ ≍ 0.1 (in the absence of dynamical Coulomb blockade renormalization), and the device is tuned to N_{1} = 0 and N_{3} = 2, effectively implementing the schematic circuit shown in the bottomleft of Supplementary Fig. 1b with a series resistance h/2e^{2}. The temperature is obtained by fitting the conductance data displayed as symbols in the main panel of Supplementary Fig. 1b, using the known values of the series resistance and of E_{C}. We find T = 8 mK (corresponding calculation shown as a red line), in agreement with quantum shotnoise thermometry within the larger uncertainty of dynamical Coulomb blockade thermometry, which we estimate to ±1 mK (grey area).
Gain calibration of noise amplification chain.
The gain G_{amp} of the noise amplification chain is calibrated with the quantum shotnoise thermometry described in the section ‘Electronic temperature’, from the linear slope of the measured shot noise at eV ≫ k_{B}T (see ref. 28 for a detailed discussion). As for the determination of T, we extract a different value of G_{amp} from each individual sweep of noise versus d.c. voltage. From an ensemble of 409 values, G_{amp} is extracted with a statistical uncertainty of ±0.1%. Note that the transmission probability τ enters as a factor τ(1 − τ) in the determination of G_{amp}. Here the value of τ is precisely measured simultaneously. Although τ exhibits a weak dependence with V (below 0.003), it is sufficiently small to have a negligible impact on G_{amp} at the approximately 0.1% level (note the particularly low impact in the vicinity of τ = 0.5) and was not taken into account.
The G_{amp} calibration was consolidated at an uncertainty level of approximately 1%, by additional quantum shotnoise measurements at τ ≃ 0.16 (for T ≃ 8 mK) and also at the higher electronic temperature T ≃ 16 mK (for τ ≃ 0.5). The comparison between the different quantum shotnoise and dynamical Coulomb thermometry described in the section ‘Electronic temperature’ further establishes the absolute calibration of G_{amp}, although at a less precise level of approximately 10%. Finally, we point out that the lowtemperature heat Coulomb blockade reduction of heat current by precisely one J_{Q}^{el} was also observed at the different integer quantum Hall filling factors ν = 3 and 4, using specific quantum shotnoise calibrations for the modified gain of the noise amplification chain (with our onchip current to voltage conversion based on the quantum Hall resistance 1/νG_{Q}^{e}, a larger ν therefore results in a lower G_{amp}).
Dissipated Joule power.
The expression P_{J} = V^{2}G_{P}/2 is used to calculate the Joule power dissipated in the electronic fluid of the floating metallic node, due to the applied d.c. bias voltage V (see Fig. 1a). It corresponds to one half of the standard twoterminal total power V^{2}G_{P} provided by the voltage generator. This expression can be straightforwardly derived for noninteracting electrons, within the Landauer–Büttiker scattering formalism. Essentially, it amounts to sharing equally the dissipation between cold electrodes, on the one hand, and central island, on the other hand, as expected in symmetric configurations. In the presence of interactions, one might wonder if the floating character of the central metallic node could possibly break this symmetry. However, the d.c. voltage of the central island as well as the d.c. current across it remain unchanged compared to their freeelectron values, at experimental accuracy (with the island d.c. voltage deduced from the measured emitted current through the quantum limited electrical conductance of the connected ballistic channels, see topleft inset of Fig. 2a) and in agreement with theory for the present case of ballistic channels. This provides further evidence that the resulting Joule power dissipated into the central metallic island retains here its standard, noninteracting expression P_{J} = V^{2}G_{P}/2. We also point out that the same noninteracting expression for P_{J} is specifically expected, on qualitative grounds (a direct quantitative derivation is yet to be done), within the theoretical heat Coulomb blockade framework for the ballistic channels of ref. 9 (Eugene Sukhorukov, private communication).
Heat Coulomb blockade predictions.
We provide the theoretical expression J_{thy}^{el} derived from ref. 9 for the net outgoing heat current J_{heat}^{el} through N ballistic electronic channels connecting a floating metallic node of charging energy E_{C} and at the temperature T_{Ω}, to large electrodes at temperature T, for arbitrary values of T_{Ω} and T:
with the function I given by
where ψ(z) is the digamma function. All the displayed theoretical predictions of the full heat Coulomb blockade theory (continuous lines in Fig. 3a, inset of Fig. 3b, Supplementary Figs 2 and 3a, inset of Supplementary Figs 3b and 4) were calculated using equation (1), without any fitting parameter. Note that these predictions assume a hot Fermi function characterized by the temperature T_{Ω} for the distribution probability of the electrons in the metallic island. This is expected since the average dwell time of the electrons in the metallic island τ_{D} = h/δN ≃ 200/N μs (see, for example, ref. 31) is estimated to be much larger, by about four orders of magnitude, than the typical timescale of ∼10 ns for electron–electron inelastic collisions in similar metals (see, for example, ref. 32 for the connected measurement of the electron coherence time in gold).
Asymptotic limits of predictions.
The function I in equations (1) and (2) has the asymptotic forms
with a crossover centred on x ≍ 1.
At T, T_{Ω} ≪ NE_{C}/πk_{B}, equation (1) therefore reduces to
with precisely one electronic channel effectively suppressed for heat conduction.
At NE_{C}/πk_{B} ≪ T, T_{Ω}, equation (1) reads
which corresponds to a net reduction of the heat conductance (T − T_{Ω} → 0) per ballistic electronic channel by the fixed amount ΔG_{heat}^{el} = E_{C}k_{B}/2h (always small with respect to G_{Q}^{h} in the considered hightemperature limit).
At T ≪ NE_{C}/πk_{B} ≪ T_{Ω}, equation (1) becomes
where the relative reduction due to heat Coulomb blockade progressively vanishes as T_{Ω} increases.
Control experiment at T ≃ 16 mK.
We here demonstrate the robustness of our result with respect to base temperature T. The experiment is performed at a temperature twice as large as before, T ≃ 15.9 ± 0.1 mK, for the setting N = 2. As seen from the J_{heat} versus T_{Ω}^{2} − T^{2} data shown as symbols in Supplementary Fig. 3a, this is still sufficiently low to directly and quantitatively establish the heat Coulomb blockade suppression of one ballistic channel. Note that this robustness also further validates the specific tests performed to rule out possible experimental artefacts (additional power injection by the measurement lines, voltagedependent noise offset, calibration and thermometry issues).
We also find that exactly the same functional 3.9 × 10^{−8}(T_{Ω}^{5.85} − T^{5.85}), attributed to electron–phonon (black continuous line in main panel of Supplementary Fig. 3b), matches the present T ≃ 16 mK data reduced by the predicted electronic heat flow (symbols in main panel of Supplementary Fig. 3b). Note that the observed independence of the electron–phonon coupling with temperature is a commonly used criterion to show that cold electrons and phonons are at the same temperature T (see, for example, ref. 33).
Supplementary experimental tests.
We also performed the following tests. (Test i) At N = 0, the measured noise is found to be independent of d.c. bias (applied either within the same 2DEG branch or in a disconnected branch, with the current flowing toward cold grounds not shown in Fig. 1), at experimental accuracy. In the language of ref. 6, the ‘source noise’ is negligible. (Test ii) At V = 0, the absolute measured noise does not change when tuning N to different values or by connecting the amplification noise chain to an edge channel emitted from a cold ground. This directly shows that the temperature T is homogeneous (the same T for all large electrodes and the metallic island, whatever N), and also that the power injected into the central island is negligible at V = 0 (in the presence of, for example, significant heating from the measurement lines, the central island temperature and consequently the noise measured would depend on N_{1,2,3}; note that such an heating takes place in one of the test configurations discussed in Test iii). (Test iii) We checked that the observed heat Coulomb blockade is independent of the specific channel realization, by comparing three different device configurations all corresponding to N = 2 (see Supplementary Fig. 4): (N_{1} = 1, N_{2} = 1, N_{3} = 0) (main manuscript, red squares in Supplementary Fig. 4), (N_{1} = 0, N_{2} = 1, N_{3} = 1) (violet squares in Supplementary Fig. 4) and (N_{1} = 1, N_{2} = 0, N_{3} = 1) (black squares in Supplementary Fig. 4). The first two configurations give exactly the same result at experimental accuracy. The third configuration has the additional complication that, to perform the noise thermometry of the central island, we had to make use of an otherwise disconnected measurement line within the 2DEG branch 3, through which a nonnegligible power was dissipated into the island even at V = 0 (as seen with measurements as discussed in Test ii, and also with other tests including quantum shotnoise and dynamical Coulomb blockade measurements). Nonetheless, heat Coulomb blockade predictions (and a full agreement with the first two device configurations) are verified when taking into account the separately calibrated temperature offset T_{Ω}(V = 0) − T ≃ 5 mK (obtained through the approach of Test ii) and the additional dissipated power of 0.06 fW at V = 0. (Test iv) Finally, we verified the robustness of our results with respect to the integer quantum Hall filling factor ν at which the experiment is performed. The heat Coulomb blockade suppression of one ballistic channel was quantitatively observed experimentally not only at ν = 2 (main manuscript), but also at ν = 3 and ν = 4.
Comparison with previous experiments.
In the previous works refs 5,6, besides the robust ΔJ_{heat} approach to extract the quantum limit of electronic heat flow J_{Q}^{el}, it was also attempted to determine the full electronic heat flow despite the nonnegligible electron–phonon contribution at T ≳ 25 mK. For this purpose, a T_{Ω}^{5} − T^{5} power law was assumed to model the transfer of energy from electrons at T_{Ω} toward phonons at T. With this model, no heat Coulomb blockade was detected^{5,6}. However, we here point out the sensitive influence of the electron–phonon power law exponent in the analysis of these previous experiments. Together with the higher T, it essentially impeded the observation of the heat Coulomb blockade. We illustrate this with the most accurate data of ref. 5, obtained at integer quantum Hall filling factor ν = 3. As pointed out in the supplementary methods of ref. 5, fitting the data for reference channel number N_{ref} = 4 of this previous experiment with the electron–phonon temperature exponent as a free parameter (instead of assuming an exponent of 5) leads to a reduced overall electronic heat flow of approximately 3.5 × J_{Q}^{el}, a factor in between N_{ref} and N_{ref} − 1, predicted respectively in the absence and in the presence of a heat Coulomb blockade. Reanalysing these previous data with the electron–phonon power law left as a free parameter, we find that they are indeed compatible at experimental accuracy with the present observation of the heat Coulomb blockade of one ballistic channel.
Data availability.
The data that support the plots within this paper and other findings of this study are available from the corresponding author upon reasonable request.
Additional Information
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Acknowledgements
This work was supported by the French RENATECH network, the national French program ‘Investissements d’Avenir’ (Labex NanoSaclay, ANR10LABX0035) and the French National Research Agency (project QuTherm, ANR16CE30001001). We thank E. Sukhorukov for discussions.
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E.S. and F.P. performed the experiment with inputs from A.A.; A.A., E.S. and F.P. analysed the data; F.D.P. fabricated the sample with inputs from A.A.; A.C., A.O. and U.G. grew the 2DEG; Y.J. fabricated the highelectronmobility transistor (HEMT) used for noise measurements; F.P. led the project and wrote the manuscript with inputs from A.A., E.S. and U.G.
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Sivre, E., Anthore, A., Parmentier, F. et al. Heat Coulomb blockade of one ballistic channel. Nat. Phys. 14, 145–148 (2018). https://doi.org/10.1038/nphys4280
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