Abstract
Mixed halide perovskites that are thermodynamically stable in the dark demix under illumination. This is problematic for their application in solar cells. We present a unified thermodynamic theory for this lightinduced halide segregation that is based on a free energy lowering of photocarriers funnelling to a nucleated phase with different halide composition and lower band gap than the parent phase. We apply the theory to a sequence of mixed iodinebromine perovskites. The spinodals separating metastable and unstable regions in the compositiontemperature phase diagrams only slightly change under illumination, while lightinduced binodals separating stable and metastable regions appear signalling the nucleation of a lowband gap iodinerich phase. We find that the threshold photocarrier density for halide segregation is governed by the band gap difference of the parent and iodinerich phase. Partial replacement of organic cations by cesium reduces this difference and therefore has a stabilizing effect.
Introduction
Metalhalide perovskites have extraordinary optoelectronic performance in solar energy harvesting and light emission applications^{1,2,3,4,5,6,7,8}. The flexibility of the perovskite ABX_{3} structure—where A is an organic or inorganic cation, B is a metal cation like Pb or Sn, and X is a halide anion like I or Br—allows to stabilize a preferred phase and tune the band gap through compositional alloying on different lattice sites^{9,10,11,12,13,14,15,16,17,18,19}. Notably, mixed halide perovskites have been successfully used in tandem solar cells, where the band gaps in the two lightabsorbing layers should be optimally tuned^{18,20,21}. However, one of the biggest problems in mixed halide perovksites is their photoinstability, specifically lightinduced halide segregation^{17,22,23,24}. Studies on mixed halide perovskites show that exposure to continuous illumination leads to the separation of the different halide ions, resulting in the formation of low and highband gap domains. The lowband gap domains act as photocarrier traps, as evidenced by redshifts in photoluminescence observations^{17,22,23,24}. The demixing is reversible because when kept in the dark for a sufficient amount of time, the perovskites return to their original mixed state. An important finding is the existence of a threshold intensity for halide segregation^{23,25}. The reversibility and the existence of an illumination threshold suggest a thermodynamic origin of the effect.
Many strategies have been proposed to suppress this halide segregation, such as enhancing grain size and improving overall crystallinity^{26}, reducing carrier diffusion lengths^{23}, partial substitution of Pb with Sn^{27}, application of external pressure^{28}, alloying Cl into the I/Br lattice^{29}, and Acation alloying^{6,30,31,32}. Acation alloying has attracted significant attention and has proven to be effective against halide segregation. It has been found that MA/Cs, FA/Cs, and FA/MA/Cs mixed halide perovskites (MA stands for methylammonium and FA for formamidinium) exhibit a reduced tendency for halide segregation^{6,28,30,31,32,33,34}. In ref. ^{33} the reduced tendency for halide segregation when replacing MA by Cs was attributed to the smaller polarizability of Cs^{+} as compared to MA^{+}, which would reduce electronphonon coupling and suppress halide segregation. In a previous study, we have shown that Acation alloying can change the band gap by changing the volume of the ABX_{3} unit cell or by introducing octahedral distortions^{35}. These structural deformations change the hybridization between the B and Xsite ions, which changes the conduction band minimum and valence band maximum energies. These electronic changes resulting from Acation alloying may also contribute to phase stability improvements.
Several explanations have been given for lightinduced halide segregation. Polaroninduced strain gradients under illumination have been suggested to drive the nucleation of lowband gap iodinerich domains^{36,37}. Other studies suggest that local electric fields caused by electronhole pairs in the thin film^{38} or at the surface^{39} are the driving force for ion migration and demixing. It has also been proposed that a strong gradient in carrier generation rate through the film thickness can be a driving force for halide segregation^{40}. These explanations, however, do not account for the observed existence of a threshold illumination intensity for halide segregation. A model based on band gap differences between perovskites with different halide compositions does account for a threshold illumination intensity^{23}. In that model, it is suggested that the band gap difference between mixed I/Br and Irich domains, where photocarriers can reduce their free energy by funneling to the Irich domains, is the driving force behind the demixing. When applied to MAPb(I_{0.5}Br_{0.5})_{3}, the model yields an illumination threshold that is of the same order of magnitude as found in a recent experiment, but it leaves the observed strong temperature dependence of the threshold unexplained^{25}.
There is a clear need for a unified theory for lightinduced halide segregation in mixed halide perovskites that is transferable and flexible. Understanding is lacking about the influence of temperature on the illumination intensity threshold for halide segregation, but also about the role of material composition. For example, we are not aware of explanations for the improved photostability after partial Cs substitution in MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3}^{6,28,30,31,32,33,34}. From this, we conclude that it is not understood how Asite alloying influences the thermodynamic stability under illumination. Such understanding is needed to avoid or mitigate the effect.
Here, we provide such a unified theory and apply it to lightinduced halide segregation in MAPb(I_{1−x}Br_{x})_{3}, FAPb(I_{1−x}Br_{x})_{3}, CsPb(I_{1−x}Br_{x})_{3}, MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, and FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, which are experimentally among the most studied perovskite compounds. We have added the latter two compounds to our study to investigate the influence of partial Cs substitution. The free energy for each compound in the dark is determined using binary alloying theory. By adding a contribution to the free energy from photocarriers, we obtain a parameterfree theory that enables us to construct the phase diagrams for each compound in the dark and under illumination, distinguishing stable, metastable, and unstable regions. The theory also enables us to determine the dependence of the illumination threshold for halide segregation on temperature and material composition.
Results
Free energy in the dark
We first consider the compositional Helmholtz free energy of the five compounds, applicable to the situation in the dark, within the quasichemical approximation (QCA, see ‘Methods’) of binary alloying theory^{41}. This starts with a calculation of the configurational mixing enthalpy ΔU of the compounds (see Eq. (5) in ‘Methods’). For this, we calculate within density functional theory (DFT) the energy of possible configurations of the halide anions in a supercell geometry. For the singlecation compounds MAPb(I_{1−x}Br_{x})_{3}, FAPb(I_{1−x}Br_{x})_{3}, and CsPb(I_{1−x}Br_{x})_{3} we take supercells with two formula units, following Brivio et al.^{42}, while for the doublecation compounds MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} and FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} we take supercells with eight formula units. Figure. 1a–e display for each of the five compounds the configurations with the lowest mixing enthalpy for x = 0.5. The mixing enthalpies per formula unit (f.u.) for the possible configurations of the I and Br anions in the supercell are given by circles in Fig. 1f–j.
By applying the QCA we obtain from the mixing enthalpies of the possible configurations at discrete relative Br concentrations x = 0, 1/6, 1/3, 1/2, 2/3, 5/6, 1 the mixing enthalpy ΔU(x, T) as a continuous function of x. The curves in Fig. 1f–j show ΔU(x, T) for different temperatures T in the range 150–350 K. Figure 1k–o display the mixing free energy ΔF(x, T) = ΔU(x, T) − TΔS(x, T) per formula unit, where ΔS(x, T) is the configurational mixing entropy.
In the singlecation materials, the width of the distribution in the mixing enthalpy ΔU for the different halide configurations increases in the order Cs–MA–FA of increasing cation size. The explanation is that, because of the different sizes of the halide anions (I is bigger than Br), the strain in the lattice for the different halide configurations is best accommodated for by CsPb(I_{1−x}Br_{x})_{3}, followed by MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3}. The increasing cation size in this sequence is also reflected in the order of increasing unit cell volumes of the three compounds (see Supplementary Note 1). The incorporation of Cs in a relative concentration of 1/8 in MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} and FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} shows an expected slight decrease of the width of the distribution as compared to MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3}. The width of the distribution in the mixing enthalpy affects the symmetry x → 1 − x in the mixing free energies curves, with the curves for CsPb(I_{1−x}Br_{x})_{3} being the most and those for FAPb(I_{1−x}Br_{x})_{3} the least symmetric. This has an effect on the symmetry of the phase diagrams, as we will show further on.
Lightinduced halide segregation
The key ingredient of our unified theory for lightinduced halide segregation is the consideration of the combination of the compositional free energy in the dark and the free energy of photocarriers in the presence of illumination. Photocarriers can reduce their free energy by funneling to lowband gap domains^{23}, which leads to a driving force for halide demixing, as illustrated in Fig. 2a. It is well known that halide anions in metalhalide perovskites are quite mobile. Because of stochastic fluctuations in halide composition, Irich regions with lower band gap than the parent phase will spontaneously arise. Accumulation of diffusing photocarriers in these regions will reduce the photocarrier free energy. The free energy can then be further reduced by the growth of these regions by inward diffusion of I, leading to nucleation of an Irich phase and to phase separation. Because the stoichiometry cannot change, the inward diffusion of I should be accompanied by the outward diffusion of Br.
In our theory, band gap differences of perovskites with different halide compositions play a central role. Figure 2b shows the band gaps as a function of Br concentration x for the five compounds. The band gaps of the three singlecation perovskites are obtained from experiment^{17,18,19}, while the band gaps of the two doublecation perovskites are obtained from an interpolation scheme (see Supplementary Note 2). The differences in band gap for different halide compositions are mainly caused by differences in the energy of the valence band maxima, where an increase in Br concentration decreases the energy of the valence band maximum^{23}. So, it will be mainly the photogenerated holes that can reduce their free energy by funneling into Irich domains. The electrons will follow the holes to establish local charge neutrality. The steepness of the band gap curves decreases for different cation compositions in the order FA–FA_{7/8}Cs_{1/8}–MA–MA_{7/8}Cs_{1/8}–Cs, following the decreasing trend in the (average) cation size. The decrease in the steepness of the band gap curves with Cs alloying may look surprising because the Asite cation does not directly contribute to the states governing the band gap. However, Acation alloying can change the band gap indirectly by changing the volume of the unit cell or by introducing octahedral distortions^{35}.
The total system consisting of the perovskite with its distribution of halide anions and the generated photocarriers will try to lower its free energy by combined motion of halide anions and photocarriers. The free energy of the total system is the compositional free energy of the perovskite for a certain distribution of the halide anions (the free energy in the dark) and the free energy of a certain distribution of the photocarriers. Because the diffusion of photocarriers is much faster than that of the halide anions, the distribution of the carriers over the different phases will be at any moment in time in equilibrium. We define n as the density of photogenerated electrons or holes per formula unit in the mixed phase. When n ≪ 1, we can use Boltzmann instead of FermiDirac statistics for the distribution of photocarriers. If phase separation occurs into two phases with Br concentrations x_{1} and x_{2}, the photocarriers will redistribute over these two phases according to the Boltzmann factors \(\exp \left({E}_{{\rm{g}}}({x}_{1})/{k}_{{\rm{B}}}T\right)\) and \(\exp \left({E}_{{\rm{g}}}({x}_{2})/{k}_{{\rm{B}}}T\right)\), where E_{g}(x) is the band gap as a function of Br concentration x and k_{B}T the thermal energy. This leads to
where n_{1} and n_{2} are the photocarrier densities in the two phases. With ϕ_{1} and ϕ_{2} the corresponding volume fractions of the two phases, the mixing free energy ΔF^{⋆} per formula unit under illumination then becomes
Neglecting the small volume difference per formula unit between the two phases, the conditions ϕ_{1} + ϕ_{2} = 1 and ϕ_{1}x_{1} + ϕ_{2}x_{2} = x should hold. The sum of the first and second terms in Eq. (2) is the volumeweighted compositional mixing free energy in the dark. The sum of the third and fourth terms is the photocarrier contribution to the free energy. Because the band gap difference between the Irich and parent phase is in general much larger than the thermal energy (k_{B}T ≈ 25 meV at room temperature), even a low illumination intensity can according to Eq. (1) lead to a relatively large change of ΔF^{⋆}, which manifests the funneling effect.
In steady state, the rate of generation of photocarriers in the system should be equal to the sum of the rates of photocarrier annihilation by monomolecular and bimolecular recombination in the different phases:
Here, G is the photocarrier generation rate per formula unit, which is proportional to the illumination intensity. The monomolecular and bimolecular recombination rates are given by an inverse photocarrier lifetime τ and a bimolecular recombination rate constant k, for which we take τ = 100 ns and k = 10^{−10} cm^{3} s^{−1}, applicable for a standard MAPbI_{3} film^{43}. For the volume per formula unit V we take the value 2.5 × 10^{−22} cm^{3} for MAPbI_{3} (see Supplementary Note 1).
Equations (1–3) are the basis of our unified theory for lightinduced halide segregation. With Eqs. (1) and (3), n_{1} and n_{2} can be calculated for a given G. Insertion in Eq. (2) then yields the mixing free energy under illumination, from which the spinodal and binodal for halide phase segregation can be obtained (see ‘Methods’). We note that Eqs. (1–3) are only generally applicable if the diffusion lengths of the photogenerated holes and electrons are large compared to the feature sizes of the demixing. In that case, an equilibrium distribution of holes and electrons is established over the two phases throughout the system, with a homogeneous photocarrier density in each phase. However, we will use these equations only to determine the onset of phase separation. The sizes of the nuclei are then much smaller than the diffusion lengths so that the distribution of holes and electrons within the nuclei is homogeneous. The distribution in the parent phase can then still be inhomogeneous, but this does not affect the applicability of our theory to the onset of phase separation (see Supplementary Note 3).
Phase diagrams
In Fig. 3a–e we show the xT phase diagrams for the five mixed compounds in the dark, obtained from Eq. (2) for vanishing photocarrier density. The red lines are the spinodals separating the metastable (grey) and unstable (pink) regions. The blue lines are the binodals separating the stable (white) and metastable regions. Apart from FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, miscibility gaps appear below the critical points (x_{c}, T_{c}), where the critical temperature T_{c} is below room temperature. This means that at room temperature the mixed compounds are thermodynamically stable. The critical temperatures decrease for different cation compositions in the order MA–FA–Cs–MA_{7/8}Cs_{1/8}. The results show that changing MA by FA as well as mixing in Cs in the MA and FA compounds has a stabilizing effect in the dark. The amount of asymmetry in the phase diagrams under the change x → 1 − x in Fig. 3a–e is in accordance with the amount of asymmetry in the free energy curves shown in Fig. 1k–o. The compound FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} is special in the sense that it is stable in the dark for all values of x and T. Like MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, the free energy curves are strongly asymmetric, but in contrast to MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} no points of common tangent or inflection points occur, which would be the locations of the binodals and spinodals, respectively; see Fig. 1l and o. We checked that this situation does not change for T < 150 K, which is the lowest temperature in Fig. 1, so that there is no critical temperature.
We note that in the case of MAPb(I_{1−x}Br_{x})_{3} our phase diagram in the dark differs from that of Brivio et al.^{42}. In particular, our T_{c} of 266 K is below the value of 343 K in ref. ^{42}. The reason for the difference is that in ref. ^{42} the symmetry lowering by the specific orientation of the MA cations is neglected, leading to a reduction of the number of considered different configurations of the halide anions. The finding that our T_{c} is below room temperature is in agreement with the observation that MAPb(I_{1−x}Br_{x})_{3} does not phase separate at room temperature in the dark^{22}. This comparison does show that subtle differences in the way the free energy is calculated can have a substantial influence on the phase diagram. Therefore, also our phase diagrams can have inaccuracies that are related to, e.g. the specific exchangecorrelation functional used in the DFT calculations (see ‘Methods’) and the limited size of the used supercells. Also, thermally induced random orientations of the MA and FA molecules^{44} can influence the phase diagrams. On the other hand, we expect that the observed trends in the phase diagrams are reliable, because the relative accuracies in the calculations of the free energies under I ↔ Br exchange for the investigated compounds are expected to be better than the absolute accuracies. It is important to note at this point that the threshold photocarrier densities for lightinduced halide segregation (see next section) mainly depend on band gap differences and are hardly influenced by the phase diagrams in the dark.
Figure 3f–t show the phase diagrams of the five compounds under illumination, obtained from Eqs. (1–3) for different photocarrier densities in the mixed state of n = 10^{−9}, 10^{−7}, and 10^{−5}/f.u. Using an absorption coefficient α = 10^{5} cm^{−1} and a photon energy hν = 3 eV^{23}, a value of n = 5 × 10^{−7}/f.u. corresponds to an illumination intensity I = 100 mW cm^{−2} of ~1 Sun (n ≈ IαVτ/hν when we neglect bimolecular recombination in the mixed state). We observe that the spinodals only slightly change with increasing photocarrier density. By contrast, important changes occur in the behaviour of the binodals with increasing n. Our theory predicts the existence of two types of binodals. The first type (full blue lines) can be viewed as a modification of the dark binodals by the illumination, which we will call ‘compositional binodals’. Under illumination, a new type of binodals appears (full green lines), which we will call ‘lightinduced binodals’. These binodals can be crossed by increasing the illumination intensity, but also by decreasing the temperature. The latter is a prediction of our theory that is experimentally testable.
With increasing photocarrier density, the phase diagrams fall into two categories, observable for all compounds except FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}. (1) At low photocarrier density n = 10^{−9}/f.u. (Fig. 3f–i) the compositional binodals connect to the lightinduced binodals after the critical point and both left and right branches of the binodals exist. When the left (right) branches of the compositional binodals are crossed by increasing (decreasing) x or decreasing T, a phase is nucleated that is Brricher (Iricher) than the parent phase, indicated by the dashed blue lines. We note that the dashed blue lines do not exactly coincide with the full blue lines at the top of the binodals. (2) At high photocarrier density n = 10^{−5}/f.u. (Fig. 3p–s) the compositional binodals connect to the green binodals before the critical point and only left branches of the compositional binodals exist. Figure 3k displays for MAPb(I_{1−x}Br_{x})_{3} a phase diagram that is very close to the transition between the two categories of phase diagrams, whereas Fig. 3l–n show both category1 and category2 phase diagrams for FAPb(I_{1−x}Br_{x})_{3}, CsPb(I_{1−x}Br_{x})_{3}, and MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}.
For both categories of phase diagrams, a phase is nucleated that is Iricher than the parent phase when the lightinduced binodals are crossed by increasing x or decreasing T, as indicated by the green dashed lines. Interestingly, triple points \(({x}_{{\rm{tr}}},{T}_{{\rm{tr}}})\) exist where two different phases with different halide composition can be nucleated from the parent phase. The Br concentrations of the parent phase (\({x}_{{\rm{tr}}}\)) and the two phases that can be nucleated at the triple points are indicated by dots in Fig. 3. For category1 phase diagrams, the Br concentrations of the nucleated phases at the triple points (blue and green dots) both have a lower Br concentration than the parent phase (black dot), whereas for the category2 phase diagram one nucleated phase is Brricher and the other is Iricher than the parent phase. The predictions of two categories of phase diagrams and the existence of triple points are unique features of our theory. Their experimental observation by careful experimentation would be extremely interesting and could substantially increase our knowledge of lightinduced halide segregation. MAPb(I_{1−x}Br_{x})_{3} could be a good candidate to experimentally investigate the occurrence of triple points. It is predicted by us to have the highest critical temperature (266 K) of the investigated compounds. This has the advantage that the thermally activated motion of the halide ions is the least suppressed around the critical point, which facilitates the observation of the segregation. Down to 235 K, for which MAPbBr_{3} shows a cubic to tetragonal transition^{45}, no interfering structural transitions are expected. One can take x slightly higher or slightly lower than the critical Br concentration x_{c} = 0.35 to investigate the triple points of the type shown in Fig. 3f and p, respectively. By tuning the temperature and the illumination level these triple points can then be searched for by looking at, e.g. different features in the absorption spectrum.
Our finding that x ≈ 0 for the photosegregated Irich phase (see the dashed green lines in Fig. 3) seems at odds with the experimental finding of Hoke et al. that x ≈ 0.2 when segregation is complete^{22}. An explanation for the latter finding was given by Ruth et al.^{46}. In their kinetic Monte Carlo simulations of vacancymediated hopping of I and Br ions during the phase segregation process, Br ions get kinetically trapped in the Irich nuclei, with a final concentration close to 0.2. Our theory applies to the onset of phase segregation and is therefore not incompatible with this result. There is recent experimental evidence from photoluminescence measurements that halide segregation commences with an almost Ipure phase, which gradually becomes less pure by the inclusion of Br^{47,48}. This is in line with our argument.
Threshold photocarrier densities
Figure 4 shows for the five compounds results for the threshold photocarrier density n_{t} for halide segregation. This is the value of n at which the lightinduced binodals are crossed for a given Br concentration x and temperature T (the full green lines in Fig. 3f–t). The lightinduced nucleated phase is almost 100% Irich (see the dashed green lines in Fig. 3f–t). From this fact, the following very accurate expression can be derived for n_{t} (see ‘Methods’):
where ΔE_{g}(x) ≡ E_{g}(x) − E_{g}(0). The prefactor in this expression is \(f(x,T)\equiv \sqrt{\left({{\Delta }}F(x,T)+x{\partial }_{x}{{\Delta }}F(x,T)\right)V/k\tau {E}_{{\rm{g}}}(x)}\). Equation (4) predicts extremely low thresholds n_{t} at room temperature. We note that n_{t} is the threshold photocarrier density in the mixed phase or in the parent phase at the onset of phase separation. The photocarrier density in the nucleated phase is according to Eq. (1) much larger. For example, for MAPb(I_{0.5}Br_{0.5})_{3} we have ΔE_{g}(x = 0.5) ≈ 0.28 eV (see the green line in Fig. 2b), so that the photocarrier density in the almost Ipure nucleated phase is at room temperature a factor of about 7 × 10^{4} larger. This also means that, while the bimolecular recombination in the mixed or in the parent phase is negligible, this is definitely not the case in the nucleated phase.
In Fig. 4a we show n_{t} as a function of Br concentration x at room temperature. Apart from the extremely low n_{t}, an extremely strong dependence on x is found. The threshold n_{t} increases for different cation composition in the order FA–FA_{7/8}Cs_{1/8}–MA– MA_{7/8}Cs_{1/8}–Cs, which is the same order as the decrease in the steepness of the band gap curves in Fig. 2b. This order and the extremely strong dependence of n_{t} on x can be explained from the exponential factor \(\exp ({{\Delta }}{E}_{{\rm{g}}}(x)/{k}_{{\rm{B}}}T)\) in Eq. (4). We thus come to the important conclusion that the threshold photocarrier density is governed by the band gap difference of the mixed halide compound and the Ipure compound.
In Fig. 4b we show the Tdependence of n_{t} at Br concentration x = 0.5 and in Fig. 4c the Tdependence of x at a low, n_{t} = 10^{−9}/f.u., and a high, n_{t} = 10^{−5}/f.u., threshold photocarrier density. Both figures cover the temperature interval 300–350 K, which is a relevant operational range for solar cells. All curves in Fig. 4b are below the photocarrier density n = 5 × 10^{−7}/f.u. at 1 Sun (dashed horizontal line), showing that all compounds with equal amounts of Br and I segregate at 1 Sun illumination. The steepness of the curves in Fig. 4b follows the same order as the steepness of the band gap curves in Fig. 2b. For both values of n_{t} the curves in Fig. 4c show a decrease in steepness for the different compounds with an order that is opposite to the order in which the steepness of the band gap curves decreases. At the same time, the steepness of the curves for all compounds increases approximately proportionally to the logarithm of n_{t}. All these observations can be explained from the exponential factor \(\exp ({{\Delta }}{E}_{{\rm{g}}}(x)/{k}_{{\rm{B}}}T)\) in Eq. (4), although the factor f(x, T) also contributes somewhat to the Tdependence.
Our results for the photostability of the different compounds agree with experimentally observed trends. First, we find that CsPb(I_{1−x}Br_{x})_{3} is more photostable than MAPb(I_{1−x}Br_{x})_{3}. This is consistent with the experimental observations that MAPb(I_{1−x}Br_{x})_{3} is found to segregate for bromine concentrations 0.2 < x < 1^{22,40}, while CsPb(I_{1−x}Br_{x})_{3} shows a smaller instability range 0.4 < x < 1^{17}. Second, we find that partial Cs alloying improves photostability, which is in agreement with the observed enhanced photostability by partial substitution of the organic cation in MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3} by Cs^{6,28,30,31,32,33,34}. This enhanced photostability is a direct consequence of the reduced dependence of the band gap on the Br concentration x in Fig. 2b. To investigate if the trend of increasing stability with Cs loading pursues, we show in Supplementary Fig. 2d–f in Supplementary Note 4 phase diagrams in the dark and for photocarrier densities n = 10^{−9} and 10^{−7}/f.u. of MA_{3/4}Cs_{1/4}Pb(I_{1−x}Br_{x})_{3}, where the Cs loading is 25% instead of the 12.5% loading in MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}. The phase diagrams are very similar to the latter compound, but are shifted down in temperature. The critical temperature decreases from 266 K without Cs loading (MAPb(I_{1−x}Br_{x})_{3}), to 244 K for 12.5% loading, and 216 K for 25% loading, indeed showing a trend of increasing stability. This trend should be broken when increasing the Cs loading further, because for 100% Cs loading (CsPb(I_{1−x}Br_{x})_{3}) the critical temperature is 250 K (see Fig. 3c). Supplementary Fig. 2g–i in Supplementary Note 4 show plots equivalent to Fig. 4a–c for MA_{3/4}Cs_{1/4}Pb(I_{1−x}Br_{x})_{3}. The photocarrier density threshold is slightly higher than that of MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, confirming the trend of increased photostability with increasing Cs loading.
Using MAPb(I_{0.5}Br_{0.5})_{3} as an example, we predict at 300 K a photocarrier density threshold of n_{t} = 9 × 10^{−9}/f.u. (see the green line in Fig. 4b), corresponding to an illumination threshold of 1750 μW cm^{−2}. In the recent experiments of ref. ^{25} a threshold for MAPb(I_{0.5}Br_{0.5})_{3} of about 35 μW cm^{−2} is reported. We also predict an increase of the illumination threshold by a factor of 5.5 between 300 and 350 K, as compared to the experimentally found increase by a factor of about 3^{25}. Considering the extremely strong sensitivity of n_{t} to the various quantities in our theory, we find the agreement satisfactory. We note in particular the extremely strong dependency of n_{t} on the Br concentration x (see Fig. 4a), which leads to an extremely large sensitivity of the illumination threshold to preparation details of the perovskite film. The model of Ruth et al.^{46} for the illumination threshold used in ref. ^{25} has a linear dependence on temperature and therefore predicts an increase of only about 17% between 300 and 350 K. We note that in this model the carrier diffusion lengths of electrons and holes, and a ‘geometrical band gap volume’ appear as parameters, quantities that do not appear in our theory.
It was recently reported that MAPb(I_{0.2}Br_{0.8})_{3} remixes for an illumination intensity of 200 W cm^{−2}^{37}. This is equivalent to about 2000 Sun, which corresponds to a photocarrier density in the parent phase of about 10^{−3}/f.u. Using Eq. (1) and the band gap difference between x_{1} = 0.8 (parent phase) and x_{2} = 0 (nucleated phase), we would find at room temperature a photocarrier density in a potentially nucleated phases of about 1.2 × 10^{6}/f.u. Obviously, our theory can no longer be applied at such extremely high densities, causing, among other things, a breakdown of the Boltzmann approximation used in Eq. (1). The explanation for the remixing could be that at these extreme densities there will be such a large spillover of photocarriers from the nucleated phase into the parent phase that the driving force for halide segregation disappears. This will essentially restore the conditions in the dark, where the mixed situation is favoured.
We remark that our theory has no adjustable parameters and can be the starting point for the inclusion of effects that were not yet accounted for. One such effect could be that the number of defects in the nucleated phase is larger than in the parent phase, possibly caused by a lattice mismatch between the two phases. This could lead to a lower photocarrier lifetime τ in the nucleated phase, which presently is assumed to be the same as in the parent phase. A lower τ in the nucleated phase will lead to a lower n_{t}. Another effect that will lower n_{t} is a lattice compression of the Irich nuclei by the surrounding mixed parent phase with smaller lattice constant, leading to a lowering of the band gap in the nucleated phase. If we take for MAPbI_{3} under compressional strain the MAPb(I_{0.5}Br_{0.5})_{3} lattice constant instead of its relaxed lattice constant, we find that the calculated DFT band gap is decreased by 0.145 eV. Using Eq. (4), this implies a decrease in n_{t} by a factor of about 300 at room temperature and thus a six times lower illumination threshold than in the experiment of ref. ^{25}. In reality, the lattice adjustment to the surrounding phase will not be complete, so that a refined analysis may lead to a result in closer agreement with the experiment.
The consequence of the mechanism for lightinduced halide segregation studied here is that the attractive band gap tunability of mixed halide perovskites at the same time leads to photostability problems. Nevertheless, routes towards optimal solutions follow from our study. For example, Fig. 4a shows that at 1 Sun illumination and room temperature CsPb(I_{1−x}Br_{x})_{3} should be photostable up to 42% Br concentration. This allows, according to Fig. 2b, reaching a band gap of 1.94 eV. This is more than sufficient for the top layer in an efficient tandem solar cell, which has an optimal band gap of 0.96 eV for the bottom and 1.63 eV for the top cell. For MAPb(I_{1−x}Br_{x})_{3} and MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, Br concentrations of about 33% and 35% can be reached, allowing band gaps of 1.73 and 1.78 eV, respectively, which are both still sufficient.
Discussion
We have presented a unified thermodynamic theory for lightinduced halide segregation in mixed halide perovskites. The theory is based on minimization of the sum of a compositional free energy, obtained from binary alloying theory, and an electronic free energy of photocarriers, which distribute thermally over a nucleated phase and a parent phase with different band gaps due to different IBr compositions. We applied the theory to MAPb(I_{1−x}Br_{x})_{3}, FAPb(I_{1−x}Br_{x})_{3}, CsPb(I_{1−x}Br_{x})_{3}, as well as the partial Cs compounds MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} and FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}. The spinodals in the Br concentrationtemperature, xT, phase space, separating unstable and metastable regions, only slightly change for photocarrier densities corresponding to relevant illumination intensities. In addition to compositional binodals that are also present in the dark, new lightinduced binodals appear, signalling the nucleation of an Irich phase from the parent phase. These binodals, which are attributed to funneling of photocarriers into the lowband gap Irich phase, occur at an extremely small photocarrier density and illumination intensity governed by the band gap difference between the mixed phase and the nucleated Irich phase.
Several predictions of the theory are in agreement with experimental findings, such as a strongly temperature and composition dependent illumination threshold for halide segregation and a stabilization effect upon alloying FA or MA with Cs. The fundamental reason for this stabilization effect is that mixing Cs into FA or MA reduces the unit cell volume, leading to smaller band gap differences between the parent and I rich phases. The theory predicts two categories of phase diagrams and the existence of photocarrier densitydependent triple points \(({x}_{{\rm{tr}}},{T}_{{\rm{tr}}})\) below room temperature, where two phases with different BrI compositions can be nucleated from the parent phase. The experimental study of these novel physical phenomena would be extremely interesting and increase our understanding of lightinduced halide segregation. The theory is flexible and transferable, making it a suitable starting point for refinements to include effects that have not yet been considered, such as different recombination rates in the different phases and changes in the band gap due to strain. The theory can also be readily applied to other semiconductors where the band gap is tuned by alloying.
We finally note that a metastable region in phase space is entered when the illumination intensity exceeds the threshold for halide segregation. According to nucleation theory, a surface free energy due to the presence of an interface between the nucleated and parent phase could inhibit phase separation. Phase separation then requires the crossing of a free energy barrier composed of a positive surface free energy and the negative bulk free energy for a nucleus of a critical size. For the investigation of a phase separation inhibition effect, it would be important to evaluate the surface free energy between a mixed IBr and an Irich phase, and the probability that a nucleus will grow spontaneously to a critical size. Differences in surface free energy and sizes of critical nuclei for different perovskites could provide additional handles to suppress lightinduced halide segregation. We suggest that the delayed onset for the acceleration of the segregation reported in ref. ^{38} is related to the induction time for the formation of critical nuclei. The existence of such an induction time is a wellknown phenomenon in nucleation theory^{49}.
Methods
Calculation of total energies
To calculate the total energies of the singlecation mixed halide perovskites MAPb(I_{1−x}Br_{x})_{3}, FAPb(I_{1−x}Br_{x})_{3}, and CsPb(I_{1−x}Br_{x})_{3}, we start from a periodic supercell of the pure I compounds containing 2 formula units, with a 2 × 1 × 1 expansion of a (pseudo)cubic perovskite building block. We then replace I anions by Br anions at different concentrations x = 0, 1/6, 1/3, 1/2, 2/3, 5/6, 1. The total number of possible configurations for each singlecation perovskite is 2^{6} = 64. For the Cs perovskite with perfect O_{h} symmetry the three halide sites are equivalent, which reduces the total number of inequivalent configurations to 21. Accounting for the deviation from O_{h} symmetry in the case of the MA and FA perovskites leads to an increase to 36 inequivalent configurations. To include the Cs cations in the doublecation perovskites MA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3} and FA_{7/8}Cs_{1/8}Pb(I_{1−x}Br_{x})_{3}, the 2 × 1 × 1 supercells of the 36 inequivalent MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3} configurations are repeated in two directions to construct 2 × 2 × 2 supercells containing 8 formula units. The doublecation perovskites are then constructed by substituting one of the 8 organic cations by Cs. The total number of inequivalent configurations is then 2 × 36 = 72, where factor 2 reflects the two inequivalent Cs substitutions in the 2 × 2 × 2 supercell. In the case of MA_{3/4}Cs_{1/4}Pb(I_{1−x}Br_{x})_{3}, studied in Supplementary Note 4, we substitute two of the MA cations on the body diagonal of the supercell by Cs cations, preserving in this way symmetry as much as possible.
The total energy calculations are performed within DensityFunctional Theory (DFT). We use the projected augmented wave (PAW)^{50} method and the PerdewBurkeErnzerhof exchangecorrelation functional revised for solids (PBEsol)^{51} within the generalized gradient approximation (GGA)^{52}, as implemented in the Vienna ab initio simulation package (VASP)^{53}. We use 4 × 8 × 8 and 4 × 4 × 4 kpoint Brillouin zone samplings for the singlecation and doublecation compounds, respectively, and a planewave kinetic energy cutoff of 500 eV. The shape and volume of the unit cell as well as the atomic positions in the unit cell of each configuration are fully optimized. The energy and force convergence parameters are set at 0.01 meV and 0.005 eV/Å, respectively.
Calculation of the mixing free energy
The mixing enthalpies ΔU_{j} per formula unit of the inequivalent configurations j = 1, … J with relative Br concentration x are given by
where E_{j}, \({E}_{{{\rm{APbI}}}_{3}}\), and \({E}_{{{\rm{APbBr}}}_{3}}\) are the total energies per formula unit of configuration j, the pure I configuration, and the pure Br configuration, respectively. ‘A’ denotes MA, FA, Cs, MA_{7/8}Cs_{1/8}, or FA_{7/8}Cs_{1/8}. The resulting enthalpies are given by the J = 36 points in Fig. 1f, g for MAPb(I_{1−x}Br_{x})_{3} and FAPb(I_{1−x}Br_{x})_{3}, respectively, and the J = 21 points in Fig. 1h for CsPb(I_{1−x}Br_{x})_{3}. To treat the doublecation perovskites on the same footing as the singlecation perovskites we take the average of the total energies of the two inequivalent Cs substitutions, resulting in enthalpies given by the J = 36 points in Fig. 1i, j. We checked that the mixing free energy curves (see below) for the two inequivalent Cs substitutions are almost indistinguishable, which validates taking this average.
We apply the quasichemical approximation (QCA)^{41} to obtain the mixing enthalpy ΔU(x, T), entropy ΔS(x, T), and Helmholtz free energy ΔF(x, T) as functions of the Br concentration x and temperature T. The QCA has been successfully employed in the thermodynamic analysis of semiconductor alloys^{42,54,55}. In the QCA, the perovskite lattice is decomposed into microclusters, which are treated independently^{41}. For the different microclusters we take the J inequivalent configurations mentioned above. In the QCA, the thermal equilibrium fraction of microclusters with configuration j is given by
where g_{j} is the degeneracy and n_{j}(Br) = 0, 1, 2, 3 the number of Br anions per formula unit of the configuration, and μ_{Br} is the Br chemical potential. This chemical potential should be determined such that the desired Br concentration is obtained:
After having found μ_{Br} from this condition, the mixing enthalpy and entropy per formula unit are obtained as:
and
with \({x}_{j}^{0}={g}_{j}{x}^{{n}_{j}({\rm{Br}})}{(1x)}^{3{n}_{j}({\rm{Br}})}\). The mixing free energy is finally obtained as ΔF(x, T) = ΔU(x, T) − TΔS(x, T).
Determination of the binodals and spinodals
To find the binodals we consider the possibility, starting from the mixed situation with Br concentration x, to decrease the free energy by demixing through nucleation of a phase with a concentration x_{2} ≠ x with a small volume fraction δϕ ≡ ϕ_{2}. In the mixed situation we can make the simplifying approximation n ≈ G/τ for the photocarrier density, because for all relevant illumination intensities bimolecular recombination is then negligible. The free energy Eq. (2) in the mixed situation is ΔF^{⋆}(x, x, 1, 0, T), while the free energy in the demixed situation is ΔF^{⋆}(x_{1}, x_{2}, 1 − δϕ, δϕ, T), with, to linear order in δϕ,
The difference in free energy between the demixed and mixed situations is then to linear order in δϕ:
with ∂_{x}ΔF(x, T) ≡ ∂ΔF(x, T)/∂x. When δΔF^{⋆} < 0, the demixed situation has lower free energy than the mixed situation. We thus find the binodals in Fig. 3 for a certain photocarrier density n by looking in xT phase space for a value of x_{2} of a nucleated phase for which δΔF^{⋆} = 0. The dashed lines in Fig. 3 give the Br concentration x_{2} of the nucleated phase. For the lightinduced binodals x_{2} is very small, indicating the nucleation of a lowband gap Irich phase. When we put x_{2} = 0 in Eq. (11) we get
where ΔE_{g}(x) = E_{g}(x) − E_{g}(0) is the band gap difference between the mixed and the pure I phase. The term \(x{E}_{{\rm{g}}}^{\prime}(x)\) is found to be very small and can be neglected. Putting δΔF^{⋆} = 0 and solving for n yields the threshold photocarrier density Eq. (4), which provides an extremely good approximation to the curves in Fig. 4.
To find the spinodals we consider the possibility to decrease the free energy by generating a volume fraction ϕ of a phase with a slightly different concentration x_{2} = x + δx. The free energies in the demixed situation can now be written as ΔF^{⋆}(x − ϕδx/(1 − ϕ), x + δx, 1 − ϕ, ϕ, T). To second order in δx the difference in free energy then becomes
When δΔF^{⋆} < 0, the demixed situation can be established from the mixed situation in a continuous way, without crossing a free energy barrier. Putting δΔF^{⋆} = 0 thus yields the spinodal separating the metastable from the unstable region in xT phase space.
We note that for the unilluminated case (n = 0, see the top panels in Fig. 3) the above procedures to find the binodals and spinodals are identical to the usual procedures, where the binodals are found from a common tangent construction and the spinodals from the inflection points of ΔF as a function of x. These usual procedures can be applied when the mixing free energy is equal to the volumeweighted sum of the free energies per volume of the different phases, which holds in the dark but not under illumination.
Data availability
Code availability
The DFT calculations were performed with the code VASP (‘Vienna Ab initio Simulation Package’), available at http://www.vasp.at.
References
Kojima, A., Teshima, K., Shirai, Y. & Miyasaka, T. Organometal halide perovskites as visiblelight sensitizers for photovoltaic cells. J. Am. Chem. Soc. 131, 6050–6051 (2009).
Green, M. A., HoBaillie, A. & Snaith, H. J. The emergence of perovskite solar cells. Nat. Photonics 8, 506–514 (2014).
Noel, N. K. et al. Leadfree organicinorganic tin halide perovskites for photovoltaic applications. Energy Environ. Sci. 7, 3061–3068 (2014).
Stranks, S. D. & Snaith, H. J. Metalhalide perovskites for photovoltaic and lightemitting devices. Nat. Nanotechnol. 10, 391–402 (2015).
Jeon, N. J. et al. Compositional engineering of perovskite materials for highperformance solar cells. Nature 517, 476–480 (2015).
McMeekin, D. P. et al. A mixedcation lead mixedhalide perovskite absorber for tandem solar cells. Science 351, 151–155 (2016).
Lin, K. et al. Perovskite lightemitting diodes with external quantum efficiency exceeding 20 percent. Nature 562, 245–248 (2018).
Jung, E. H. et al. Efficient, stable and scalable perovskite solar cells using poly(3hexylthiophene). Nature 567, 511–515 (2019).
Yi, C. et al. Entropic stabilization of mixed Acation ABX_{3} metal halide perovskites for high performance perovskite solar cells. Energy Environ. Sci. 9, 656–662 (2016).
Saliba, M. et al. Cesiumcontaining triple cation perovskite solar cells: improved stability, reproducibility and high efficiency. Energy Environ. Sci. 9, 1989–1997 (2016).
Li, N. et al. Cation and anion immobilization through chemical bonding enhancement with fluorides for stable halide perovskite solar cells. Nat. Energy 4, 408–415 (2019).
Zuo, F. et al. Binarymetal perovskites toward highperformance planarheterojunction hybrid solar cells. Adv. Mater. 26, 6454–6460 (2014).
Hao, F., Stoumpos, C. C., Chang, R. P. & Kanatzidis, M. G. Anomalous band gap behavior in mixed Sn and Pb perovskites enables broadening of absorption spectrum in solar cells. J. Am. Chem. Soc. 136, 8094–8099 (2014).
Anaya, M. et al. Optical analysis of CH_{3}NH_{3}Sn_{x}Pb_{1−x}I_{3} absorbers: a roadmap for perovskiteonperovskite tandem solar cells. J. Mater. Chem. A 4, 11214–11221 (2016).
Goyal, A. et al. Origin of pronounced nonlinear band gap behavior in leadtin hybrid perovskite alloys. Chem. Mater. 30, 3920–3928 (2018).
Jung, Y. K., Lee, J. H., Walsh, A. & Soon, A. Influence of Rb/Cs cationexchange on inorganic Sn halide perovskites: from chemical structure to physical properties. Chem. Mater. 29, 3181–3188 (2017).
Beal, R. E. et al. Cesium lead halide perovskites with improved stability for tandem solar cells. J. Phys. Chem. Lett. 7, 746–751 (2016).
Noh, J. H., Im, S. H., Heo, J. H., Mandal, T. N. & Seok, S. I. Chemical management for colorful, efficient, and stable inorganicorganic hybrid nanostructured solar cells. Nano Lett. 13, 1764–1769 (2013).
Eperon, G. E. et al. Formamidinium lead trihalide: a broadly tunable perovskite for efficient planar heterojunction solar cells. Energy Environ. Sci. 7, 982–988 (2014).
Bush, K. A. et al. 23.6%efficient monolithic perovskite/silicon tandem solar cells with improved stability. Nat. Energy 2, 1–7 (2017).
Rajagopal, A. et al. Highly efficient perovskiteperovskite tandem solar cells reaching 80% of the theoretical limit in photovoltage. Adv. Mater. 29, 1–10 (2017).
Hoke, E. T. et al. Reversible photoinduced trap formation in mixedhalide hybrid perovskites for photovoltaics. Chem. Sci. 6, 613–617 (2015).
Draguta, S. et al. Rationalizing the lightinduced phase separation of mixed halide organicinorganic perovskites. Nat. Commun. 8, 1–8 (2017).
Wang, X. et al. Suppressed phase separation of mixedhalide perovskites confined in endotaxial matrices. Nat. Commun. 10, 1–7 (2019).
Elmelund, T., Seger, B., Kuno, M. & Kamat, P. V. How interplay between photo and thermal activation dictates halide ion segregation in mixed halide perovskites. ACS Energy Lett. 5, 56–63 (2020).
Hu, M., Bi, C., Yuan, Y., Bai, Y. & Huang, J. Stabilized wide bandgap MAPbBr_{x}I_{3−x} perovskite by enhanced grain size and improved crystallinity. Adv. Sci. 3, 6–11 (2015).
Yang, Z. et al. Stabilized wide bandgap perovskite solar cells by tin substitution. Nano Lett. 16, 7739–7747 (2016).
Hutter, E. M. et al. Thermodynamic stabilization of mixedhalide perovskites against phase segregation. Cell Rep. Phys. Sci. 1, 100120 (2020).
Xu, J. et al. Triplehalide wideband gap perovskites with suppressed phase segregation for efficient tandems. Science 367, 1097–1104 (2020).
Braly, I. L. et al. Currentinduced phase segregation in mixed halide hybrid perovskites and its impact on twoterminal tandem solar cell design. ACS Energy Lett. 2, 1841–1847 (2017).
Rehman, W. et al. Photovoltaic mixedcation lead mixedhalide perovskites: links between crystallinity, photostability and electronic properties. Energy Environ. Sci. 10, 361–369 (2017).
Dang, H. X. et al. Multication synergy suppresses phase segregation in mixedhalide perovskites. Joule 3, 1746–1764 (2019).
Bischak, C. G. et al. Tunable polaron distortions control the extent of halide demixing in lead halide perovskites. J. Phys. Chem. Lett. 9, 3998–4005 (2018).
Bush, K. A. et al. Compositional engineering for efficient wide band gap perovskites with improved stability to photoinduced phase segregation. ACS Energy Lett. 3, 428–435 (2018).
Tao, S. et al. Absolute energy level positions in tin and leadbased halide perovskites. Nat. Commun. 10, 1–10 (2019).
Bischak, C. G. et al. Origin of reversible photoinduced phase separation in hybrid perovskites. Nano lett. 17, 1028–1033 (2017).
Mao, W. et al. Lightinduced reversal of ion segregation in mixedhalide perovskites. Nat. Mater. 20, 55–61 (2021).
Knight, A. J. et al. Electronic traps and phase segregation in lead mixedhalide perovskite. ACS Energy Lett. 4, 75–84 (2018).
Belisle, R. A. et al. Impact of surfaces on photoinduced halide segregation in mixedhalide perovskites. ACS Energy Lett. 3, 2694–2700 (2018).
Barker, A. J. et al. Defectassisted photoinduced halide segregation in mixedhalide perovskite thin films. ACS Energy Lett. 2, 1416–1424 (2017).
Sher, A. et al. Quasichemical approximation in binary alloys. Phys. Rev. B 36, 4279–4295 (1987).
Brivio, F., Caetano, C. & Walsh, A. Thermodynamic origin of photoinstability in the CH_{3}NH_{3}Pb(I_{1−x}Br_{x})_{3} Hybrid Halide Perovskite Alloy. J. Phys. Chem. Lett. 7, 1083–1087 (2016).
Johnston, M. B. & Herz, L. M. Hybrid perovskites for photovoltaics: chargecarrier recombination, diffusion, and radiative efficiencies. Acc. Chem. Res. 49, 146–154 (2016).
Dalpian, G. M., Zhao, X. G., Kazmerski, L. & Zunger, A. Formation and compositiondependent properties of alloys of cubic halide perovskites. Chem. Mater. 31, 2497–2506 (2019).
Keshavarz, M. et al. Tracking structural phase transitions in leadhalide perovskites by means of thermal expansion. Adv. Mater. 31, 1900521 (2019).
Ruth, A. et al. Vacancymediated anion photosegregation kinetics in mixed halide hybrid perovskites: coupled kinetic monte carlo and optical measurements. ACS Energy Lett. 3, 2321–2328 (2018).
Suchan, K., Merdasa, A., Rehermann, C., Unger, E. L. & Scheblykin, I. G. Complex evolution of photoluminescence during phase segregation of MAPb(I_{1−x}Br_{x})_{3} mixed halide perovskite. J. Lumin. 221, 117073 (2020).
Babbe, F., Masquelier, E., Zheng, Z. & SutterFella, C. M. Flash formation of IRich Clusters during multistage halide segregation studied in MAPbI_{1.5}Br_{1.5}. J. Phys. Chem. C. 124, 24608–24615 (2020).
Kashchiev, D. Induction time. In Nucleation (eds Kashchiev, D.) Ch. 29 413–427 (ButterworthHeinemann, Oxford, 2000).
Blöchl, P. E. Projector augmentedwave method. Phys. Rev. B 50, 17953–17979 (1994).
Perdew, J. P. et al. Restoring the densitygradient expansion for exchange in solids and surfaces. Phys. Rev. Lett. 100, 1–4 (2008).
Perdew, J. P., Burke, K. & Ernzerhof, M. Generalized gradient approximation made simple. Phys. Rev. Lett. 77, 3865–3868 (1996).
Kresse, G. & Furthmüller, J. Efficient iterative schemes for ab initio totalenergy calculations using a planewave basis set. Phys. Rev. B  Condens. Matter Mater. Phys. 54, 11169–11186 (1996).
Schleife, A. et al. Ab initio description of heterostructural alloys: thermodynamic and structural properties of Mg_{x}Zn_{1−x}O and Cd_{x}Zn_{1−x}O. Phys. Rev. B  Condens. Matter Mater. Phys. 81, 1–15 (2010).
De Carvalho, L. C., Schleife, A., Furthmüller, J. & Bechstedt, F. Distribution of cations in wurtzitic In_{x}Ga_{1−x}N and In_{x}Al_{1−x}N alloys: consequences for energetics and quasiparticle electronic structures. Phys. Rev. B  Condens. Matter Mater. Phys. 85, 1–14 (2012).
Acknowledgements
The authors thank Prof. Dr. René Janssen and MSc Kunal Datta for stimulating discussions about the subject of this work. ZC acknowledges funding from the Eindhoven University of Technology. ST acknowledges funding by the Computational Sciences for Energy Research (CSER) tenure track program of Shell and NWO (Project No. 15CST042) as well as NWO STARTUP from the Netherlands.
Author information
Authors and Affiliations
Contributions
The project was conceived and planned by P.A.B. and S.T. All calculations were done by Z.C. S.T. and G.B. guided the work on the DFT calculations and P.A.B. guided the work on the phase diagrams. The first version of the paper was written by Z.C. under the guidance of P.A.B. All authors contributed to the results of this work and to the final version of the paper.
Corresponding authors
Ethics declarations
Competing interests
The authors declare no competing interests.
Additional information
Peer review information Nature Communications thanks Masaru Kuno and the other, anonymous, reviewer(s) for their contribution to the peer review of this work. Peer reviewer reports are available.
Publisher’s note Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Supplementary information
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Chen, Z., Brocks, G., Tao, S. et al. Unified theory for lightinduced halide segregation in mixed halide perovskites. Nat Commun 12, 2687 (2021). https://doi.org/10.1038/s4146702123008z
Received:
Accepted:
Published:
DOI: https://doi.org/10.1038/s4146702123008z
This article is cited by

Advances and challenges in understanding the microscopic structure–property–performance relationship in perovskite solar cells
Nature Energy (2022)

Allinorganic perovskite quantum dot lightemitting memories
Nature Communications (2021)

Enhancing the stability and crystallinity of CsPbIBr2 through antisolvent engineering
Journal of Materials Science (2021)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.